Dynamic curvature regulation accounts for the symmetric and asymmetric beats of Chlamydomonas flagella
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Abstract
Cilia and flagella are model systems for studying how mechanical forces control morphology. The periodic bending motion of cilia and flagella is thought to arise from mechanical feedback: dynein motors generate sliding forces that bend the flagellum, and bending leads to deformations and stresses, which feed back and regulate the motors. Three alternative feedback mechanisms have been proposed: regulation by the sliding forces, regulation by the curvature of the flagellum, and regulation by the normal forces that deform the crosssection of the flagellum. In this work, we combined theoretical and experimental approaches to show that the curvature control mechanism is the one that accords best with the bending waveforms of Chlamydomonas flagella. We make the surprising prediction that the motors respond to the time derivative of curvature, rather than curvature itself, hinting at an adaptation mechanism controlling the flagellar beat.
https://doi.org/10.7554/eLife.13258.001Introduction
Cilia and flagella are long, thin organelles whose oscillatory bending waves propel cells through fluids and drive fluid flows across the surfaces of cells. The internal motile structure, the axoneme, contains nine doublet microtubules, a central pair of single microtubules, motor proteins of the axonemal dynein family and a large number of additional structural and regulatory proteins (Pazour et al., 2005). The axonemal dyneins power the beat by generating sliding forces between adjacent doublets (Summers and Gibbons, 1971; Brokaw, 1989). The sliding is then converted to bending (Satir, 1965) by constraints at the base of the axoneme (e.g. the basal body) and/or along the length of the axoneme (e.g. nexin links) (Brokaw, 2009).
While the mechanism by which the sliding of a doublet is converted to bending is well established, it is not known how the activities of the dyneins are coordinated in space and time to produce the periodic beating pattern of the axoneme. For example, bending the axoneme in one direction requires higher dynein activity on one side of the axoneme than on the other; if the activities are equal then the forces will cancel and there will be no bending. Therefore, to alternatively bend in one direction and then the other requires dynein activity to alternate between the two sides (Satir and Matsuoka, 1989). The switching of dynein activity is rapid, taking place twice per beat cycle and at rates above 100 times per second for Chlamydomonas. The coordination required for such rapidly alternating bending is thought to result from mechanical feedback: the axonemal dyneins generate forces that bend and deform the axoneme; and the deformations, in turn, regulate the dyneins. Because of the geometry of the axoneme, deformation leads to stresses and strains that have components in various directions (e.g. axial and radial). However, which component (or components) regulates the dyneins is not known.
Three different, but not mutually exclusive, molecular mechanisms for dynein coordination have been suggested in the literature (Figure 1D). (i) In the sliding controlmechanism, the dyneins behave as 'slip bonds': they detach when subject to forces acting parallel to the long axis of the microtubule doublets and that oppose sliding (Brokaw, 1975; Jülicher and Prost, 1997; Camalet and Jülicher, 2000; RiedelKruse et al., 2007). The buildup of sliding forces on one side of the axoneme therefore induces detachment of the dyneins on the other side (and vice versa): the two sides are antagonistic. The resolution of this reciprocal inhibition or 'tug of war' is a catastrophic detachment of dyneins on one side of the axoneme, leading to an imbalance of sliding forces and therefore to axonemal bending. (ii) In the curvaturecontrol mechanism, the detachment of dynein is regulated by doublet curvature (Morita and Shingyoji, 2004; Brokaw, 1972; Brokaw, 2009). This leads to a similar reciprocal inhibition because the sign of the curvature is opposite on opposite sides of the axoneme. (iii) In the normalforce control mechanism, also called the geometric clutch, the detachment of dynein is regulated by transverse forces that act to separate adjacent doublets when they are curved (Lindemann, 1994b). Which, if any, of these mechanisms regulates the beating of the axoneme is not known.
In this work, we developed a twodimensional mathematical model of the axoneme that can incorporate any or all of these different feedback mechanisms. The model extends earlier models (Camalet and Jülicher, 2000; RiedelKruse et al., 2007) by including static curvature, which gives rise to asymmetric beats such as those of Chlamydomonas and of ciliated epithelial cells. This model is similar to a recent model (Bayly and Wilson, 2014). We then tested the different feedback mechanisms by comparing the predictions of the associated models with high spatial and temporal resolution measurements of the bending waveforms of isolated, reactivated Chlamydomonas axonemes (Hyams and Borisy, 1975; Bessen et al., 1980). We found that the curvaturecontrol mechanism accorded with experiments using both wild type cells, which have an asymmetric beat, and with experiments using the mbo2 mutant, which has a nearly symmetric beat. By contrast, the sliding mechanism gave poor fits to both the wild type and mbo2 data, and the normalforce mechanism gave unsatisfactory fits to the mbo2 data.
Theoretical model
Twodimensional model of the axoneme
In the two dimensional model, we project the crosssection of the threedimensional axoneme onto a pair of filaments (Figure 1A,B). The projection retains the key idea that motors on opposite sides of the axoneme generate bends in opposite directions (Satir and Matsuoka, 1989). The dyneins that give rise to the principle bend (this corresponds to bends that lie on the outside of the curved path along which an axoneme swims [Gibbons and Gibbons, 1972]; Figure 1A,B green), which in Chlamyodomonas has the same sign as the static curvature, are combined to generate sliding in one direction. The dyneins that give rise to the reverse bend (Figure 1A,B blue), are combined to generate sliding in the opposite direction.
The two filaments have the same polarity (all motors move towards the base) and have combined bending rigidity $\kappa $. They are assumed to be inextensible and held together by elastic elements that maintain the filaments at a constant distance ($a$) from each other. Although there is some evidence that doublet separation is not constant (Lindemann and Mitchell, 2007), our assumption simplifies the theory while still allowing us to calculate the normal force in the elastic elements that keeps the separation constant (Mukundan et al., 2014). In our normalforce mechanism the motors are regulated by the force rather than by the separation of the doublets, as in Lindemann (1994a). However, if the normal force is small, the separation is proportional to the force and the two models are equivalent.
The filaments are immersed in an aqueous fluid and experience drag forces arising from the fluid viscosity. The hydrodynamic forces are proportional to the velocity, with friction coefficients ${\xi}_{\mathrm{n}}$ and ${\xi}_{\mathrm{t}}$ (per unit length) for motion normal to and tangential to the axis of the filament. The values of the mechanical parameters are estimated in Appendix 5.
The position of each point on the filament pair is specified at each time by the vector $\mathbf{\mathbf{r}}(s)$, a function of the arclength $s$, along the centerline between the filaments. Calculating the tangent vector as $\mathbf{t}\left(s\right)=\dot{\mathbf{r}}\left(s\right)$, where dots denote arclength derivatives, allows us to define the tangent angle, $\psi (s)$, with respect to the horizontal axis of the laboratory frame. The tangent angle characterizes the shape of the filament. For a given filament shape, the pair of filaments will have a local sliding displacement, $\mathrm{\Delta}(s)$. We assume that the filaments are incompressible, though they can support tension along their centerline. For incompressible filaments, sliding is linearly related to the tangent angle via
where ${\mathrm{\Delta}}_{\mathrm{b}}=\mathrm{\Delta}(0)$ is the basal sliding (Figure 1C). The sign convention is defined in Figure 10 and Appendix 4.
To compare the observed periodic beats to those predicted by the model, we write the tangent angle as a sum of Fourier modes
where $\omega $ is the angular frequency of the beat ($\omega /2\pi $ is the beat frequency in cycles per second), $t$ is time, i is the imaginary unit, and ${\psi}_{n}$ are the modes (indexed by $n$). The modes are complexvalued functions of arclength that represent the amplitude and phase of the beat waveforms. They satisfy ${\psi}_{n}={\psi}_{n}^{*}$ to keep the angle real (* represents the complex conjugate). For each value of $n>1$, there is an associated equation of motion. We refer to $n=0$ as the static mode, which corresponds to the timeaveraged shape. We refer to $n=1$ as the fundamental mode, which corresponds to the dynamic shape at the beat frequency. The static and fundamental modes are the only ones considered in this work. In this case, we can write $\psi (s,t)={\psi}_{0}(s)+\mid {\psi}_{1}(s)\mid sin[\omega t+\varphi (s)]$ where $\mid {\psi}_{1}(s)\mid $ is the amplitude of the fundamental mode and $\varphi (s)$ is the phase ($arg\psi $). We use the complex formulation because it simplifies the theory, whose goal is to make predictions for $\mid {\psi}_{1}(s)\mid $ and $\varphi (s)$ to compare to the experimental data (e.g. Figure 3ii–iii). The same modal decomposition can be done for all other parameters that depend on time including the sliding displacement, $\mathrm{\Delta}(s)$, the basal sliding, ${\mathrm{\Delta}}_{\mathrm{b}}$, the sliding force between the filaments, $f$, and the tension, $\tau $, in the centerline of the filaments.
Force balance in the axoneme
The shape of the axoneme depends on the balance between the mechanical forces (from the motors and the elastic elements) and the hydrodynamic forces. The mechanical force is the derivative (with respect to the position vector r) of the work functional $U$ (Appendix 1, Equation 11), which depends on the bending rigidity of the doublets, the stiffness of the cross linkers, motor forces and the shape of the filament. This force is balanced by the hydrodynamic force from the fluid, which is proportional to the velocity (${\partial}_{t}\mathbf{\mathbf{r}}$) of the axoneme at each point: $\hat{\mathbf{\Pi}}\cdot {\mathrm{\partial}}_{t}\mathbf{r}=\delta U/\delta \mathbf{r}$, where $\hat{\mathbf{\Pi}}$ is the friction matrix (Lauga and Powers, 2009). For a slender body at low Reynolds number the friction matrix is $\hat{\mathbf{\Pi}}={\xi}_{\mathrm{n}}\mathbf{n}\mathbf{n}+{\xi}_{\mathrm{t}}\mathbf{t}\mathbf{t}$, where $\mathbf{\mathbf{n}}(s)$ a unit vector normal to the tangent vector $\mathbf{\mathbf{t}}(s)$ (Figure 1C). Force balance yields nonlinear equations of motion (Equations 14–16 in Appendix 1, also see Sartori, 2015). We then derive the static solution, corresponding to mode $n=0$, and the periodic solution at the beat frequency, corresponding to mode $n=1$.
