Lagrangian Time Scale of Passive Rotation for Mesoscale Particles in Turbulence

1. Introduction

Understanding the dynamic response of a particle suspended in turbulent flow is applicable to many small marine organisms. For instance, the rate of prey capture, predator sensitivity, feeding efficiency, and habitat selection of an organism depend on how an organism responds to the varying intensity of turbulence across the ocean (Rothschild and Osborn, 1988; MacKenzie et al., 1994; Gilbert and Buskey, 2005; Reidenbach et al., 2009; Sutherland et al., 2014; Byron, 2015; Michalec et al., 2017). The alignment and rotation of a non-spherical organism may influence its nutrient uptake by influencing the surrounding boundary layer thickness, and hence the biological cycles of the environment at various scales (Pahlow et al., 1997; Nguyen et al., 2011; Byron, 2015). Further, the local distribution of micro-organisms such as phytoplankton relate to their mechanistic response to the turbulence in the ocean (Durham and Stocker, 2012).

Organisms such as phytoplankton are typically smaller than the smallest scale of oceanic turbulence. Orientation and rotation of sub-Kolmogorov particles in turbulence have been widely studied in the past and are relatively well-understood (Jeffery, 1922; Maxey, 1983; Ferrante and Elghobashi, 2003; Lundell and Carlsson, 2010; Pumir and Wilkinson, 2011; Pujara and Variano, 2017). Of particular interest to this research are the mesoscale organisms such as zooplankton; their sizes exceed the Kolmogorov scale but are within the inertial subrange of turbulence. Earlier studies have shown that the orientation of an organism plays a significant role in their gravitaxis, settlement, and directed swimming (Roberts and Deacon, 2002). Besides, the active swimming characteristics of such organisms add further complexity to the problem (Michalec et al., 2017).

The motion, aggregation and fragmentation of microplastics in the ocean are also affected by turbulence. Such mesoscale particles are also often non-spherical. Besides being an obvious threat to the environment, these particles also act as rafting mechanism in long distance transport for various organisms that influences the ecological connectivity of the ocean (Thiel and Gutow, 2005; Wright et al., 2013). However, the kinematics of rotation of mesoscale particles are complex; because they experience non-linear shear along their size, these organisms respond to the ambient distribution of angular velocities in a non-trivial way.

Several fundamental studies in the past few years have been devoted to the passive rotation induced by turbulence of spheres (Zimmermann et al., 2011; Klein et al., 2013; Mathai et al., 2016), of complex particles (Pujara et al., 2018), and axisymmetric anisotropic particles [Voth and Soldati (2017) and reference therein]. Two important goals related to these inquiries are to understand: (A) how the statistics of rotation relates to the particle size, and (B) once set to motion by the ambient turbulence, how long a particle continues to preserve its rotation. Considering the simple cylindrical shape as analogous to the shape of various oceanic organisms, the first piece of this puzzle has been addressed extensively in the past for both non-inertial (tracer) (Parsa et al., 2012; Marchioli and Soldati, 2013; Pujara and Variano, 2017) and inertial particles (Parsa and Voth, 2014; Bordoloi and Variano, 2017; Sabban et al., 2017; Bounoua et al., 2018; Kuperman et al., 2019). Inertia might arise due to the density difference between the fiber and the fluid, and/or because of the fiber dimensions (length and diameter) being larger than the Kolmogorov length η_K. In the latter category, long fibers with negligible diameter (d ≤ η_K) were shown to obey Kolmogorov inertial-range scaling such that the variance of the tumbling rate, $\langle {\dot{p}}_i{\dot{p}}_i\rangle \approx {(L/{\eta }_K)}^{-4/3}{\tau }_K^{-2}$ (Parsa and Voth, 2014). Here, η_K and τ_K are Kolmogorov length and time scales, respectively. For fibers with large diameter (d ≫ η_K) and small aspect ratio (L/d = 1, 4), Bordoloi and Variano (2017) modified this relationship by replacing particle length (L) by the spherical-volume-equivalent diameter $d_{eq}={(L{d}^2)}^{1/3}$. The d_eq-based scaling was also found to be consistent for particles of other complex shapes, such as cubes, cuboids, and cones (Pujara et al., 2018).

