Dynamics of swimming bacteria at complex interfaces

Dynamics of swimming bacteria at complex interfaces

Diego Lopez diego.lopez@univ-amu.fr Aix Marseille Université, CNRS, IUSTI UMR 7343, 13013 Marseille, France    Eric Lauga e.lauga@damtp.cam.ac.uk Department of Applied Mathematics and Theoretical Physics, Centre for Mathematical Sciences, Wilberforce Road, Cambridge, CB3 0WA,United Kingdom
July 5, 2019
Abstract

Flagellated bacteria exploiting helical propulsion are known to swim along circular trajectories near surfaces. Fluid dynamics predicts this circular motion to be clockwise (CW) above a rigid surface (when viewed from inside the fluid) and counter-clockwise (CCW) below a free surface. Recent experimental investigations showed that complex physicochemical processes at the nearby surface could lead to a change in the direction of rotation, both at solid surfaces absorbing slip-inducing polymers and interfaces covered with surfactants. Motivated by these results, we use a far-field hydrodynamic model to predict the kinematics of swimming near three types of interfaces: clean fluid-fluid interface, slipping rigid wall, and a fluid interface covered by incompressible surfactants. Representing the helical swimmer by a superposition of hydrodynamic singularities, we first show that in all cases the surfaces reorient the swimmer parallel to the surface and attract it, both of which are a consequence of the Stokes dipole component of the swimmer flow field. We then show that circular motion is induced by a higher-order singularity, namely a rotlet dipole, and that its rotation direction (CW vs. CCW) is strongly affected by the boundary conditions at the interface and the bacteria shape. Our results suggest thus that the hydrodynamics of complex interfaces provide a mechanism to selectively stir bacteria.

I Introduction

Swimming microorganisms are ubiquitous in nature, and have long been known to play important roles in marine life ecosystems, animal reproduction, and infectious diseases. In these processes, cell motility is crucial.Bray (2000) At the small scales relevant to swimming cells, inertial forces are negligible, and locomotion is constrained by Purcell’s “scallop” theorem stating that any body deformation reversible in time yields zero net motion.Purcell (1977) Fluid-based cellular motility relies therefore on non-time reversible deformation, for instance by propagating waves along cilia or flagella.Lauga and Powers (2009)

Among the various types of locomotion seen in nature, one commonly observed for bacteria is that of helical propulsion, where a flagellum (or a bundle of flagella) rotates as a helix, inducing forward propulsion. A typical example of an organism employing helical propulsion is the bacterium Escherichia coli (E. coli).Berg (2004) This bacterium alternates “run” and “tumble” periods: in the former, flagella are synchronized in a coherent bundle and propel the cell forward, whereas in the latter flagella are disorganized, changing the cell orientation and subsequent swimming direction. During run periods, when E. coli cells are isolated in a bulk flow, they swim in straight (noisy) lines.

However, cell locomotion is strongly affected by nearby boundaries. Swimming microorganisms often evolve in confined environments, be it by solid boundaries, free surfaces, or liquid interfaces. In some cases, confinement results from channel boundaries, for example along the mammalian female reproductive tract.Fauci and Dillon (2006) Surfaces can also be a key element in the microorganism function, as in the case of surface associated infection or biofilm formation.Lauga and Powers (2009); Costerton et al. (1995) Since such problems are dominated by viscous dissipation, long-range hydrodynamic interactions have been argued to play important roles, resulting in a significant alteration of the locomotion of microorganisms.Lauga and Powers (2009) Over the past years, intensive theoretical, numerical and experimental work has helped uncover the kinematics and dynamics modifications of swimming properties by boundaries.Fauci and McDonald (1995); Harshey (2003); Drescher et al. (2011); Shum, Gaffney, and Smith (2010); Denissenko et al. (2012)