Static mode
If the motor forces do not change with time, then the axoneme will not move and the hydrodynamic forces are zero, causing the tension in the axoneme to be zero. The static mode of the filament pair can be calculated from the static forcebalance equation
where ${\dot{\psi}}_{0}\left(s\right)$, the arclength derivative of the tangle angle, is the curvature of the static mode and ${F}_{0}(s)$ is the static mode of the integrated motor force (Appendix 1, Equation 19). The static mode is the timeaveraged shape which, in Chlamydomonas axonemes, has approximately constant curvature all along the length, and as a result $\dot{\psi}}_{0}\left(s\right)\approx {C}_{0$ (Geyer et al., 2016; Eshel and Brokaw, 1987) (see Results). In our theoretical analysis, we therefore ignore deviations from constant curvature. Such deviations are not expected to significantly affect the conclusions of this work because we found that the static curvature had little effect on the dynamics (the wild type and mbo2 axonemes have similar beats, see Results). According to the static forcebalance equation, bending an axoneme into a shape with constant curvature requires the integrated motor force to be independent of arclength, which in turn requires the motor forces be concentrated near the distal end (Mukundan et al., 2014). We therefore approximate the static component of the motor force density by
where $\delta $ is the Dirac delta function, and the minus sign ensures that a positive dynein force produces a negative curvature in accord with our sign convention (Appendix 4).
Dynamic mode
To obtain the equation of motion at the beat frequency (i.e the $n=1$ dynamic mode), we substitute the modal expansions of the tangent angle (Equation 2), the motor force and the tension into the nonlinear dynamic equations and keep only the terms at the fundamental frequency ($n=1$):
(Appendix 1, Equations 14–16, Appendix 2, Equation 21). Associated with these equations are boundary conditions specifying the tangent angle (and its spatial derivatives) and the tension at the basal and distal ends (Appendix 2, Equation 20). The boundary conditions for a freely swimming axoneme correspond to no external forces or torques acting at the ends.
Equation 5 generalizes previous models of symmetrically beating axonemes (Machin, 1958; RiedelKruse et al., 2007; Camalet and Jülicher, 2000, in which the static curvature (${C}_{0}$) and the axial tension (${\tau}_{1}$) are zero. For ${C}_{0}\ne 0$ new terms appear, and the system of equations is of order six rather than four in the symmetric case. The magnitude of the new terms can be estimated by considering the planewave approximation, in which ${\psi}_{1}\left(s\right)=\mathrm{e}\mathrm{x}\mathrm{p}(2\pi is/\lambda )$, with $\lambda \approx L$ the wavelength. The plane wave is sinusoidal, $\psi (s,t)=\mathrm{s}\mathrm{i}\mathrm{n}(\omega t2\pi s/\lambda )$. Though the plane wave is only an approximation to the shape and does not satisfy the boundary conditions (e.g. the curvature at the distal end of an axoneme is always zero), it is nevertheless useful for calculating approximate values of parameters. For example, the fourth term on the right hand side of the upper equation is of order $({\xi}_{\mathrm{n}}/{\xi}_{\mathrm{t}}){C}_{0}^{2}\kappa {(2\pi /\lambda )}^{2}$ and is in phase with the first term, which is of order $\kappa {(2\pi /\lambda )}^{4}$. For Chlamydomonas axonemes $\lambda \sim L$ and ${C}_{0}\sim \pi /L$, and since ${\xi}_{\mathrm{n}}/{\xi}_{\mathrm{t}}\approx 2$ (Appendix 5) the ratio of these terms is $\sim 0.5$. A similar reasoning shows that the third term is in antiphase, and its contribution is of order $\sim 1$. This shows that the new terms, which enter through the asymmetry, can not be neglected a priori. Thus, for the large observed asymmetry of the Chlamydomonas axoneme, we expect that there is coupling between the $n=0$ and $n=1$ modes, significantly modifying the dynamics of the beating axoneme. As we will see, the static curvature ${C}_{0}$ has little effect in the curvaturecontrol model but has a large effect in the normalforce model.
Equation 5 shows how an oscillatory active sliding force, $f(s,t)={f}_{1}(s){e}^{i\omega t}+{f}_{1}^{*}(s){e}^{i\omega t}$, can produce dynamic bending of the axoneme (with appropriate parameter and boundary conditions). To see this, note that the upper equation can be rearranged to provide an expression for ${\tau}_{1}$ in terms of ${\psi}_{1}$ and ${f}_{1}$ (and their derivatives). This expression can then be substituted into the lower equation, to provide a relationship between ${\psi}_{1}$ and ${f}_{1}$, so that if ${f}_{1}$ is known, ${\psi}_{1}$ can be calculated. A trivial example is when ${f}_{1}=0$, in which case the only solutions are ${\psi}_{1}=0$ and ${\tau}_{1}=0$. If ${f}_{1}$ is non zero, the equation may have nontrivial solutions, corresponding to bending oscillations.
Three mechanisms of motor control
We now build the three molecular mechanisms of motor control into the twodimensional model of the axoneme. Equation 5 shows that an oscillating sliding force can produce a dynamic beating pattern. However, we do not expect the motor proteins themselves to be the oscillators, because oscillations have never been observed in singlemolecule recordings (but see Shingyoji et al., 1998). Rather, we expect that the sliding forces generated by the dyneins are regulated directly or indirectly by the shape of the axoneme. Such regulation constitutes mechanical feedback. If we have an expression for how the motor force depends on the tangent angle (and its derivatives), this can be substituted into the equation of motion, which can then be solved (using the boundary conditions) to predict bending waveforms.
The most general linear expression for the dependence of the motor force on sliding, curvature and normal force is
where $n\ge 0$ is the mode index. $\chi (\omega )$, $\beta (\omega )$ and $\gamma (\omega )$ are complex, frequencydependent coefficients describing how the motor force responds to sliding, curvature and normal forces, respectively. The coefficients depend on the molecular properties of the dyneins such as their density along the doublets, their forcevelocity curves, and the sensitivity of their unbinding on load force, on curvature or on normal force; they also depend on the elastic and viscous resistance to sliding between the doublets (Camalet and Jülicher, 2000; RiedelKruse et al., 2007). If the density of motors and the mechanical properties are independent of arclength, then the coefficients will also be independent of the arclength. Though light and electron microscopy studies have shown that there are longitudinal variations in dynein isoforms and dynein density (Yagi et al., 2009; Bui et al., 2012), we ignore these variations in the present work. Such variation could be included in more elaborate models (e.g. RiedelKruse et al., 2007). The coefficients are complex because in general the force could depend on the instantaneous value of the parameter (the real part) and or on the rate of change of the parameter (the imaginary part). To see this, suppose that the force depends on the sliding displacement ($\mathrm{\Delta}$) and the sliding velocity (${\partial}_{t}\mathrm{\Delta}$). Then $f(s,t)=k\mathrm{\Delta}(s,t)+\xi {\partial}_{t}\mathrm{\Delta}(s,t)$, and in the Fourier representation ${f}_{1}(s)=(k+i\omega \xi ){\mathrm{\Delta}}_{1}(s)$, so $\chi =k+i\omega \xi $. Finally, the coefficients will in general depend on frequency through delays caused by the finite detachment times. The response coefficients are the generalization to active motors of the linear response coefficient of a passive system. For example, the basal force of the axoneme, ${F}_{\mathrm{b}}=F(0)$, is described by ${F}_{\mathrm{b}}={k}_{\mathrm{b}}{\mathrm{\Delta}}_{\mathrm{b}}+{\xi}_{\mathrm{b}}{\partial}_{t}{\mathrm{\Delta}}_{\mathrm{b}}$, where k_{b} is the basal stiffness and ξ_{b} is the basal damping coefficient. Thus, the fundamental mode of the basal force is given by ${F}_{\mathrm{b},1}={\chi}_{\mathrm{b}}(\omega ){\mathrm{\Delta}}_{\mathrm{b},1}$ with basal impedance ${\chi}_{\mathrm{b}}(\omega )={k}_{\mathrm{b}}+i\omega {\xi}_{\mathrm{b}}$.
In our model, the response coefficients are small at zero frequency. This is because the observed, nearly constant static curvature implies that the static component of the force (${f}_{0}$) is approximately zero all along the length except near the distal end of the axoneme (see Equation 4).
The motor force equation (Equation 6) together with the equation of motion (Equation 5), define a dynamical system, which can become unstable and produce spontaneous oscillations (Jülicher and Prost, 1997; Camalet et al., 1999). At the critical point, these oscillations are periodic and we only retain the fundamental mode ($n=1$). These criticalpoint oscillations constitute the predicted beat waveforms of our twodimensional model (see last paragraph of Appendix 1).
Normalforce control
We conclude the theory section with a discussion of the normal force. Unlike the sliding control and curvature control mechanisms in which the motor force depends linearly on the tangent angle (and its derivatives), the feedback in the normalforce model is nonlinear. This is because the normal force is the product of the integrated sliding force and the curvature, $f}_{\perp}=F\dot{\psi$ (Appendix 1, Equation 16), both of which depend on arclength. However, under the assumption that the static curvature is constant, $\stackrel{.}{{\psi}_{0}}={C}_{0}$, the normal force can be linearized, simplifying the solution of the dynamical equations. Expanding $F$ and $\dot{\psi}$ into their static and fundamental Fourier modes, and using the static force balance $a{F}_{0}=\kappa {C}_{0}$, we obtain the following expression for the fundamental mode of the normal force:
where ${F}_{1}$ is the fundamental mode of the integrated sliding force (Appendix 1, Equation 19). Thus, the force is linear in the curvature and the integrated motor force. Equation 7 vanishes for symmetric beats in which the static curvature is zero (${C}_{0}=0)$. The important implication is that for symmetric beats, there is no reciprocal inhibition across the axoneme, unlike sliding and curvature control. This is related to the property that static bends produce normal forces that always tends to separate filaments, independent of the sign of the bend (Mukundan et al., 2014). Thus the static curvature, ${C}_{0}\ne 0$, of the Chlamydomonas beat opens a way for regulation by normal forces, something impossible in symmetrically beating cilia, of which sperm is an approximate example (RiedelKruse et al., 2007).