In general, the rotation of a rigid fiber can be described by the conservation of angular momentum, written in the frame of the particle as

$\begin{array}{ll}I\stackrel{.}{\Omega }+\Omega \times (I·\Omega )={\Gamma }_f& (1)\end{array}$

Here, Ω is the total rotation (i.e., spinning and tumbling) rate; I is the moment of inertia tensor of the fiber, and Γ_f is the total torque applied on the fiber by the turbulent flow. Considering a viscous torque (linear in velocity profile), Bounoua et al. (2018) model the torque as ${\Gamma }_f~-4\pi \eta \Omega L^3/3+4\pi \eta \int {\text{u}}_f\times \text{s}ds$. The first term corresponds to the viscous dissipation. The second term is the forcing term which is responsible for the transfer of energy from the fluid to the fiber. The Coriolis term Ω × (I·Ω) is generally neglected for long fibers assuming that the spinning rate is smaller than the relaxation rate of tumbling. This disputable assumption is generally justified by the weak alignment of long fibers with coarse grained vorticity (Pujara et al., 2019). The Equation (1) then reduces to a simplified Langevin equation,

$\begin{array}{ll}{\ddot{p}}_i+\frac{1}{{\tau }_r}{\dot{p}}_i=\frac{1}{{\tau }_r}\xi .& (2)\end{array}$

Here, ${\tau }_r=I/4\pi \eta L^3$ is the rotational response time and $\xi ~\int {\text{u}}_f\times \text{s}ds/L^3$ is a colored noise related to the background turbulence. The tumbling rate (ṗ) is then determined by the nature of the forcing ξ and by the ratio of the response time of the particle (τ_r) and the characteristic time of the forcing ${\tau }_L~L/u_L~{ϵ}^{-1/3}{L}^{2/3}$. This ratio defines the tumbling Stokes number $S{t}_{\stackrel{\bullet }{\text{p}}}~{\tau }_r/{\tau }_L$ that scales as:

$\begin{array}{ll}S{t}_{\stackrel{.}{p}}~\frac{1}{48}\frac{\rho }{{\rho }_f}{\left(\frac{d}{{\eta }_K}\right)}^{4/3}{\left(\frac{d}{L}\right)}^{2/3}\left[1+\frac{3}{4}{\left(\frac{d}{L}\right)}^2\right].& (3)\end{array}$

for a cylindrical fiber of length L and diameter d.

In a previous letter (Bounoua et al., 2018), we modeled ξ as a Dirac function peaked at fiber length, L. This provided a theoretical basis to understand the influence of the fiber inertia on the variance of the tumbling rate via:

$\begin{array}{ll}\langle {\dot{p}}_i{\dot{p}}_i\rangle ~\frac{1}{1+S{t}_{\stackrel{.}{p}}^2}{\left(L/{\eta }_K\right)}^{-4/3}{\tau }_K^{-2}.& (4)\end{array}$

The model stated in Equation (4) unified results from Parsa and Voth (2014) and Bordoloi and Variano (2017), and our experimental data over a wide range of aspect ratios. This relation has also been verified recently by Kuperman et al. (2019) for long nylon fibers in air.

While the variance of rotation rate has been investigated in detail, few studies have been devoted to the correlation time of rotation. The main results come from numerical simulation, which are limited to either short (L ≈ 10η_K) (Marchioli and Soldati, 2013) or slender (d < η_K) (Shin and Koch, 2005) fibers. Shin and Koch (2005) showed that in the slender body limit, the correlation time is constant for fiber length smaller than 10η_K and then increases with fiber length. For fibers smaller than Kolmogorov length but heavier than the carrying fluid, Marchioli and Soldati (2013) showed that the correlation time increases with the Stokes number, so with the fiber inertia. Extrapolating our previous model (Bounoua et al., 2018) to inertial fibers longer than the Kolmogorov length, we find that the correlation time of the tumbling rate scales with the forcing time scale, ${\tau }_L~L^{2/3}$ independent of fiber inertia (see section 3). The correlation time is important in understanding the temporal response of an organism to the surrounding turbulence and its rotational diffusivity. For example, a comparison between the response time of a copepod with the frequency of fluctuating nutrient field can help better understand the nutrient uptake event of the organism (Peters and Marrasé, 2000).