For bacteria employing helical propulsion (such as E. coli), two different effects induced by boundaries have been discovered and quantified. These organisms swim in the forward direction (cell body forward) and are being propelled from the back. They thus push on the surrounding fluid forward and backward, and such swimmers are referred to as “pushers”. In the presence of a nearby solid wall, E. coli tends to aggregate close to walls.Rothschild (1963) This is in fact observed for any kind of pusher, not necessarily one exploiting helical propulsion.Berke et al. (2008); Smith et al. (2009); Giacché, Ishikawa, and Yamaguchi (2010); Li et al. (2011) A second property, observed solely for helical swimmers, is a circular motion of the cells in a plane parallel to the surface. This was accounted for both experimentally and theoretically in the case of a solid wall Berg and Turner (1990); Lauga et al. (2006) and a free surface.Lemelle et al. (2010); Di Leonardo et al. (2011) Notably, the circular motion occurs in an opposite direction in the presence of a solid wall (clockwise, CW, when viewed from inside the fluid) or a free surface (counterclockwise, CCW, see Fig. 1). This change in rotation direction is qualitatively similar to the drag increase or decrease observed for the motion of a colloidal particle near a rigid wall and a free surface.Kim and Karrila (1991) Indeed, a solid wall and a free surface induce opposite effects, no-slip for a rigid boundary vs. free slip in the case of a free interface.

Figure 1: Experimental evidence of clockwise motion for bacteria near a solid wall (left panel) [reprinted with permission from E. Lauga, W. R. DiLuzio, G. M. Whitesides, and H. A. Stone, Biophys. J. 90, 400-412 (2006). Copyright (2006) by the Biophysical Society], and counter-clockwise motion at a free surface (right panel) [reprinted figure with permission from R. Di Leonardo, D. Dell’Arciprete, L. Angelani, and V. Iebba, Phys. Rev. Lett. 106, 038101 (2011). Copyright (2011) by the American Physical Society].

Past experimental results have been explained theoretically considering Newtonian fluids and perfect interfaces, meaning either a no-slip wall or a shear-free surface. Theoretical models do predict a single circular direction, CW in the presence of a solid wall vs. CCW in the presence of a free surface, and are consistent with the results illustrated in Fig. 1. However, recent experiments on E. coli swimming near glass plates and free surfaces show that the distinction in the direction of the circular motion is not straightforward, and both CW and CCW rotations are observed under seemingly similar experimental conditions.Lemelle et al. (2010, 2013); Morse et al. (2013) In the initial study of Lemelle et al. (2010),Lemelle et al. (2010) only CW motion was observed above a glass plate, but both CW and CCW at a free surface, suggesting that particles and surfactants could alter the free slip boundary condition. This hypothesis was further investigated by changing the concentration of a particular polymer that can aggregate at a free surface.Morse et al. (2013) The authors confirmed this qualitative change of behavior, observing a clear dependence on the polymer concentration of the fraction of cells undergoing CCW motion. A similar change in rotation direction was recently highlighted experimentally at a solid wall, when the solution contains polymers.Lemelle et al. (2013) Using a special surface treatment, the polymer concentration at the solid wall was modified, generating possible slip, and resulting in CCW motion. These recent experiments demonstrate that the presence of polymers or surfactants could have a dramatic effect on motility of nearby cells. In this paper we present a modeling approach to quantify the dynamics of swimming bacteria near complex interfaces.

When polymers are present in the solution, their concentration close to surfaces is reduced due to higher shear and confinement.Barnes (1995); Sochi (2011) This wall depletion results in the formation of a thin fluid layer of lower viscosity at the wall, thereby modifying significantly the no-slip condition. On scales larger than this thin layer, the equivalent behavior at the wall is an apparent partial slip, characterized by its slip length ranging from  nm to 10 m.Barnes (1995); Mhetar and Archer (1998); Servantie and Müller (2008); Lemelle et al. (2013) Similarly, a liquid interface covered with surfactants acts as a thin two-dimensional fluid layer separating the liquid phases. This layer has its own rheological properties, and modifies the stress and velocity jumps between the two fluids.Bos and van Vliet (2001); Fuller (2003); Fuller and Vermant (2012) As a consequence, the presence of surfactants can affect significantly the boundary conditions and resulting flow.Bławzdziewicz, Cristini, and Loewenberg (1999); Wang and Ardekani (2013)