Results
Quantification of the beat of wild type and mbo2 cilia
To test the different mechanisms of beat regulation, we measured the flagellar beating waveforms in wild type and mbo2 axonemes with high temporal and spatial precision (Materials and methods and Figure 2iii). We tracked trajectories of 20 points along the arclength of the axoneme as a function of time over up to 200 beat cycles (Figure 2iii). Copies of the movies and the extracted tangent angles are available (see Sartori et al., 2016). The uncertainty of the position in $\mathbf{\mathbf{x}\mathbf{y}}$ space was ≈5 nm and the uncertainty in the tangent angle was ≈20 mrad (Figure 2ivv). The latter corresponds to a sliding displacement between adjacent doublet microtubules of only 1.3 nm.
Because the beat of Chlamydomonas is periodic in time, it is convenient to decompose the tangent angle $\psi (s,t)$ into Fourier modes $\psi}_{n$ (Equation 2). Before doing so, we note that wild type Chlamydomonas axonemes swim counterclockwise in circles at a slow angular rotation speed $\omega}_{rot}\approx 30\text{}\mathrm{r}\mathrm{a}\mathrm{d}/\mathrm{s$ (Figure 2Ai,iii). While the effect of this rotation is small for a single beat it becomes large for a long time series. Before performing the Fourier decomposition we therefore subtracted ${\omega}_{\mathrm{rot}}t$ from the tangent angle $\psi (s,t)$ (for simplicity we use the same notation for $\psi (s,t)$ and $\psi (s,t){\omega}_{\mathrm{rot}}t$). The power spectrum of the tangent angle (averaged over the flagellar length) shows clear peaks at harmonics of its fundamental frequency (Figure 3Ai). Because the peak at the fundamental frequency $(n=1$) accounts for $90\%$ of the total power, we neglected the higher harmonics (n = 2,3,4, ...) for reconstructing the flagellar shape. We found that using just the $n=0$ and $n=1$ modes gave excellent reconstitutions of both the wild type and mbo2 beats (Figure 3C–D). Thus, the static and fundamental modes provide a good description of the beats.
The amplitude of the static mode ($n=0$) and the amplitude and phase of the fundamental mode ($n=1$) are shown in (Figure 3ii–iv). The main difference between the wild type and mutant axonemes comes from the static mode, ${\psi}_{0}$ (Figure 3ii; Eshel and Brokaw, 1987; Geyer et al., 2016). For wild type axonemes, ${\psi}_{0}$ decreased approximately linearly over arclength. This corresponds to an approximately constant static curvature ≈0.25 rad/μm, and indicates that the timeaveraged shape is close to a semicircular arc of radius ≈4 μm. The static curvature of wild type axonemes leads to the highly asymmetric waveform. In contrast, mbo2 mutant axonemes have a small static mode, with a curvature ≈0.025 rad/μm, corresponding to an approximately symmetric waveform.
In comparison to the large differences in the static mode between wild type and mutant axonemes, the fundamental modes, ${\psi}_{1}$, are similar. The amplitude of ${\psi}_{1}$ is roughly constant and has a characteristic dip in the middle (Figure 3iii). The argument of ${\psi}_{1}$, which determines the phase of the wave, decreases at a roughly constant rate in both cases (Figure 3iv), indicating that the beat is a traveling wave. Because the total phase shift is about $2\pi $, the wavelength of the beat is approximately equal to the length of the axoneme. Thus, both wild type and mutant axonemes have approximately sinusoidal dynamic beats whose amplitudes dip in the middle of the axoneme and whose wavelengths are approximately equal to their lengths.
Motor regulation in the axoneme: experiment versus theory
To gain insight into how molecular motors in the axoneme are controlled, we compared experimental beating patterns to those calculated from theory. In the slidingcontrol model the motor force depends only on sliding through the sliding coefficient $\chi ={\chi}^{\prime}+i{\chi}^{\mathrm{\prime \prime}}$. The single and double primes denote real and imaginary parts. ${\chi}^{\prime}$ and $i{\chi}^{\mathrm{\prime \prime}}$ describe the dependence of force on the sliding displacement and the sliding velocity. They are the elastic and damping components of the sliding response, respectively. Because the response must be active for oscillations to occur, we have ${\chi}^{\prime},{\chi}^{\mathrm{\prime \prime}}\le 0$ (Machin, 1958). In the slidingcontrol model, the motor force is independent of curvature and normal forces so the curvature coefficient ($\beta $) and the normal force coefficient ($\gamma $) were set to zero. In the curvaturecontrol model, the curvature coefficient is nonzero ($\beta \ne 0$). In addition, we allow the possibility that the motors have a passive response to sliding (corresponding to elastic resistance to shear between adjacent doublets at the beat frequency), so that ${\chi}^{\prime}>0$. The motors are not regulated by normal force ($\gamma =0$). In the normalforce model, $\gamma \ne 0$. We again allow for the possibility that the motors have a passive response to sliding (${\chi}^{\prime}>0$). The motors are not regulated by curvature ($\beta =0)$). Note that for backward traveling waves the signs of ${\beta}^{\prime},{\beta}^{\mathrm{\prime \prime}}$ and ${\gamma}^{\prime},{\gamma}^{\mathrm{\prime \prime}}$ change, but those of ${\chi}^{\prime},{\chi}^{\mathrm{\prime \prime}}$ do not.
We tested the three motor models by adjusting the appropriate response coefficients, together with the basal stiffness (${k}_{\mathrm{b}}$) and the basal damping coefficient (${\xi}_{\mathrm{b}}$), to obtain the closest fit of their predictions to the dynamic mode. The fitting procedure is described in Appendix 3 using the mechanical parameters described in Appendix 5. The result of a typical fit for wild type axonemes is shown in Figure 4A. The real and imaginary parts of the fundamental mode ${\psi}_{1}(s)$ – corresponding to the cosine and sine components of the waveforms – agree well with the data in the cases of curvature control and normalforce control, but not for sliding control. In the latter case, the real and imaginary parts of the predicted mode are in antiphase (Figure 4A, left panel), corresponding to a standing wave and contradicting the observed propagating wave. The xy representation of the beating pattern predicted by the curvaturecontrol model agrees well with the experimental beating pattern reconstructed from the static and fundamental modes (Figure 4C). The good agreement reinforces the conclusion from Figure 4A that the curvature control model accords with the experimental data for wild type axonemes. Similar good agreement for wild type axonemes was found with the normalforce model. Table 1 summarizes average parameters resulting from the fits to data from 9 wild type axonemes.
We compared the theory to the dynamic modes measured from the mbo2 mutant, where the static curvature is reduced by at least one order of magnitude compared to wild type beats (Figure 3). The results were similar to those of wild type (Figure 4B): sliding control could not produce bend propagation, while curvature and normal force control were in good agreement with the experimental data. The parameters obtained from the fit of mbo2 beats are given in Table 2. We also fit the model to the wild type waveforms in which the static curvature had been subtracted. A good fit to the curvature control model was obtained, but not to the sliding control model. Thus, the fundamental mode was well fit by the curvature and normalforce models but not sliding control.
Regulation of the beat by sliding
The slidingcontrol model provides a poor fit to the observed beating patterns. This can be understood using three different, but related, arguments. First, in the planewave approximation, ${\psi}_{1}=\mathrm{exp}(2\pi is/\lambda ),$ the wavelength satisfies
Because the equation is unchanged when $\lambda \to \lambda $, there are solutions for propagation from base to tip ($\lambda >0$) and for propagation from tip to base ($\lambda <0$). These two waves superimpose to form a standing wave, inconsistent with the observed traveling wave.
The second argument is that in the limit of very short axonemes ($L\to 0$), sliding control predicts that there will only be standing waves, irrespective of whether the boundary conditions are symmetric or not (Camalet and Jülicher, 2000). Chlamydomonas axonemes are short in the sense that are much shorter than the critical length:
which is $26\mu \mathrm{m}$ using the Chlamydomonas parameters (Appendix 5). Based on this limit we only expect standing waves.
The third argument, is a generalization of the second. Though short, Chlamydomonas axonemes have a nonzero length. We therefore computed the bend propagation speed according to $v={\int}_{0}^{L}{{\psi}_{1}}^{2}{\partial}_{s}\mathrm{arg}{\psi}_{1}\mathrm{d}s$. Using the amplitude and phase of the experimental data for Chlamydomonas, ${\psi}_{1}\sim 0.68$ (Figure 2Aiii and (Geyer et al., 2016) and arg ${\psi}_{1}=2\pi s/L$ (Figure 2Aiv), the bend propagation speed is $\approx $ 3. By contrast, the bend propagation speed predicted by the sliding control model is only 0.005 $\ll $3. Thus, the slidingcontrol model predicts a bend propagation speed much lower than observed.
That the low bend propagation speed is due to the short length of the Chlamydomonas axoneme can be appreciated by plotting the predicted speed (normalized by the measured speed of Chlamydomons) against length $L$ (normalized by the critical length). Figure 5A shows that at short lengths, such as for Chlamydomonas, the wave propagation speed is very slow, whereas for lengths above the critical length, such as for sperm, the propagation speed is high.
Thus, there are several arguments for why sliding control does not work for the short flagella of Chlamydomonas.
Regulation of the beat by normal forces
The normalforce model provides a good fit to the beating patterns of wild type and mbo2 axonemes. However, there are two related arguments against the normalforce model. First, despite the similarities in the dynamics of the beats of wild type and mbo2 axonemes (Figure 3iii–iv), the normal force model requires very different values for the response coefficient, $\gamma $, for wild type and mbo2 axonemes (Tables 1 and 2). Second, the normalforce model applied to mbo2 requires large differences in $\gamma $ from axoneme to axoneme, despite the similarity in the dynamics among the axonemes (Figure 3Biii–iv). To understand why this is the case, we plotted $\gamma $ as a function of the inverse of the curvature. The two are strongly correlated: $\gamma \propto {{C}_{0}}^{1}$(Figure 6A). This correlation follows from Equation 7, which predicts that the dynamic component of the normal force is linearly proportional to the static curvature ${C}_{0}$. In other words, the normalforce model requires there be static curvature; if the static curvature were exactly equal to zero then the model would break down. However, the static curvature in mbo2 axonemes is so small, as few as 3 degrees over the length of the axoneme, that it is likely to be residual and of no significance. It is therefore puzzling why the key control parameter would depend so strongly on a residual property. By contrast, the curvaturecontrol coefficient, $\beta $, is similar for wild type and mbo2 axonemes and is independent of the static curvature (Figure 6B). Thus, we conclude that normal force is not a plausible parameter for controlling the ciliary beat.