Herein, we take an experimental approach to measure the correlation time of rotation for inertial fibers over a wide range of length and diameter. We also take the work of Bounoua et al. (2018) a step further and propose a new model that predicts both variance of tumbling rate and the correlation time scale of tumbling. In section 2, we review the experimental setup and describe our data analysis method. In section 3, we present our results and a theoretical model interpreting the results. Finally, we provide concluding remarks with a discussion about future research directions in section 4.

2. Experimental Setup and Method

The experimental setup consists of a cubic tank (each side = 60 cm) filled with water. We generate homogeneous and isotropic turbulence inside the tank by strategically stirring the water using 8 disks (diameter = 17 cm) with straight blades (height = 5 mm), each mounted on one corner of the tank. Each impeller is set to rotate independently via a 1.5 kW brushless motor at the same frequency but with opposite chirality to its adjacent three nearest neighbors. The turbulence inside the tank, set by the impeller frequency (f = 5, 10, or 15 Hz), is characterized using standard PIV measurements (Xu and Chen, 2013), and is found to be fairly homogeneous and isotropic in the central region (volume ≈ 10 × 10 × 10 cm³). The relevant characteristics of turbulence in the tank are summarized in Table 1. Rigid polystyrene fibers cut to specific length (L = 3.2–40 mm) and diameter (d = 0.5–2.5 mm) are introduced in dilute concentration (<0.01% by volume) into the turbulence tank. We perform experiments on 18 different cases with aspect ratio (Λ = L/d) varying between 1.28 and 80. The details of each experimental case is provided in Table 2. The density of polystyrene (ρ_d = 1.04 g/cm³) makes the fibers near-neutrally buoyant, and the low fiber concentration allows to neglect the interaction between fibers and the retro-action of the fiber on the turbulence.

TABLE 1

Table 1. Characteristics of turbulence in the cube tank facility.

TABLE 2

Table 2. Fiber-dimensions (L, d) normalized by Kolmogorov length scale (η_K), aspect ratio (Λ = L/d), and rotational Stokes number (St_ṗ) of fibers tested under three specific Reynolds number (Re_λ) of the background turbulence.

We image the fibers on two orthogonally arranged 1-MP-high-speed-cameras, all cameras being triggered simultaneously at a frame rate of 0.5–1 kHz. The fibers are backlit onto each camera by an accompanying LED panel with diffuser. Each fiber is reconstructed into the 3D space using a custom MATLAB code. First, the extremities of each fiber are detected in all two images. Then, those extremities are triangulated into the 3D space. Finally, the centroid location (x_{c, i}) and the orientation (p_i) of each fiber are optimized such that the difference between the projection of the fiber onto each camera and the actual image is minimized. The measurement volume is that of a cube of ≈ 13 cm length centered at the center of the tank. N ≥ 5, 000 individual trajectories are stored and used to compute the rotation statistics for each case.

The characteristic time of the dynamics of a random signal is given by the correlation function. The correlation function of ṗ_i(t) is defined as,

$\begin{array}{ll}{C}_{{\dot{p}}_i}(t)=\langle {\dot{p}}_i(t){\dot{p}}_i(t+\tau )\rangle .& (5)\end{array}$

Here there is no summation over i. The angle-bracket 〈.〉 indicates mean over all temporal lags, τ = 0 → ∞. For our calculations, we consider trajectories which are longer than 10 ms. Typically, a fast moving particle remains in the camera frame for a shorter duration compared to a slow moving particle. Hence, the trajectory length is dependent on particle speed. To avoid bias in the mean of C_ṗi due to the correlation between trajectory length and particle speed, we compute the mean weighted on trajectory length, such that