In the present work, we address the role of altered boundary conditions on swimming microorganisms, focusing on interface-induced reorientation, attraction vs. repulsion by the surface, and the impact on circular motion. Using an analytical framework based on multipole expansions for describing the hydrodynamic interactions between a swimming microorganism and an interface, we show how complex interfaces affect hydrodynamic interactions, providing possible explanations to past experimental results. Whereas interface alignment and attraction are seen to be universal properties, the direction of the circular motion turns out to strongly depends on the properties of the fluid, on the bacterium shape and, in some cases, the distance to the interface.

In Sec. II we present the modeling approach used throughout the paper. We first introduce the different interfaces considered, and then our solution method quantifying the leading-order effect of hydrodynamic singularities. In Sec. III we recall some existing results for the flow generated by a point force near boundaries and derive in particular the solution in the case of a surfactant-covered interface. Sec. IV is devoted to the main results of the paper, quantifying the impact of complex boundary conditions on swimming bacteria, first on reorientation and attraction, and then on circular motion. We finally conclude in Sec. V while some of the technical details are given in Appendices A-C.

Ii Modeling

ii.1 Interfaces and boundary conditions

Throughout the paper, we use the word interface to refer to any boundary separating two phases. We denote phase 1 the fluid where the swimming bacterium is located, while the second phase can either be a solid, a liquid, or a gas. The presence of a nearby interface affects bacteria locomotion in different ways depending on its flow boundary conditions. In this work, we consider three types of interfaces, sketched in Fig. 2a: (i) a clean interface, i.e. a fluid-fluid interface with no surfactant, (ii) a flat surface with a partial slip condition as a model for a polymer depletion layer, and (iii) a liquid interface covered with incompressible surfactants. In the case of flow generated by swimming microorganisms, the typical capillary number, scaling the flow-induced stress with surface tension, is very small, typically lower than . As a consequence we will neglect any interfacial deformation induced by the microorganisms, and focus therefore on planar interfaces with normal (Fig. 2a).

Figure 2: Schematic representation of a swimming bacterium close to a liquid interface: (a) three different interfaces considered in this work and sketch for their flow profiles; (b) notations for the calculations in this paper.

ii.1.1 Clean interface

The first type of interface we will consider is a clean interface between two fluids. This problem is characterized by the viscosity ratio between the two fluids,

(1)

where the reference viscosity is the viscosity of the fluid where the bacterium is located. If the viscosity of the second fluid vanishes, , the interface behaves as a free surface, whereas if the second fluid viscosity tends to infinity, we have , and the interface becomes equivalent to a rigid wall. A clean liquid interface imposes impermeability and the continuity of tangential velocities and stresses.Aderogba and Blake (1978) The corresponding boundary conditions written at are

(2)
(3)

where is the symmetric rate of strain tensor, and where we have used the superscript to denote fluid . In the case of a free surface (), these equations reduce to a free slip condition, whereas in the limit of a rigid wall (), the boundary imposes a no-slip condition, .

ii.1.2 Slip surface

The second type of interfaces that we will consider models a rigid wall when the fluid contains polymers, and therefore is subjected to wall depletion. For simplicity, we focus solely on the modification of the boundary conditions and assume no change in the fluid rheology. The model problem will therefore become that of a bacterium swimming in a Newtonian fluid close to a partial-slip boundary, meaning that the wall velocity is proportional to the normal velocity gradient. Defining the slip length, the boundary conditions read

(4)

where is the flow velocity in the plane of the interface.