Regulation of the beat by curvature
The curvature control model provides a good fit to the experimental data for both wild type and mbo2 axonemes (Figure 4A and B, middle panel). Initially, we fitted the data using nonzero values for both the sliding control parameters (${\chi}^{\prime}$, ${\chi}^{\mathrm{\prime \prime}}$) and for both the curvature control parameters (${\beta}^{\prime}$, ${\beta}^{\mathrm{\prime \prime}}$). We found that the best fit values of ${\chi}^{\mathrm{\prime \prime}}$ and ${\beta}^{\prime}$ were not significantly different from zero. Furthermore, the quality of the fits were as good when we set both to zero. We therefore took ${\chi}^{\mathrm{\prime \prime}}$ = ${\beta}^{\prime}=0$ (Tables 1 and 2). We present an argument in the Discussion for why these two parameters are expected to be zero. Thus, the curvature control model is specified by just two free parameters, the sliding elasticity between doublet microtubules at the beat frequency $({\chi}^{\mathrm{\prime}})$ and the rate of change of axonemal curvature (${\beta}^{\mathrm{\prime \prime}}$) (note that the parameters, ${\chi}_{\mathrm{b}}^{\prime}$ and ${\chi}_{\mathrm{b}}^{\mathrm{\prime \prime}}$, which characterize the stiffness and viscosity at the base respectively, are determined once ${\chi}^{\prime}$ and ${\beta}^{\mathrm{\prime \prime}}$ are specified in order to satisfy the boundary conditions [final paragraph of Appendix 2]).
The average values of ${\chi}^{\prime}$ and ${\beta}^{\mathrm{\prime \prime}}$ varied little between wild type and mbo2 mutant axonemes (compare the third column of Table 1 with that of Table 2, see also Figure 6B). This accords with the observation that there is little difference in the dynamical properties of the beat between wild type and mbo2 axonemes. Furthermore, the standard deviations of ${\chi}^{\prime}$ and ${\beta}^{\mathrm{\prime \prime}}$ are small, indicating that there is little variation from axoneme to axoneme. Thus, the tight distribution of values of the parameters in the model reflects the similarity in the observed shapes in different axonemes. In other words, ${\chi}^{\prime}$ and ${\beta}^{\mathrm{\prime \prime}}$ are well constrained by the experimental data.
To understand what aspects of the experimental data specify these two parameters, we performed a sensitivity analysis on ${\chi}^{\prime}$ and ${\beta}^{\mathrm{\prime \prime}}$. In Figure 7A we show a density map of the mean square distance ${R}^{2}$ between the theoretical waveforms and a reference experimental beating pattern as a function of ${\chi}^{\prime}$ and ${\beta}^{\mathrm{\prime \prime}}$. The red ellipse delimits a region of good fit in which ${R}^{2}>0.90$. This region closely coincides with the region where ${\chi}_{\mathrm{b}}^{\prime}$ and ${\chi}_{\mathrm{b}}^{\mathrm{\prime \prime}}$ are both positive, which is delimited by the central pair of black lines. This is important because negative values of the basal parameters imply an active process at the base, which would result in a whiplike motion of the axoneme, as noted by Machin (Machin, 1958). From the shapes of beating spermatozoa, Machin argued against such an active base.
We systematically varied ${\chi}^{\prime}$ and ${\beta}^{\mathrm{\prime \prime}}$ parallel and perpendicular to the long axis of the ellipse. Moving perpendicular into the region of active base indeed results in whiplike beats, with a larger amplitude at the base (Figure 7B, blue circles). This argues against a basal, whiplike driving of the motion of Chlamydomonas axonemes. Moving parallel affects the amplitude of the beat, with the middledip becoming more or less prominent (Figure 7B, green circles). Thus, the arclength dependence of the amplitude of the fundamental mode constrains the value of the response coefficients and the sign of the basal response.
To better understand the celltocell variability we plotted data from all the axonemes in the $({\chi}^{\prime},{\beta}^{\mathrm{\prime \prime}})$ space (Figure 8A). Points scatter mainly along the long axis of the ellipse, where there is a large region of small shape variation. We consistently saw a shift perpendicular to the long axis between the wild type and mbo2 axonemes. This variation correlates with the difference in normalized lengths between wild type and mutant axonemes (Figure 8B), suggesting a possible dependence of the response coefficients on length and/or frequency.
A striking difference between the wild type and mbo2 axonemes is that the curvefitting indicates that the basal stiffness in the mutant is about 20fold smaller than in the wild type (Table 1 and 2). This softening at the base is associated with a larger basal sliding in the mutant. Whether this difference causes the difference in beat frequency (the mutant beats more slowly) or whether it is a consequence of the shorter lengths of the mutant axonemes (Figure 8C) will require additional study.
Discussion
In this work we imaged isolated axonemes of Chlamydomonas with high spatial and temporal resolution. We decomposed the beating patterns into Fourier modes and compared the fundamental mode, which is the dominant dynamic mode, with theoretical predictions of three motor control mechanisms built into a twodimensional model of the axoneme (Figure 1). The sliding control model provided a poor fit to the experimental data. We argued that the reason for this is that sliding control cannot produce wave propagation for axonemes as short as those of Chlamydomonas (Figure 5). While the normalforce model (also termed the geometric clutch model) provided good fits to the experimental data, it relies on the presence of static curvature (Bayly and Wilson, 2015), which varies greatly between the mbo2 and wild type axonemes. As a result of this large difference in static curvature, the control parameters in this model had to be varied over a wide range to fit the data from the different axonemes (Figure 6). Because the waveforms of mbo2 and wild type axonemes have similar dynamic characteristics, such variation in the control parameter seems implausible and we therefore argue against regulation by normal forces in the twodimensional model. Finally, the curvaturecontrol model provided a good fit to the experimental data with similar parameters for mbo2 and wild type axonemes. Thus, we conclude that only the curvaturecontrol model is fully consistent with our experimental data.
A potential caveat of these conclusions is that the model used here is twodimensional. Importantly, in order to simplify the geometry, the model only contains one pair of filaments. While this captures the essential features of the sliding control and curvature control models, it oversimplifies the normalforce model, because in the threedimensional axoneme there are radial and transverse forces acting on the doublets as the axoneme bends. Yet the twodimensional model does not distinguish between them. To bridge this gap, in other work (Sartori et al., 2015) we developed a full threedimensional model of the axoneme to calculate the radial and transverse stresses. The threedimensional model shows that even when there is a static curvature (without twist), normal (transverse) forces are not antagonistic across the centerline and therefore cannot serve as a control parameter for motors.
Relation with past work
Earlier results showed that sliding control can account for the beating patterns of sperm (Camalet and Jülicher, 2000; RiedelKruse et al., 2007; Brokaw, 1975). This is consistent with the present results because the bull sperm axoneme is approximately five times longer than the Chlamydomonas axoneme and we have shown that sliding control can lead to bend propagation in long axonemes (Figure 5 and see Brokaw, 2005). Thus, it is possible that different control mechanisms operate in different cilia and flagella, with sliding control being used in longer axonemes and curvature control being used in shorter ones. However we do note that curvature control models can account for the bull sperm data (RiedelKruse et al., 2007), as well as data from other sperm (Brokaw, 2002; Brokaw, 1985; Bayly and Wilson, 2015), so there is no strong morphological evidence favoring either sliding or curvature control in sperm. The normalforce model produces beating patterns that resemble those of sperm (Lindemann, 1994b; Bayly and Wilson, 2015; Bayly and Wilson, 2014). However, these models rely on there being an asymmetry which is small and variable in sperm, arguing against normalforce control. Thus, the curvature control model, unlike the other two models, robustly describes symmetric and asymmetric beats in short and long axonemes, and could serve as a 'universal' regulator of flagellar mechanics.
Dynamic curvature control as a mechanism for motor regulation
An unexpected feature of our curvature control model is that the motor force depends only on the time derivative of the curvature. This follows from the fact that the curvature response function $\beta $ has no real part (Table 1 and 2, see Theoretical Model section). Such a model is fundamentally different from the current views of curvature control, in which motors are thought to respond to instantaneous curvature (Brokaw, 1972; Brokaw, 2002; Brokaw, 2009) and not to its time derivative.
While motors can respond to time derivatives of sliding displacement through their forcevelocity relation, it is hard to understand how a similar mechanism could apply to curvature. One possibility is that there is a curvature adaptation system analogous to that of sensory systems, like the signaling pathway of bacterial chemotaxis (Macnab and Koshland, 1972; Yi et al., 2000; Shimizu et al., 2010). In an adaptation mechanism, curvature (or motor activity) would be 'remembered', and the average curvature (or motor activity) over past times would in turn downregulate the activity of the motors on a long timescale. Such regulation could occur, for example, via phosphorylation sites in the dynein regulatory complex or the radial spokes (Witman, 2009; Smith and Yang, 2004; Porter and Sale, 2000). Just as methylation of the chemoreceptors of bacteria modifies their ligand affinity, phosphorylation of regulatory elements within the axoneme could modify the motor sensitivity to curvature over times long compared to the period of the beat.
The molecular mechanisms underlying curvature sensing are unknown. A difficulty with dyneins directly sensing microtubule curvature is that the strain in a curved microtubule (radius of curvature 4 μm) is very small (≈1%), corresponding to a subangstrom strain in a tubulin dimer. Such a small strain would be difficult for an individual dynein microtubulebinding domain to detect, though this difficulty could be circumvented if dynein binding were cooperative, as found for microtubule curvaturesensing by doublecortin (Bechstedt et al., 2014). On the other hand, indirect curvaturesensing mechanisms that rely on the central pair pathway (Witman, 2009) are difficult to reconcile with mutants missing the central pair and radial spokes (Yagi and Kamiya, 2000; Frey et al., 1997). Thus, our findings highlight the question of how curvature might be sensed in the axoneme.
Independence of static and dynamic waveform components
Our dynamic curvature control model adds to the view that dynamic and static components of the beat are regulated independently. The problem with models in which dynein activity is regulated by the instantaneous value of the curvature is that both the static and dynamic components of the beat would contribute to regulation and hence the dynamic component of the waveform would be highly dependent on the static component (Sartori, 2015). Yet the dynamic beats of wild type and mbo2 are similar, as also noted in (Eshel and Brokaw, 1987). Our dynamic curvature control model provides a solution to this problem because static curvature is 'adapted' away. We now bring together several lines of evidence supporting the notion that the static and dynamic modes are separable in their origin and in their affect on the beat.