$\begin{array}{ll}{\overline{C}}_{{\dot{p}}_i}(\tau )=\frac{{\displaystyle {\sum }_{k=1}^N{C}_{{\dot{p}}_i}}(\tau )T_k}{{\displaystyle {\sum }_{k=1}^N{T}_k}},& (6)\end{array}$

where T_k is the length of a trajectory and N is the total number of trajectories. The correlation function is normalized by the variance 〈 ṗ_iṗ_i〉, such that ${\bar{C}}_{{\dot{p}}_i}(0)=1$. For our analysis, we use the average of the three components of ${\bar{C}}_{{\dot{p}}_i}$, which were statistically indistinguishable. We denote the average as ${\bar{C}}_{\dot{p}}(\tau )$ and use it to compute two time scales of rotation. The first time scale is based on the zero-crossing time (τ_d1) of the Lagrangian autocorrelation function ${\bar{C}}_{\dot{p}}(\tau )$ as described in Shin and Koch (2005). The second time scale is the integral time scale computed as:

$\begin{array}{ll}{\tau }_{d2}={\displaystyle {\int }_0^{\infty }{\overline{C}}_{\dot{p}}}{\left(\tau \right)}^{2}d\tau \approx {\displaystyle \sum {\overline{C}}_{\dot{p}}}{\left(\tau \right)}^2\Delta \tau & (7)\end{array}$

which is more tractable theoretically as shown later.

Before computing the statistics of rotation, the experimental noise in p_i(t) is removed by filtering it through a series of one-dimensional Gaussian kernels of window-size σ ≤ 20 ms (Mordant et al., 2004; Volk et al., 2007). The tumbling rate (ṗ_i(t)) for each σ is then computed using a symmetric second-order central-difference scheme. Figure 1 demonstrates this method by showing the effect of σ on (a): the mean autocorrelation of tumbling rate ${\bar{C}}_{\dot{p}}(\tau )$, and (b): the integral time-scale of rotational dispersion (τ_d2). Assuming that the experimentally measured ṗ_i(t) contains only uncorrelated noise, we extract the noise-free τ_d2 by fitting a straight line for the linear segment (σ ≥ 10 in this example) of each plot and extrapolating it to σ = 0 (see Figure 1B). We use a critical σ_c to compute the noise-free mean autocorrelation (${\bar{C}}_{\dot{p}}(\tau )$) of rotation and the zero-crossing time (τ_d1). We choose σ_c to be the smallest σ at which the filtered data deviated from the fit by less than 10%. We tested the sensitivity of this criterion by varying it between 5 and 20% and did not find it to affect our results. This is demonstrated in Figure 1B (inset) where we show the evolution of zero-crossing time for the example case.

FIGURE 1

Figure 1. (A) Lagrangian autocorrelation of fiber tumbling rate, (B) the integral time scale of rotation (τ_d2) and in inset: the zero-crossing time (τ_d1) of a representative fiber (L = 3.2η_K, d = 0.64η_K) for different filtering window size. The two dashed lines in the inset of (B) indicate a range of ±10% of τ_d1 obtained from the σ_c shown by the square symbol.

3. Correlation Time Scale of Tumbling Rate

3.1. Experimental Observation

If we neglect inertia and assume that a fiber of size L is rotated only by eddies of size L, the tumbling rate of the fiber should correlate to a timescale ${\tau }_L~L/u_L\approx {(L/{\eta }_K)}^{2/3}{\tau }_K$, where u_L is the typical velocity at scale L. The mean Lagrangian autocorrelation function ${\bar{C}}_{\dot{p}}(\tau )$ of tumbling for various fibers are shown in Figure 2A. This plot includes our measurements and the longest fiber (L = 41.7η_K) simulated by Shin and Koch (2005) at R_λ = 39.9 neglecting fiber inertia (I = 0). With the horizontal-axis normalized by τ_L, the measurements of the autocorrelation function for fibers with St_ṗ < 0.7 are independent of St_ṗ and close to the one obtained by Shin and Koch (2005). In all these cases, the zero-crossing time is τ_d1 = 0.43τ_L with a 95% confidence interval ±0.02. The difference from the slender body approximation appears after the zero-crossing time, such that our measurements decorrelate on a shorter time scale than simulations by Shin and Koch (2005). For fibers with St_ṗ > 0.7, ${\bar{C}}_{\dot{p}}(\tau )$ becomes sensitive to St_ṗ, such that the zero-crossing time increases with St_ṗ.