ii.1.3 Surfactant-covered interface

The last type of interface we are interested in characterizing are those covered with surfactants. This type of interface behaves as an impermeable, bi-dimensional fluid layer separating the two phases, and the bulk stress jump in the absence of surface forces is given by

(5)

where is the surfactant concentration, the surface velocity, the in-plane gradient operator, and (resp. ) the bulk (resp. surface) stress tensor.Fuller (2003) In the present analysis, it is appropriate to focus on the stationary limit on the length scales of swimming bacteria. Additionally, we assume that the concentration of surfactant on the surface is large enough so that the relative change in surface tension is of order 1. In that case, as the capillary number is very small (typically lower than ), the surfactant concentration can be considered to be uniform on the surface.Bławzdziewicz, Cristini, and Loewenberg (1999) Under this assumption, the interface is incompressible, , and the surface stress tensor reads

(6)

where is the surface tension and the in-plane rate of strain tensor.Stone (1990); Bławzdziewicz, Cristini, and Loewenberg (1999) The resulting boundary conditions at state continuity of in-plane velocity, no flow perpendicular to the surface, in-plane incompressibility, and balance between shear stresses from the outside flows, surface viscous stresses and Marangoni stresses

(7)
(8)
(9)
(10)

where is the non-dimensional surface viscosity,

(11)

being a flow length scale, chosen here to be the bacterium distance to the wall.Bławzdziewicz, Cristini, and Loewenberg (1999) The parameter is often referred to as Boussinesq number, comparing surface to bulk stresses Fuller (2003). Note that the condition for incompressibility prevents the limit of a clean interface to be reached by simply applying , and only the case of a no-slip boundary can be recovered in the limit .

ii.2 Impact of interface on swimming dynamics

In order to analyze the effect of an interface on the swimming microorganism, we decompose the flow into two contributions, one being the flow generated by the same organism in the absence of interface, , and a contribution due solely to the interface, , so that . The effect of the interface on the swimming microorganism is then determined using Faxén’s law, modeling the bacterium shape as that of a prolate ellipsoid swimming along an intrinsic direction . Noting the aspect ratio of the entire organism (i.e. cell body and flagellar bundle), the interface-induced velocity, , and rotation rate, , of the microorganism are given by

(12)
(13)

where is the location of the bacterium Kim and Karrila (1991) (Fig. 2b). The fact that the interface effect is evaluated only at the location of the swimmer is a key point here – we do not seek to describe the entire flow field in the presence of the aforementioned interfaces, but only the flow at a specific location.

ii.3 Flow singularities

The Reynolds numbers associated with swimming microorganisms are very small.Purcell (1977); Lauga and Powers (2009) In this limit, the flow generated by a swimming microorganism satisfies the linear Stokes equations,Kim and Karrila (1991) which allow for a multipole expansion of any flow.Chwang and Wu (1975) In the present work, we will represent the flow induced by a swimming microorganism using flow singularities. General flow singularities and notation are presented below while in Sec. IV we will focus on the specific singularity model used for microorganisms using helical propulsion.

Flow singularities are derived from the Green’s function for Stokes flows, , which gives the flow at position generated by a point force located at and oriented along the direction as

(14)

where , and . This solution is called the Stokeslet, and higher-order singularities are then derived from this fundamental singularity.Chwang and Wu (1975) We introduce here the Stokeslet dipole, , and quadrupole, ,

(15)
(16)

and the (potential) source dipole, , and quadrupole, ,

(17)
(18)

where the notation is used to denote a gradient taken with respect to the singularity location, . An useful combination of Stokes dipoles is the rotlet,Chwang and Wu (1975) which is the anti-symmetric part of a Stokeslet dipole, and models the flow generated by a point torque

(19)

where . The symmetric part of a Stokeslet dipole is called a stresslet, . Note that all these singularities are -linear functions of their orientation vectors. A singularity oriented along arbitrary directions can thus be expressed as a combination of similar singularities along the different basis vectors.

ii.4 Solution method

The mathematical method used for solving the problem of a point singularity located close to a boundary with specific conditions is Blake’s method, presented first for the problem of a Stokeslet close to a rigid wall Blake (1971). The effect of the interface is mathematically equivalent to an additional flow generated by a system of hydrodynamic image singularities located on the other side of the interface. For complex boundary conditions, the image system is a spatial distribution of singularities.