Dynamic and static components of the beat can exist independently of each other. This is evidenced by the existence of bent, nonmotile cilia at low ATP concentrations on the one hand, as well as symmetrically beating mutants on the other (Geyer et al., 2016).
The waveform of mbo2 has a fundamental dynamic mode similar to that of wild type, Figure 3 Aiii and Biii. However, the static mode is absent in the former, Figure 3 Aii and Bii. The same also holds for the two beating modes of the uniflagellar mutant (Eshel and Brokaw, 1987). Thus, altering the static mode of Chlamydomonas has little effect on the dynamic mode.
The dynamic motor response coefficients are largely independent of the asymmetry, and very similar for mbo2 and wild type axonemes, (Figure 6 A).
If the dynamic and static modes are indeed independently controlled, the dynamic motor response is robust to changes in the asymmetry. This has important biological implications: power generation (the beat) and steering (the asymmetry) can be independently controlled so that the swimming direction can be adjusted without having to alter the motor properties. We note, however, that the molecular origin of asymmetry is not known nor is the mechanism by which the mbo2 mutation leads to symmetric beats (see Geyer et al., 2016 for a discussion of possible mechanisms).
Phase of motor activity during the beat
Our work predicts how the timing of motor activity drives the bending of the axoneme during the beat. The simplest way to understand the spatiotemporal relationship between motor force, $f$, and axoneme curvature, $\dot{\psi}$, is to use the planewave approximation $\psi (s,t)=sin(\omega t2\pi s/\lambda )$, where $\omega $ is the frequency in radians per second and $\lambda $ is the wavelength in microns. Differentiation with respect to time $t$, leads to a phase advance by $\pi /2$ (90 degrees or a quarter of a cycle). This can be appreciated by noting that the cosine function (the derivative of sine) reaches its maximum before the sine function (in the complex representation, $exp[i(\omega t2\pi s/\lambda )]$, differentiation with respect to time leads to multiplication by $i$, which is equivalent to a phase lead of $\pi /2$, since $i=exp(i\pi /2)$). For a traveling wave moving from base to tip (i.e. moving in the direction of increasing arclength, $s$), the wavelength is positive and differentiation with respect to arclength leads to a phase delay by $\pi /2$. This can be appreciated by noting that $cos(s)$, the derivative of $sin(s)$, reaches its maximum after the original function. Thus, time derivatives lead and spatial derivatives lag.
Using these differentiation rules, we can represent the phase relations between the axonemal parameters on a phase plot (Figure 9A). For the reference phase, we use the sliding displacement, $\mathrm{\Delta}$, or the tangent angle $\psi $, which are proportional to each other in the planewave approximation $(\mathrm{\Delta}=a\psi )$: we define them (arbitrarily) to zero degrees (compass bearing east, E). The sliding velocity ${\partial}_{t}\mathrm{\Delta}$ has a phase lead of $\pi /2$ (i.e. compass bearing N on the phase plot). The curvature, the derivative of tangent angle with respect to arclength, ${\partial}_{s}\psi =\dot{\psi}$, has a phase delay of $\pi /2$ (i.e. S on the phase plot). The key parameter is motor force, which, in the curvaturecontrol model, is $f}_{1}={\chi}^{\mathrm{\prime}}{\mathrm{\Delta}}_{1}+i{\beta}^{\mathrm{\prime}\mathrm{\prime}}\text{}{\mathrm{\partial}}_{s$$\psi}_{1}\approx [a{\chi}^{\mathrm{\prime}}+{\beta}^{\mathrm{\prime}\mathrm{\prime}}(2\pi /\lambda )]{\psi}_{1$. Using the parameters for wild type axonemes in Table 1, the sliding stiffness ${\chi}^{\prime}=+20nN/\mu {m}^{2}$ and the dynamic curvature coefficient ${\beta}^{\mathrm{\prime \prime}}=6.5nN$, together with $a=0.066\mu m$ and $\lambda =L=11.7\mu m$, we find that the absolute magnitude of the first term in the square bracket is smaller than the second term, which is negative. Thus, in the planewave approximation, the sign of the force is opposite that of the tangent angle and so the motor force is out of phase with the tangent angle and sliding (compass bearing W).
An exact calculation shows that the phases predicted by the curvature control model are similar to those of the planewave approximation. Thus, the tangent angle (Figure 9A, gray arrow) lags slightly behind the sliding displacement (Figure 9A, black arrow, E) due to the delay associated with the basal compliances. Furthermore, the curvature (Figure 9A, blue arrow) lags the planewave curvature (S) due to the basal compliance and because the wavelength has a small imaginary component. Likewise, the motor force (Figure 9A, red arrow) lags slightly behind the planewave force (W). Thus, the exact theory shows that curvature leads the motor force by approximately one quarter of a cycle and is nearly out of phase with the sliding displacement. The time series for the various parameters are plotted in Figure 9B.
From these phase relations, we can use the curvaturecontrol model to predict the activity of the motors in relation to the curvature of the axoneme. These predictions can then be compared to structural studies, such as cryoelecton microscopy. Because the motor force lags the curvature (Figure 9B), the motor force is in phase with the spatial derivative of the curvature. Thus, the motor force is positive in the region marked green in Figure 9D and negative in the blue region. In other words, the motors whose bases are statically attached to the upper filament are actively interacting with the lower filament with their microtubulebinding domains to drive the bend that will develop at this place as the wave travels towards the distal tip. The motors with opposite polarity (i.e. on the opposite side of the axoneme) will be active proximal to the bend. Such a relative phase of the motor activity with respect to curvature is a consequence of the dynamic curvature mechanism: the force that generates the curvature (Figure 9C, green) is activated by the rate of change in curvature with a sign (${\beta}^{\mathrm{\prime}\mathrm{\prime}}\text{}\text{}0$) consistent with our sign convention. Note that if these predictions are to be compared to experiments, then the static curvature needs to be subtracted.
Efficiency and energetics
Our finding that the motor force is nearly out of phase with the sliding displacement (and tangent angle) shows that the Chlamydomonas flagellum does not operate close to optimal efficiency. The maximally efficient phase was defined as the phase of the motors that maximized the swimming speed while minimizing the elastic and viscous dissipation (i.e. minimizing energy consumption) (Machin, 1958). Machin showed that for a plane wave, the optimum occurs when the phase of the motors is at 225 degrees (compass bearing SW), considerably different from our predicted motor phase, which is <180 degrees. Thus, unlike sperm, which Machin calculated to be close to the optimum, the short cilia of Chlamydomonas deviate considerably from optimum efficiency.
The reason that Chlamydomonas deviates from optimum efficiency is that the elastic dissipation dominates over the viscous dissipation. Elastic dissipation arises from the straightening of the bent axoneme and the loss of the associated bending energy (for an asymmetric beat like that of Chlamydomonas, in which the static and dynamic modes have approximately equal amplitudes, the elastic loss is almost twice as great as that for a symmetric beat). Indeed, in the plane wave approximation, the ratio of the viscous to elastic dissipation is $\left(\pi /2\right){\left(L/\ell \right)}^{4}\ll 1$. This inequality, which was noted recently (Chen et al., 2015), holds for Chlamydomonas because Chlamydomonas axonemes are shorter than the critical length ($\ell$). By contrast, the inequality is $\gg 1$ for the much longer mammalian sperm axonemes (and $\approx 1$ for seaurchin sperm). Note that the dependence of the critical length (Equation 9) on the mechanical parameters  drag coefficient and bending rigidity  is very weak due to the 1/4 power dependence. As a result, even if the bending rigidity were five times smaller than our estimate (Pelle et al., 2009), our argument would still be valid. Thus, the short length of Chlamydomonas axonemes has important implications for the energetics of the flagellar beat.
The reasoning behind the relatively small viscous dissipation also allows us to understand why the curvature mechanism is sensitive to the rate of change of curvature rather than the instantaneous value. Equation 5 for a symmetric plane wave (${C}_{0}=0$) regulated by curvature (using ${f}_{1}=\chi a\psi$$+\beta \dot{\psi}$$=\chi a\psi +i\beta \psi 2\pi /\lambda$) gives
The upper line of Equation 10 shows that ${\beta}^{\prime}$ produces an active motor force to counter the viscous dissipation due to the fluid and the interfilament sliding. If the fluid damping coefficient is small, then we can have solutions with ${\chi}^{\mathrm{\prime \prime}}={\beta}^{\prime}\approx 0$. Furthermore, if the sliding response coefficient is small (${\chi}^{\prime},{\chi}^{\mathrm{\prime \prime}}$ small) then $\mid {\beta}^{\mathrm{\prime}}/{\beta}^{\mathrm{\prime}\mathrm{\prime}}\mid \phantom{\rule{thinmathspace}{0ex}}\approx (\lambda /l{)}^{4}\ll 1$, showing that the dynamic curvature response dominates over the instantaneous response. Thus, the dynamic curvature dependence is a consequence of the viscous forces being small compared to the elastic forces.
Summary and outlook
We finish the discussion by noting that the short length of Chlamydomonas flagella, relative to the critical length $\ell =2\pi (\kappa /{\xi}_{n}\omega {)}^{1/4}$ is key to understanding not just the energetics, but also the mechanism of motor control. Indeed, it was the shortness of the axonemes that implied that the sliding control model only generated a standing wave and so could not recapitulate the observed traveling wave. Furthermore, it was the shortness that gave rise to the imaginary curvature control coefficient, leading to the dynamic curvaturecontrol mechanism. In addition, the shortness implies that the viscous dissipation is small compared to the elastic dissipation. These conclusions are robust because the power of 1/4 in the expression for the critical length makes it quite insensitive to the parameter values. The long length of sperm leads to quantitatively different properties (e.g the viscous and elastic energies are of similar magnitude, leading to efficient motion, as argued by Machin). Whether the long axonemes use the same dynamic curvaturecontrol mechanism as short axonemes will require further study.
Materials and methods
Preparation and reactivation of axonemes
Request a detailed protocolAxonemes from Chlamydomonas reinhardtii wild type cells (CC125 wild type mt+ 137c, R.P. Levine via N.W. Gillham, 1968) and mutant cells that move backwards only (CC2377 mbo2 mt, David Luck, Rockefeller University, May 1989) were purified and reactivated. The procedures described in the following are detailed in Alper et al. (2013).