FIGURE 2

Figure 2. (A) Lagrangian autocorrelation ${\bar{C}}_{\dot{p}}(\tau )$ of tumbling rate, (B) the zero-crossing time τ_d1 and the integral time scale τ_d2 (see inset) for inertial fibers. Numerical result from Shin and Koch (2005) for a slender fiber with L = 41.7η_K, Re_λ = 39.9 is included in (A) and slender fibers at multiple lengths and Re_λ = 16.5 (), 30.7 (), 39.9 (), and 53.3 () are included in (B) for comparison. The dashed lines in (B) represent the linear fit (τ_d/τ_K = 2.66+0.063L/η_K) suggested in Shin and Koch (2005). This fit is multiplied by the mean ratio of the zero crossing time and the integral time from our data in the inset. Data include particles from very little inertia () to those with St_ṗ > 0.7 ( ).

In Figure 2B, we directly show the evolution of zero-crossing time (τ_d1) normalized by the Kolmogorov time scale (τ_K) with respect to normalized fiber length (L/η_K). We also include the zero-crossing time for all slender fibers computed by Shin and Koch (2005). Irrespective of the Reynolds number (Re_λ), a 2/3 power-law scaling qualitatively captures the evolution of τ_d1 for fibers with St_ṗ < 0.7. Also, the zero-crossing times reported in Shin and Koch (2005) approach this power-law scaling as their length enters the inertial range. A similar plot for the integral time (τ_d2) is shown in inset that also demonstrates the 2/3 power-law fit. Shin and Koch (2005) proposed a linear fit for τ_d1 from their simulations with long fibers (25η < L < 60η); the inertial-range scaling was not obvious there because of the limited range of fiber length they simulated.

Our data agree with the scaling law when St_ṗ < 0.7, but not when St_ṗ > 0.7. To investigate this effect, we propose an improved version of the model proposed in Bounoua et al. (2018) which captures both the evolution of the variance and the tumbling rate for inertial fibers (L ≥ 10η_K).

3.2. Theoretical Model

In Bounoua et al. (2018), we modeled the forcing torque ξ as a Dirac function peaked at the fiber length, L. As we saw, this assumption fails to predict the effect of fiber inertia on the correlation time scale (τ_d) measured from our experiments. Here, we assume that the process of filtering due to the integration of the viscous forces along the fiber length is smoother and can be described by a bandpass filter peaked on ${\omega }_L~{ϵ}^{1/3}{L}^{-2/3}$. In that case, the forcing torque ξ in Fourier space can be scaled as,

$\begin{array}{ll}\xi (x)~{\xi }_L\frac{1}{1+ıQ(x-1/x)},& (8)\end{array}$

with x = ω/ω_L and Q is the quality factor of the filter. ξ_L is the amplitude of the turbulent spectrum at scale L, such that $|{\xi }_L{|}^2~{\tau }_K^{-2}{({\eta }_K/L)}^{4/3}$. The quality factor Q determines the width of the band-pass filter as shown on Figure 3. The spectrum reduces to the Dirac function when Q → ∞.

FIGURE 3

Figure 3. The effect of quality factor (Q) on (A) the white noise spectrum, the transfer functions for (B) variance of tumbling rate and (C) correlation time scale. The colormap indicates the value of Q used for this computation.