The problem can be significantly simplified by guessing part of the image system. Noting the image system, the flow is decomposed as

(20)
(21)

where is the bulk solution due to the singularity itself, is a guess in the image system, and and are the unknowns. For example, in the case of a Stokeslet close to a free surface, a good guess for is a Stokeslet symmetric with respect to the interface, which is enough to enforce both the impermeability condition and that of zero shear stress, resulting in . The major advantage of this decomposition is that the forcing term due to the singularity in the flow equation is solved by the bulk flow term . As a result, and satisfy Stokes equations in the absence of forcing terms

(22)

where is the velocity field and the pressure, being the fluid viscosity. That problem can be more easily solved in Fourier space,Blake (1971); Lauga and Squires (2005) using a two-dimensional (2D) Fourier transform, defined as

(23)

Some useful Fourier transforms are referenced in Appendix A. The solution of Stokes equations in a 2D Fourier space is straightforward, and reads for and

(24)

The unknown coefficients in this solution are determined using the continuity equation

(25)

together with the relevant boundary conditions.

Once the solution is obtained for the Stokeslet, it is then possible to derive the solution for higher-order singularities from the Stokeslet solution. This is achieved by applying the same operator acting on the singularity position, , where is the direction where the derivative is taken. Note that this can be done more easily in Fourier space, as

(26)

However, it is also possible to directly apply Blake’s method to any singularity, which can be more convenient if a good guess of is found.

Iii Stokeslet close to a complex interface

As a singularity is a linear function of its orientation vectors, one only needs to solve the problem for the Stokeslet along the directions parallel and perpendicular to the interface. The flow generated by higher-order singularities can then be derived from these projections. By symmetry reasons, all orientations in the plane parallel to the interface are equivalent, we therefore choose to be the singularity plane. We review below some solutions of the flow generated by parallel and perpendicular Stokeslets close to a fluid boundary, and then use the method described in the previous section for determining the flow in the presence of a surface covered with incompressible surfactant, providing an alternative to the derivation by Bławzdziewicz et al. (1999).Bławzdziewicz, Cristini, and Loewenberg (1999) The solution in the case of slip is given in Lauga and Squires (2005)Lauga and Squires (2005) along the same lines.

iii.1 Stokeslet near a clean fluid-fluid interface

The case of parallel and perpendicular Stokeslets were derived by Blake in the case of a solid wall, a free surface, and a fluid-fluid interface.Blake (1971); Aderogba and Blake (1978) In the presence of a clean fluid-fluid interface, the image system is made of a finite number of point singularities located at the image position in fluid 2 (see notation in Fig. 2b). The image system is composed of a Stokeslet, a Stokes dipole, and a source dipole, whose intensities vary with the viscosity ratio and the distance to the interface. For Stokeslets parallel, , and perpendicular to the surface, , the image system is given by

(27)
(28)

where we use in order to simplify the notations, and where the superscript implies that the singularity is located at the image position, . These singularities give the flow in fluid 1, where the singularity is located. The flow in fluid 2 is given by a second set of singularities, given by

(29)
(30)

This second set of images is located at the singularity position , in fluid 1 (see Fig. 2b). The solutions are therefore obtained fully analytically, and higher-order solutions can be obtained by taking derivatives with respect to the singularity position (). Note that since the image strengths are functions of the singularity distance to the interface , taking derivatives of the image system along generates additional singularities.Spagnolie and Lauga (2012)

In the presence of a solid wall, the second set of images vanishes since there is no flow in the solid region. This was the no-slip solution originally presented by Blake.Blake (1971) As we are interested in this work only on the effect of the interface on the swimming bacterium, we will focus only on the first set of images, Eqs. (27) and (28), giving the flow field in the region where the swimming microorganism is located.