Chemicals were purchased from Sigma Aldrich, MO if not stated otherwise. In brief, cells were grown in TAP+P medium under conditions of illumination (2x75 W, fluorescent bulb) and air bubbling at 24°C over the course of 2 days, to a final density of 10^{6} cells/ml. Flagella were isolated using dibucaine, then purified on a 25% sucrose cushion and demembranated in HMDEK (30 mM HEPESKOH, 5 mM MgSO${}_{4}$, 1 mM DTT, 1 mM EGTA, 50 mM potassium acetate, pH 7.4) augmented with 1% (v/v) Igpal and 0.2 mM Pefabloc SC. The membranefree axonemes were resuspended in HMDEK plus 1% (w/v) polyethylene glycol (molecular weight 20 kDa), 30% sucrose, 0.2 mM Pefabloc and stored at −80°C. Prior to reactivation, axonemes were thawed at room temperature, then kept on ice. Thawed axonemes were used for up to 2 hr.
Reactivation was performed in flow chambers of depth 100 μm, built from easycleaned glass and doublesided sticky tape. Thawed axonemes were diluted in HMDEKP reactivation buffer containing 1 mM ATP and an ATPregeneration system (5 units/ml creatine kinase, 6 mM creatine phosphate) used to maintain the ATP concentration. The axoneme dilution was infused into a glass chamber, which was blocked using casein solution (from bovine milk, 2 mg/mL) for 10 min and then sealed with vacuum grease. Prior to imaging, the sample was equilibrated on the microscope for 5 min and data was collected for a maximum time of 20 min.
Imaging of axonemes
Request a detailed protocolThe reactivated axonemes were imaged by either phase constrast microscopy (wild type axonemes) or darkfield microscopy (mbo2 axonemes). Phase contrast microscopy was set up on an inverted Zeiss Axiovert S100TV microscope using a Zeiss 63× PlanApochromat NA 1.4 Phase3 oil lens in combination with a 1.6× tube lens and a Zeiss oil condenser (NA 1.4). Data were acquired using a EoSens 3CL CMOS highspeed camera. The effective pixel size was 139 nm/pixel. Darkfield microscopy was set up on an inverted Zeiss Axiovert 200 microscope using a Zeiss 63× Plan achromat NA iris 0.7–1.4 oil lens in combination with an 1.25× tube lens and a Zeiss oil darkfield condenser (NA 1.4). Data were acquired using a pco dmaxS highspeed camera. In both cases, the illumination was performed using a Sola light engine with a 455 LP filter. Movies of up to 3000 frames were recorded at a frame rate of 1000 fps. The sample temperature was kept constant at 24°C using an objective heater (Chromaphor).
High precision tracking of isolated axonemes
Request a detailed protocolTo track the axoneme in each movie frame with nm precision, the Matlabbased software tool FIESTA was used (Ruhnow et al., 2011). Prior to tracking, movies were background subtracted to remove static inhomogeneities arising from uneven illumination and dirt particles. The background image contained the mean intensity in each pixel calculated over the entire movie. This procedure increased the signaltonoise ratio by a factor of 3 (Alper et al., 2013). Phasecontrast images were inverted; darkfield images were tracked directly.
The tracking algorithm FIESTA uses manual thresholding to determine the filament skeleton, which is then divided into square segments. During tracking, the filament position in each segment is determined independently. For tracking, a segment size of 733 nm (approximately 5x5 pixels) was used, corresponding to the following program settings: a full width at half maximum of 750 nm, and a “reduced box size for tracking especially curved filaments” of 30%. Along the arclength of each filament, 20 equally spaced segments were fitted using twodimensional Gaussian functions. Two examples of splinefitted shapes are presented in Figure 2Ai and Bi superimposed on the image. The mean localization uncertainty of the center position of each of these segments was about 5 nm (Figure 2Aiv and Biv). For localization of the ends, the program uses a different fitting function, resulting in an increased uncertainty.
Appendices
1. Nonlinear dynamics of the axoneme
The equations that describe the dynamics of the axoneme are obtained by balancing mechanical and fluid forces. We used a variational approach similar to that in Camalet and Jülicher (2000), RiedelKruse et al. (2007), Sartori (2015). The work done on the filament pair when it is bent and tensed by the motor force $f$ is
where $\kappa $ is the bending rigidity and ${k}_{\mathrm{b}}$ the stiffness of crosslinkers at the base. The normal force ${f}_{\u27c2}$ is a Lagrange multiplier that ensures that the interfilament spacing ${a}^{\prime}$ is a constant. Similarly, $\mathrm{\Lambda}$ is a multiplier that ensures the incompressibility constraint ${\dot{\mathbf{\mathbf{r}}}}^{2}=1$, and is related to the tension in the centerline through $\tau =\mathrm{\Lambda}+\kappa {\dot{\psi}}^{2}aF\dot{\psi}$, where $F$ is the integrated motor force (Equation 3).
The instantaneous mechanical force that the axoneme exerts on the fluid is given by $\delta U/\delta \mathbf{\mathbf{r}}$, and calculating it requires computing $\delta \dot{\psi}$. From the relation $\mathbf{\mathbf{r}}(s)={\mathbf{\mathbf{r}}}_{0}+{\int}_{0}^{s}(\mathrm{cos}(\psi ({s}^{\prime})),\mathrm{sin}(\psi ({s}^{\prime})))\mathrm{d}{s}^{\prime}$, where ${\mathbf{\mathbf{r}}}_{0}$ is the position of the base, it follows that $\dot{\psi}=\mathbf{\mathbf{n}}\cdot \dot{\mathbf{\mathbf{t}}}$ and $\delta \dot{\psi}=\mathbf{\mathbf{n}}\cdot \delta \stackrel{"}{\mathbf{\mathbf{r}}}$. Using this, we arrive at $\delta U/\delta \mathbf{\mathbf{r}}={\partial}_{s}\left[(\kappa \stackrel{"}{\psi}af)\mathbf{\mathbf{n}}\tau \mathbf{\mathbf{t}}\right]$ (Camalet and Jülicher, 2000; Sartori, 2015). The net sliding force exerted at the base is $\delta U/\delta {\mathrm{\Delta}}_{\mathrm{b}}=F(0)+{k}_{\mathrm{b}}{\mathrm{\Delta}}_{\mathrm{b}}$(Mukundan et al., 2014). To obtain the dynamics of the axoneme we balance these mechanical forces by the fluid friction $\widehat{\mathbf{\mathbf{\Pi}}}\cdot {\partial}_{t}\mathbf{\mathbf{r}}$ and the basal friction ${\xi}_{\mathrm{b}}{\partial}_{t}{\mathrm{\Delta}}_{\mathrm{b}}$, which results in
We can calculate a dynamic equation for the tangent angle using that ${\partial}_{t}\dot{\mathbf{\mathbf{r}}}=\mathbf{\mathbf{n}}{\partial}_{t}\psi $, which results in
This equation contains no information about the trajectory of the basal point ${\mathbf{\mathbf{r}}}_{0}(t)$, which can be determined from the condition that the total force on the cilium vanishes (Friedrich et al., 2010; Sartori, 2015; Johnson and Brokaw, 1979).
The tension $\tau $ and normal force ${f}_{\u27c2}$ are obtained by imposing the corresponding constraints. For the case of the tension we take the time derivative of ${\dot{\mathbf{\mathbf{r}}}}^{2}=1$. This gives $\mathbf{\mathbf{t}}\cdot {\partial}_{t}\dot{\mathbf{\mathbf{r}}}=0$, where we can replace the dynamic equation for $\mathbf{\mathbf{r}}$. For the normal force ${f}_{\u27c2}$ we use the force balance $\delta G/\delta a=0$ (Camalet and Jülicher, 2000; Mukundan et al., 2014). The resulting equations are
Because Equation 16 plays a key role in normalforce control, we expand out the modes:
where the second term corresponds to Equation 7. To solve the dynamic equations we need to use boundary conditions. These represent force and torque balances at the ends of the filament pair. For the case of a freely swimming axoneme (no external forces or torques at either end) we have
where the basal force is ${F}_{\mathrm{b}}={k}_{\mathrm{b}}{\mathrm{\Delta}}_{\mathrm{b}}+{\xi}_{\mathrm{b}}{\partial}_{t}{\mathrm{\Delta}}_{\mathrm{b}}$. Equation 14–16 together with the boundary conditions and the forceresponse equation Equation 6 constitute the full, nonlinear model for the axonemal beat. Rather than solving this nonlinear model, we only considered the first two modes and assumed that the static curvature was constant. This leads to an ordinary differential equation in arclength for the tangent angle, with constant coefficients. A discrete set of solutions can then be obtained by solving the boundary value problem as described in Appendix 2. Each periodic solution corresponds to the critical point of a nonlinear dynamic solution at the point of a Hopf bifurcation, as described in Camalet et al. (1999).
2. Asymmetric equation for the fundamental mode
The periodic dynamics of the tangent angle can be decomposed into Fourier modes as defined in Equation 2. For asymmetric beating patterns in which ${\dot{\psi}}_{0}\ne 0$, the static mode is characterized by the force balance $\kappa {\dot{\psi}}_{0}=a{F}_{0}$, obtained from integrating Equation 12 and using the boundary conditions. The static mode of the tension vanishes (also by Equation 12). The dynamics of a small amplitude oscillation dominated by the fundamental mode can be described by expanding Equation 14 and 15 around the static component and keeping only terms in the n=1 mode. This results in
The equations above have been made dimensionless using the following rescalings: $\xi ={\xi}_{n}/{\xi}_{t}$, $\overline{s}=s/L$, $\overline{\mathrm{\Delta}}=\mathrm{\Delta}/a$, $\overline{\omega}={\xi}_{n}\omega {L}^{4}/\kappa $, $\overline{f}=a{L}^{2}f/\kappa $, $\overline{\tau}={L}^{2}\tau /\kappa $, ${\overline{k}}_{\mathrm{b}}={a}^{2}L{k}_{\mathrm{b}}/\kappa $ and ${\overline{\xi}}_{\mathrm{b}}={a}^{2}L\omega {\xi}_{\mathrm{b}}/\kappa $. This choice results in the additional rescalings ${\overline{f}}_{\u27c2}=a{L}^{2}{f}_{\u27c2}/\kappa $, $\overline{\chi}={a}^{2}{L}^{2}\chi /\kappa $, $\overline{\beta}=aL\beta /\kappa $ and $\overline{\gamma}=\gamma $, since $\gamma $ is already dimensionless. This pair of equations is the generalization of the equations for the symmetric beat (Machin, 1958; Camalet et al., 1999). In them, the fundamental mode is coupled to the static mode. For the particular case in which the static shape has constant curvature ${\dot{\psi}}_{0}={C}_{0}$, Equation 21 reduces to the asymmetric beat equations used in the main text (Equation 5).