The solution of Equation (2) leads to:

$\begin{array}{ll}{\dot{p}}_i=\frac{\xi (\omega )}{1+ı\omega {\tau }_r}.& (9)\end{array}$

For a given spectrum of ξ_L, one can determine the variance and the correlation time of tumbling rate from Equation (9). For simplicity, we will assume that ξ_L is a white noise to derive analytical expression for the variance and the tumbling rate. This assumption should hold as long as the quality factor is not too low and that the spectrum is indeed peaked at the frequency ω_L. Further, this assumption will be justified by the agreement between the model and our experimental results (which do not match when the Dirac function selects the amplitude of the spectrum only at the frequency ω_L). Within this framework, the variance of ṗ_i is:

$\begin{array}{ll}\langle {\dot{p}}_i{\dot{p}}_i\rangle ={\xi }_L^2{\displaystyle \int \frac{1}{1+S{t}_{\dot{p}}^2{x}^2}}\frac{x^2}{x^2+Q^2{(x^2-1)}^2}dx.& (10)\end{array}$

In a similar vein, we can derive an analytical expression for the correlation time (τ_d) of the tumbling rate:

$\begin{array}{ll}{\tau }_d={\displaystyle \int C_{\dot{p}}}{\left(t\right)}^{2}dt={\displaystyle \int {\widehat{C}}_{\dot{p}}}(\omega ){\widehat{C}}_{\dot{p}}^{*}(\omega )d\omega ,& (11)\end{array}$

where, Ĉ_ṗ(ω) is the Fourier transform of the autocorrelation of ṗ_i. Contrary to the definition of the zero-crossing time, this expression is suitable analytically. From Equations (8) and (9), the modulus of the correlation function Ĉ can be written:

$\begin{array}{ll}{\left|{\widehat{C}}_{\dot{p}}(x)\right|}^2=\frac{1}{{\langle {\dot{p}}_i{\dot{p}}_i\rangle }^2}\left(\frac{{\xi }_L^4}{1+S{t}^2{x}^2}\frac{x^4}{{(x^2+Q^2{(x^2-1)}^2)}^2}\right).& (12)\end{array}$

Hence, the correlation time τ_d is,

$\begin{array}{ll}{\tau }_d=\frac{{\xi }_L^4}{{\langle {\dot{p}}_i{\dot{p}}_i\rangle }^2}{\displaystyle \int \frac{1}{1+S{t}_{\dot{p}}^2{x}^2}}\frac{x^4}{{(x^2+Q^2{(x^2-1)}^2)}^2}dx.& (13)\end{array}$

The solutions for the two transfer functions: $\langle {\dot{p}}_i{\dot{p}}_i\rangle {\tau }_K^{-2}{(L/{\eta }_K)}^{4/3}$ and ${\tau }_d{(L/{\eta }_K)}^{-2/3}/{\tau }_K$ are shown for multiple Q values in Figures 3B,C, respectively. The rescaled variance $\langle {\dot{p}}_i{\dot{p}}_i\rangle {\tau }_K^2{(L/{\eta }_K)}^{-4/3}$ for all Q values show similar trends with a plateau for low Stokes number, and its value decreasing as $S{t}_{\dot{p}}^{-2}$ for higher Stokes numbers as observed for the Dirac function approximation in Bounoua et al. (2018). Also, the Stokes number where the transition between these two regimes occurs increases with decreasing Q (see Figure 3B). The correlation time for the large values of Q is almost constant irrespective of Stokes number, which is a trend observed for the Dirac function formulation in Bounoua et al. (2018). For smaller values of Q, we observe that the correlation time increases beyond St_ṗ ≈ 1 and eventually reaches a plateau.

We test this model on our experimental measurements of 〈 ṗ_iṗ_i〉 and τ_d1 in Figures 4A,B, respectively. We fit Equations (10) and (13) simultaneously using two least-squares fits with 3 fitting parameters: besides the quality factor Q, we introduce a parameter α to compensate the scaling in tumbling Stokes number St_ṗ (see Equation 4), and a parameter β to compensate the scaling in the amplitude of the spectrum ξ (see Equation 8). This last parameter is fully justified to compare our prediction with the measurement of the zero-crossing time τ_d1 and to compensate the finiteness of the trajectory for the evaluation of the correlation time τ_d2. The best fit for τ_d1 is reached for Q = 0.72, α = 0.41, and β = 3.12. A similar fit to the integral time (τ_d2) has yielded the same Q and α, but a smaller scaling factor (β = 0.64) because of the lower magnitude in τ_d2 seen previously (see Figure 2B). The dashed lines in each plot represent the predictions from Bounoua et al. (2018). Results show that although the previous model is able to predict the variance of tumbling rate, it fails to estimate the evolution of the correlation time. The current model predicts both quantities very well. Our fitted results for Q shows that the inertial effects begin for St_ṗ between 0.1 to 1. This agrees qualitatively with the critical St_ṗ = 0.7 that we chose by eye in Figure 2.