The no-slip and no-shear solutions have been used in the past to explain different swimming behaviors of bacteria observed experimentally, such as wall attraction, alignment, and circular motion.Lauga et al. (2006); Berke et al. (2008); Di Leonardo et al. (2011) The particular case of no-slip boundary () is noteworthy, and will be used in the following as a reference solution

(31)
(32)

In the presence of slip or surfactants, the image system is no longer a set of point singularities. The solution to the problem of a Stokeslet close to a partial slip boundary was addressed by Lauga and Squires,Lauga and Squires (2005) using Blake’s method. The case of a surfactant-covered interface has been addressed by Bławzdziewicz et al.,Bławzdziewicz, Cristini, and Loewenberg (1999) using a Batchelor-type decomposition of the flow. In order to use the same formalism throughout our paper, we derive below the solution of a Stokeslet close to a surface covered with incompressible surfactants using Blake’s method.

iii.2 Stokeslet close to an interface covered with incompressible surfactant

We consider here the case of a Stokeslet perpendicular and parallel to a surfactant-covered interface as defined in Sec. II.1. Without loss of generality, the Stokeslet strength is taken to be 1. For this problem, we take to be the opposite Stokeslet located at the image position . This choice yields at for a perpendicular and parallel Stokeslet respectively

(33)

where . The problem is then solved in Fourier space.

iii.2.1 Solution for a perpendicular Stokeslet

In the case of a perpendicular Stokeslet, the boundary conditions read in Fourier space

(34)
(35)
(36)

for and 2, where index 1 (resp. 2) is associated with the (resp. ) coordinate. This set of equations is satisfied by , which corresponds to a solid wall. We recover therefore a known result: because of surface incompressibility, the flow generated by a Stokeslet perpendicular to an interface covered with incompressible surfactants is identical to that in the presence of a solid wall.Bławzdziewicz, Cristini, and Loewenberg (1999)

iii.2.2 Solution for a parallel Stokeslet

In this case, the boundary conditions are given in Fourier space by

(37)
(38)
(39)

Introducing the coefficients , , and from Sec. II.4, this system can be solved directly, leading to , and

(40)
(41)

It is interesting to note that the coefficients in the no-slip problem read

(42)

Hence, introducing , the flow field can be written as

(43)

where is the known solution of the problem in the presence of a no-slip boundary, . After an inverse Fourier transform of , one can identify two differential equations satisfied by and in real space, which can be written as a single vectorial differential equation on ,

(44)

where is a dipole along of rotlets along , located at . The rotlet dipole involved in this flow corresponds to two vertical counter-rotating point vortices, merging at . Note that this singularity can also be written in a way similar to that of Ref.Bławzdziewicz, Cristini, and Loewenberg (1999) as . The flow in the second fluid satisfies a similar problem,

(45)

with the rotlet dipole being located at . As a result, the total flow generated by a Stokeslet parallel to an interface covered with surfactants can be written as

(46)

where is the flow generated by a Stokeslet along in the presence of a no-slip boundary. We recover therefore the result of Ref.Bławzdziewicz, Cristini, and Loewenberg (1999) where the flow is the sum of the no-slip contribution and a “surface-solenoidal” flow, i.e. a 2D flow decaying in .

In order to obtain the exact expression for the flow at the position of the singularity, one still needs to integrate a third order differential equation, Eq. (44). Since our goal is not to derive the entire flow but only the effect of the boundary on the swimming microorganism, we can simplify in the following way. The singularity is located at and since the differential equations giving the flow are equations in , it is possible to set before integrating. As a result, the additional flow induced on the singularity is given by , where and

(47)

The latter equation yields , which could have been anticipated by symmetry. The former equation can be integrated analytically, as detailed in the next section.