Equation 5 together with Equation 6 form a system of ordinary differential equations with constant coefficients. Using the boundary conditions, the discrete spectrum of solutions can be obtained (Cross and Hohenberg, 1993; Camalet and Jülicher, 2000; Sartori, 2015)]. While the system is of sixth order, it contains an integral term in the expression for the normal force, Equation 7. It is thus convenient to convert the system to seventh order by taking the derivative of Equation 7, which eliminates the integral term. Provided values for the response coefficients $\chi $, $\beta $ and $\gamma $ we can then use the ansatz ${\psi}_{1}=A{\mathrm{e}}^{ks}$ to obtain a characteristic polynomial of order seven in $k$. The general solution to the boundary value problem is ${\psi}_{1}={\sum}_{i=1}^{7}{A}_{i}{\mathrm{e}}^{{k}_{i}s}$, where the roots ${k}_{i}(\chi ,\beta ,\gamma )$ of the characteristic polynomial are implicit functions of the motor response coefficients. The amplitudes ${A}_{i}$ are then determined, up to an arbitrary factor, imposing that the boundary conditions be satisfied. Determining the amplitudes will in turn result in a fixed discrete spectrum of solutions for the possible basal compliances. Conversely, if the basal compliance is provided, calculating the amplitudes will return a discrete set of solutions for the real and imaginary parts of one of the response coefficients. These are the critical modes in Camalet and Jülicher (2000), two examples are shown in Figure 5.
3. Fitting procedure
The fitting procedure was done as follows. Given a set of values for the response coefficients $\chi $, $\beta $ and $\gamma $, a theoretical solution ${\psi}_{\mathrm{the}}$ was obtained in the manner described in the previous section, up to an arbitrary complex amplitude. Given this solution, the force balance ${\chi}_{\mathrm{b}}{\mathrm{\Delta}}_{\mathrm{b}}=F(0)$ allows us to determine ${\chi}_{\mathrm{b}}$. If the value for the real or imaginary parts of ${\chi}_{\mathrm{b}}$ were negative, corresponding to an active base, the solution was discarded. If they were positive, then the complex amplitude was chosen as to minimize the mean square displacement ${R}^{2}({\psi}_{\mathrm{the}},{\psi}_{\mathrm{exp}})$ given by
where $N=20$ and the points ${s}_{i}$ were equally spaced along the axonemal length. Finally, a value of ${R}^{2}<1$ was obtained. This quality function, which takes the response coefficients as an input, was maximized with the routine Find Minimum of Mathematica 10 using the Principal Axis method.
4. Sign convention
The signs of the geometric parameters such as sliding displacement, tangent angle and curvature, as well as the forces, are defined in Figure 10. The tangent angle is measured with respect to the horizontal $\mathbf{\mathbf{x}}$ axis and grows counterclockwise (the $\mathbf{\mathbf{x}\mathbf{y}}$ frame has the usual orientation). When a dynein motor is attached to the upper filament and walks towards the base on the lower filament (corresponding to the minus end of the microtubule), the filament pair bends downwards: the tangent angle is therefore negative ($\psi \text{}\text{}0$), as is the curvature ($\dot{\psi}\text{}\text{}0$). The sliding displacement, in which the lower filament extends beyond the upper filament, is therefore also negative ($\mathrm{\Delta}\text{}\text{}0$). The force generated by this motor on the lower filament is defined as positive ($f\text{}\text{}0$) as the lower filament slides with its distal end leading. The integrated force acting at the base, ${F}_{\mathrm{b}}={\int}_{0}^{L}f(s)\mathrm{d}s$ is therefore negative. This is consistent with the static force balance equation, $\kappa \dot{\psi}(0)=a{F}_{\mathrm{b}}$, in which the basal curvature ($\dot{\psi}(0)$) and the basal force have the same sign. The sliding force will tend to make the upper filament extend leftwards beyond the lower one; because the basal force and the basal shear have the same sign, this shear is therefore negative (${\mathrm{\Delta}}_{\mathrm{b}}\text{}\text{}0$).
The signs of the parameters shown in the Figures and defined in the equations are consistent with this convention. For example, because the flagellum swims counterclockwise, the tangent angle slowly grows more positive over time, as shown in Figure 2Aiii. Also, the average angle shown in Figure 3Aii has a negative slope, which corresponds to a negative static curvature ${C}_{0}\text{}\text{}0$.
5. Estimation of mechanical parameters of the axoneme
The only mechanical parameters entering the problem are the bending rigidity $\kappa $, the spacing $a$ of the filaments, and the two friction coefficients ${\xi}_{\mathrm{n}}$ and ${\xi}_{\mathrm{t}}$.
The bending rigidity of a single microtubule is ≈20 $\mathrm{pN}\mu {\mathrm{m}}^{2}$ (Gittes et al., 1993) and see (Schaedel et al., 2015) and the bending rigidity of one doublet is expected to be approximately three times that of a single microtubule (Howard, 2001). Together, the axoneme is comprised of 9 doublet and 2 singlet microtubules which amounts to a bending rigidity of 580 $\mathrm{pN}\mu {\mathrm{m}}^{2}$.
The diameter $D$ of the axoneme, determined from a circle through the centers of the 9 doublets, is $192\pm 4$ nm (SD, n=19), measured from two different axonemes in Figure 1 of Bui et al. (2012) and Nicastro (2006). The spacing between the centers of adjacent doublets, $a$, is given by $a=Dsin(\pi /9)$, which is 66 nm. The hydrodynamic radius $r$ of the axoneme was calculated as $r=(D+25$ nm$)/2$ and was 108 nm.
The tangential and normal friction coefficients per unit length of a slender rod of hydrodynamic radius $r$ near a surface (at height $h$ from surface to rod center) are given by ${\xi}_{\mathrm{t}}\approx 2\pi \eta /ln(2h/r)$, where $\eta $ is the viscosity and ${\xi}_{\mathrm{n}}=2{\xi}_{\mathrm{t}}$ (RiedelKruse et al., 2007). Considering the axoneme being immersed in water at $24}^{\circ}\mathrm{C$ ($\eta ={\mathrm{0.91\hspace{0.17em}10}}^{3}\mathrm{pN}\mathrm{s}\mu {\mathrm{m}}^{2}$), and beating at height $h=0.55\mu $m, from the surface, then ${\xi}_{\mathrm{t}}\approx 0.0025\mathrm{pN}\mathrm{s}\mu {\mathrm{m}}^{2}$ and ${\xi}_{\mathrm{n}}\approx 0.0049\mathrm{pN}\mathrm{s}\mu {\mathrm{m}}^{2}$.
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Decision letter

Raymond E GoldsteinReviewing Editor; University of Cambridge, United Kingdom
In the interests of transparency, eLife includes the editorial decision letter and accompanying author responses. A lightly edited version of the letter sent to the authors after peer review is shown, indicating the most substantive concerns; minor comments are not usually included.
Thank you for submitting your work entitled "Dynamic curvature regulation accounts for the symmetric and asymmetric beats of Chlamydomonas flagella" for consideration by eLife. Your article has been reviewed by two peer reviewers, and the evaluation has been overseen by Raymond E. Goldstein as the Reviewing Editor and Aviv Regev as the Senior Editor. One of the reviewers has agreed to reveal his identity: Michael J. Shelley.
The reviewers have discussed the reviews with one another and the Reviewing Editor has drafted this decision to help you prepare a revised submission.
Summary:
Through a combination of experiment and theory this paper analyzes the beating waveforms of Chlamydomonas flagella as a means of distinguishing between different microscopic models. Using isolated reactivated axonemes of both wildtype and mutant Chlamydomonas the authors find strong evidence that regulation by curvature if favoured over that by sliding or normal forces. In addition, the analysis supports the regulation by the timevarying curvature rather than its static value.
Essential revisions:
1) The reviewers were in agreement that the paper, while important and insightful, is difficult to follow in its present form. For instance, it is not always very well organized, especially since the fully nonlinear model is never fully specified, and one has to bounce around the text to try and piece together what is being done.
2) Accessibility. The mathematics behind the continuum model is not easily accessible to a general biological readership. Although the authors have done some work to make it more easily understandable, we feel that more needs to be done. One of the main things is to extend the level of explicit derivation within the Appendix, and then in the main paper reference to specific equations, rather than generically to "the Appendix". Also, it would be beneficial to expand on points like: i) why does (4) show that an oscillatory f_{1} produces dynamic bending? ii) in the subsection second paragraph of the subsection “Three mechanisms of motor control”, why are sliding and curvature controls "linear" (in what?) and normal force control "nonlinear"? iii) in the subsection “Dynamic curvature control as a mechanism for motor regulation”, why does the dependence on timederivative of the curvature follow from β(ω) having no real part? iv) in the Appendix, make more explicit the interpretation of the boundary conditions.
3) With respect to that model itself, it would be nice to see a better explanation of how two coupled elastica moving under the constraints of equal spacing and (equal and opposite) sliding interactions, must yield the form of centerline dynamics given in (11). Also, has there been any fuller 1st principles modeling, say from microscopics, of the form that sliding interactions must take, especially under active forcing from motorproteins ala Figure 1?
4) Please clarify that the nonlinear simulations were performed using models for sliding regulation – at least by sliding or curvature feedback – using constant coefficient functions? If not, what were they (that is, what were their frequency dependencies). Was there an sdependence in those coefficient functions?
5) Having made the arguments against sliding and normal force mechanisms and for curvature control, what would be the prediction of this model for changes in beat frequency and shape for increases in solvent viscosity? (ala Figure 4 in Fauci's Annual Reviews of Fluid Mechanics article).
6) The wild type timeaveraged shape is claimed to have constant curvature, equivalent to the black curve in Figure 3A(ii) being a line. We are not convinced that this is the case. At the very least there is an initial bend, then again a change in slope at ~5μm. We would like to see a plot of the first and second derivatives of ψ_{0}(s), showing directly the local curvature and the local force component f_{0}(s). Looking at the curve, it seems that there will be components to f_{0}(s) localised around the base and at s~5μm. How would these affect the conclusions on the n=0 behaviour of the motor response coefficients?
7) The authors claim that the force leading to the constant curvature is localised at the tip. However, there are no molecular motors at the flagellar tip. Can the authors comment on this discrepancy?