FIGURE 4

Figure 4. Evolution of transfer functions of (A) variance of tumbling rate and (B) correlation time-scale of rotation with respect to rotational Stokes number for fibers of various length and diameter.

4. Summary and Closing Comments

We report experimental measurements of Lagrangian autocorrelation of tumbling rate of inertial fibers in homogeneous isotropic turbulence that is applicable to zooplankton-like organisms in their non-active state. Based on the zero-crossing and the integral of the mean autocorrelation function, we compute two correlation times (τ_d1 and τ_d2) for fibers with a wide range of length and aspect ratio. The inertia of a fiber is quantified using a rotational Stokes number (St_ṗ) that takes into account fiber length, diameter, as well as the relative density. For low St_ṗ, both correlation times from our measurement follow Kolmogorov's inertial range scaling of ${(L/{\eta }_K)}^{2/3}$. This scaling is further supported by the numerically computed zero-crossing times for long slender fibers (L > 10η_K) in Shin and Koch (2005). For fibers with high St_ṗ, the rotation rate escapes this prediction. We find that our previous model (Bounoua et al., 2018) designed for the variance of tumbling rate does not capture the effect of fiber inertia on correlation time. Instead of assuming the spectrum of background excitation to be a simple Dirac function peaked at the fiber length, we model the excitation as a white noise filtered by a bandpass filter (viscous torque). The evolution of the tumbling rate can then be described by a Langevin equation with a response time given by the fiber inertia. We show that this model recovers the evolution of both the variance and the correlation time of tumbling rate for the range of explored Stokes number.

Recent studies on settling of anisotropic particles in turbulent flows (Lopez and Guazzelli, 2017; Gustavsson et al., 2019; Roy et al., 2019) argue that non-linear torque plays an important role on the orientation dynamics. It can be surprising that our model, which only considers viscous torque, is in very good agreement with our measurements. We attribute this contradiction to two main differences between ours and these studies on settling: (a) the settling speed in our case is negligible compared to turbulent fluctuations, and (b) the size of particles considered in the latter case are generally smaller than the Kolmogorov length. A direct estimation of inertial torque requires measurement of fluid velocity around the particle, which is beyond the scope of this work. Future experiments or DNS study will help better understand the importance of inertial torque in the rotational kinematics of fibers.

Oceanic organisms such as zooplankton are capable of active locomotion in turbulence. Results from this investigation will help in addressing the biological aspect of their locomotion by separating the passive rotation from their active swimming.

Finally, to fully characterize the rotation of an anisotropic inertial particle, it is necessary to investigate also its spinning motion, which is currently underway in our laboratory. This quantity has been shown to be larger than the tumbling for fibers smaller than the Kolmogorov length due to a preferential alignment (Parsa et al., 2012). Measuring spinning along with tumbling will also help estimating the total torque and lift experienced by a fiber.

Data Availability Statement

The datasets generated for this study are available on request to the corresponding author.

Author Contributions

GV collected the data. AB and GV analyzed the data. AB, GV, and EV wrote the manuscript. All authors contributed to the article and approved the submitted version.

Funding

This work was carried out in the framework of FlexFiT Project (ANR-17-CE30-0005-01) funded by the French National Research Agency (ANR), the Labex MEC Project (No. ANR-10-LABX-0092) and of the A*MIDEX Project (No. ANR-11-IDEX-0001-02), funded by the Investissements d'Avenir French Government program managed by the French National Research Agency (ANR). In addition to NSF, this work and its open-access publication was supported by the University of California.

Conflict of Interest

The authors declare that the research was conducted in the absence of any commercial or financial relationships that could be construed as a potential conflict of interest.

Acknowledgments

The authors acknowledge the support of S. Bounoua and G. Bouchet in collection of data used in this manuscript.

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