8) One of the main conclusions of the paper is the suggestion that the static and dynamic components of the curvature are regulated independently. The authors comment on the origin of the dynamic regulation. Could they also comment on the origin of the static curvature? Based on what is known of the mbo2 mutation, is it possible to speculate on how might this affect the static curvature?
9) The authors state that the 2D model oversimplifies the effect of normal force, and have developed a 3D model within a working paper (Sartori et al., 2015) which from its title suggest that normal forces can account for motor regulation. Why, then, was the 2D model used here instead of the 3D one? Wouldn't the conclusions presented here be negated, instead of confirmed, by the full 3D model?
10) In the variational principle outlined in the Appendix the contribution to the energy functional from the work done by the motors is written as fΔ and the variation is done assuming only that f is a function of arclength but not itself functionally dependent on the angle ψ. But later when specific forms of f are considered they do depend on the tangent angle ψ. This appears to be an inconsistency and we request clarification.
https://doi.org/10.7554/eLife.13258.018Author response
Essential revisions:
1) The reviewers were in agreement that the paper, while important and insightful, is difficult to follow in its present form. For instance, it is not always very well organized, especially since the fully nonlinear model is never fully specified, and one has to bounce around the text to try and piece together what is being done.
We apologize that the manuscript was difficult to follow. We have made many revisions in the main text, the Theory and the Appendix and we hope that the overall argument, including the mathematical arguments, are now much clearer. Regarding the nonlinear model, we actually solve a linearized model, and now make that very clear in the revised text.
2) Accessibility. The mathematics behind the continuum model is not easily accessible to a general biological readership. Although the authors have done some work to make it more easily understandable, we feel that more needs to be done. One of the main things is to extend the level of explicit derivation within the Appendix, and then in the main paper reference to specific equations, rather than generically to "the Appendix". Also, it would be beneficial to expand on points like: i) why does (4) show that an oscillatory f_{1} produces dynamic bending? ii) in the subsection second paragraph of the subsection “Three mechanisms of motor control”, why are sliding and curvature controls "linear" (in what?) and normal force control "nonlinear"? iii) in the subsection “Dynamic curvature control as a mechanism for motor regulation”, why does the dependence on timederivative of the curvature follow from β(ω) having no real part? iv) in the Appendix, make more explicit the interpretation of the boundary conditions.
We have put a lot of effort into making the paper accessible for a general biological readership.
A) We have substantially rewritten the Introduction to get across the main ideas of reciprocal inhibition of motors across the section of the axoneme.
B) In the Theory, we have added extra panels in Figure 1 to show how the 2D model is derived from the 3D model and how the dyneins on opposite sides of the axoneme lead to bending in opposite directions.
C) We have also made the predictions of the dynamic curvature model clear in Figure 9, showing precisely where and when the motors are active relative to the curvature of the axoneme. These predictions can then be directly tested by structural studies, such as cryoEM.
D) We have made the mathematical analysis in the Appendix more logical and have referenced the specific equations in the main paper.
E)We have also expanded on the four points mentioned, as well as many others:
i) We explain explicitly how an oscillatory force gives an oscillating waveform;
ii) Why sliding and curvature control are linear and normalforce control not (though it becomes linear in the presence of constant static curvature);
iii) The significance of the imaginary part of the control coefficients;
iv) How the boundary conditions arise (i.e. no external forces or torques).
3) With respect to that model itself, it would be nice to see a better explanation of how two coupled elastica moving under the constraints of equal spacing and (equal and opposite) sliding interactions, must yield the form of centerline dynamics given in (11). Also, has there been any fuller 1st principles modeling, say from microscopics, of the form that sliding interactions must take, especially under active forcing from motorproteins ala Figure 1?
We provide references to earlier papers (Camalet & Jülicher 2000 and Mukundan et al. 2014) for a more detailed treatment of the equal spacing constraint. We reference a paper from the Bayly group at U. Washington that solved a microscopic model; however, we feel that the ODEbased approach here is well suited for fitting to experimental data because there is a clear link between the parameters and the shape.
4) Please clarify that the nonlinear simulations were performed using models for sliding regulation – at least by sliding or curvature feedback – using constant coefficient functions? If not, what were they (that is, what were their frequency dependencies). Was there an sdependence in those coefficient functions?
First, we linearized the models so that they are ODEs with constant coefficients. We solved the associated boundary value problem to identify the critical point solutions. The coefficients are all assumed to be independent of arc length, and we have made this clear. The coefficients depend on frequency, but because we only consider the first mode, the curve fitting yields parameters at that frequency only.
5) Having made the arguments against sliding and normal force mechanisms and for curvature control, what would be the prediction of this model for changes in beat frequency and shape for increases in solvent viscosity? (ala Figure 4 in Fauci's Annual Reviews of Fluid Mechanics article).
This is a very good and important question. This is still work in progress. Note that the effects of viscosity in the sliding control model were computed in Camalet and Jülicher (2000).
6) The wild type timeaveraged shape is claimed to have constant curvature, equivalent to the black curve in Figure 3A(ii) being a line. We are not convinced that this is the case. At the very least there is an initial bend, then again a change in slope at ~5μm. We would like to see a plot of the first and second derivatives of ψ_{0}(s), showing directly the local curvature and the local force component f_{0}(s). Looking at the curve, it seems that there will be components to f_{0}(s) localised around the base and at s~5μm. How would these affect the conclusions on the n=0 behaviour of the motor response coefficients?
This is a reasonable question. Author response image 1 shows the requested plots. The reviewers are correct that the static curvature is not constant. We have qualified our statements in the text to say that the curvature is only approximately constant.
The curvature and the basal and distal ends approaches zero. It is difficult to measure curvature at the ends and we were worried about potential artifacts; we are confident, however that the curvature decreases at both ends. At the distal end it is easy to understand: there are no external torques. See the Mukundan et al. 2014 paper for a possible model. The decrease in the curvature at the basal end is presumably due to the (static) compliance at the base. Importantly, the curvature is fairly constant over the central region of the axoneme: the standard deviation is about 20% of the mean. We therefore model the curvature as being due to sliding motors active near (but not at the distal end). Note that an alternative model in which motors are active all along the length would give a static shape that is a spiral (see Mukundan et al. 2014), which is certainly not the case.
One reason we think that the constant curvature approximation is a good one, is that the waveform data shows that the dynamic beats are similar in the wild type and the mbo2 mutant, so the large static curvature cannot be critical to the beat. Furthermore, in the curvaturecontrol model, the effect of static curvature is small.
7) The authors claim that the force leading to the constant curvature is localised at the tip. However, there are no molecular motors at the flagellar tip. Can the authors comment on this discrepancy?
We have qualified this statement by saying the force is mainly (but not completely) localized near (but not at) the tip.
8) One of the main conclusions of the paper is the suggestion that the static and dynamic components of the curvature are regulated independently. The authors comment on the origin of the dynamic regulation. Could they also comment on the origin of the static curvature? Based on what is known of the mbo2 mutation, is it possible to speculate on how might this affect the static curvature?
It is very difficult to interpret the mbo2 mutant. Part of the problem is that most structural mutants in Chlamydomonas (i.e. mutants that are observed by EM to be missing structural elements such as dyneins and regulatory complexes) are assembly mutants, meaning that they miss proteins required to assemble the structures but do not necessarily encode for the missing proteins.
9) The authors state that the 2D model oversimplifies the effect of normal force, and have developed a 3D model within a working paper (Sartori et al., 2015) which from its title suggest that normal forces can account for motor regulation. Why, then, was the 2D model used here instead of the 3D one? Wouldn't the conclusions presented here be negated, instead of confirmed, by the full 3D model?
We have uploaded the 3D paper to the arXiv so that it is accessible to the reviewers. In this paper, we show that if the doublets twist around the surface of the axoneme, then there is coupling between curvature and transverse force (which in the 2D model becomes a normal force that separates the two filaments). This is of course a hypothesis that would need to be tested. However, in the absence of twist, the transverse force is symmetric as is the normal force in the 2D model (i.e. the transverse force is expansive on both sides of the axoneme and so cannot lead to reciprocal inhibition). In other words, our 2D model captures the behavior of an untwisted 3D axoneme. So the 3D model does support the present conclusions.
10) In the variational principle outlined in the Appendix the contribution to the energy functional from the work done by the motors is written as fΔ and the variation is done assuming only that f is a function of arclength but not itself functionally dependent on the angle ψ. But later when specific forms of f are considered they do depend on the tangent angle ψ. This appears to be an inconsistency and we request clarification.
We have clarified this point in the text.
We need to know the instantaneous external force f_{ext} (that acts on the fluid), given the shape and the internal stresses due to the force f between filaments (generated by the motors). This relation between f_{ext} and f for a given shape corresponds to an instantaneous force balance in the filament.
From this we can then write the dynamic equations by also balancing f_{ext} with viscous forces in the fluid.
To derive the instantaneous force f_{ext}, we define the work dW=f_{ext}dr exerted by the external forces under a small displacement. If we keep f constant during such a displacement (no change in f(s) while the displacement is being changed), then the work dW=dU can be written as a change of a potential, where U is the potential defined in (11) in the appendix. The external force f_{ext}=δU/δr can thus be calculated from (11) by variation using f(s)=const.
If f(s) also varies by δf(s) when the displacement δr occurs, then dW can in general not be written as a change dU of a potential. The force balance condition between f_{ext} and f always remains the same but dW=dU is valid only for constant f. For a dynamic flagellum with time varying motor forces f, the forces f_{ext} are not potential forces because this is a nonequilibrium system. However, f_{ext} still obeys the instantaneous force balance obtained for δf=0 from the potential U.
https://doi.org/10.7554/eLife.13258.019Article and author information
Author details
Funding
Yale University
 Jonathon Howard
MaxPlanckGesellschaft
 Frank Jülicher
The funders had no role in study design, data collection and interpretation, or the decision to submit the work for publication.
Reviewing Editor
 Raymond E Goldstein, University of Cambridge, United Kingdom
Publication history
 Received: November 22, 2015
 Accepted: May 8, 2016
 Accepted Manuscript published: May 11, 2016 (version 1)
 Version of Record published: June 28, 2016 (version 2)
Copyright
© 2016, Sartori et al.
This article is distributed under the terms of the Creative Commons Attribution License, which permits unrestricted use and redistribution provided that the original author and source are credited.
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