Iv Swimming microorganisms and interfaces

iv.1 Bacteria modeled as point singularities

In this work, we model a swimming bacterium in the far field and thus assume that it is small compared to any flow length scale. In particular, the distance between the cell and the interface, , must remain larger than the bacterium size. This far-field approach allows for a representation of a swimming microorganism as a combination of point singularities, while the organism size and shape play a role only through the aspect ratio involved in Faxén’s law, Eq. (13).

Figure 3: (a) The forces generated by a swimming bacterium such as E. coli include two flow singularities which impact the wall dynamics: (b) a force dipole due to thrust from the flagella and drag on the body and (c) a rotlet dipole arising from the counter-rotation between body and flagella.

We focus here on microorganisms using helical propulsion, like E. coli, as illustrated schematically in Fig. 3a. Such micro-swimmers are force- and torque-free, and can be considered as axisymmetric in average. We choose as a convention that the microorganism swims in the plane, along direction . At leading order (spatial decay ), the far-field flow generated by a swimming bacterium is well captured by an axisymmetric Stokeslet dipole, , as sketched in Fig. 3b.Drescher et al. (2011) This singularity is force- and torque-free, and accounts for the spatial distribution of thrust and drag on a flagellated swimming cell.Lauga and Powers (2009) This representation is commonly used for describing far-field hydrodynamic interactions, both to quantify collective dynamics Aditi Simha and Ramaswamy (2002); Hernandez-Ortiz, Stoltz, and Graham (2005); Saintillan and Shelley (2008); Koch and Subramanian (2011) and wall effects.Berke et al. (2008); Smith et al. (2009); Spagnolie and Lauga (2012)

However, by symmetry, this leading-order singularity cannot be responsible for the observed circular rotation along the normal to the interface since is a symmetry plane of the Stokes dipole. It is thus necessary to add higher-order singularities decaying as to capture circular swimming. Those singularities could be: (i) a Stokes quadrupole, related to the length asymmetry between the flagella and the body, (ii) a potential source dipole accounting for the finite size of the bacterium, and (iii) a rotlet dipole capturing the counter-rotation between the flagella and the body. By symmetry, it is straightforward to see that the only singularity that could potentially lead to nonzero rotation along is the rotlet dipole , illustrated in Fig. 3c.

We are interested in three effects induced by a nearby boundary: (a) reorientation in the swimming plane, given by rotation rate ; (b) attraction or repulsion by the wall, quantified by wall-induced velocity ; and (c) circular motion, measured by the out-of-plane rotation rate . Reorientation and attraction can both be accounted for by the leading-order Stokes dipole, as analyzed in Sec. IV.2. In contrast, the circular swimming which is due to the rotlet dipole is addressed in Sec. IV.3.

iv.2 Leading order: Stokes dipole close to a complex interface

We consider here the leading order singularity representing a swimming microorganism, a Stokes dipole, and focus on two effects. We first address the issue of reorientation in the plane induced by a boundary on a tilted micro-swimmer moving along the direction . With the stable wall-induced orientations derived, , we then address the attractive vs. repulsive nature of the interface.

A Stokes dipole tilted along the angle is a combination of parallel and perpendicular Stokes dipoles as

(48)

The wall-induced rotation rate is dependent on the orientation of the microorganism and the local strain rate, see Eq. (13). In the following, the strength of the Stokes dipole is taken to be 1, modeling a “pusher” swimmer as relevant to any flagellated bacteria moving cell body first (a puller corresponds to a negative strength).

iv.2.1 Clean interface

In the presence of a clean interface, the image system is the set of point singularities listed above, and the problem can be solved analytically, leading to the wall-induced rate

(49)

Notably, the sign of this rotation rate is given by as the term in the bracket is always positive. As a result, the interface will always tend to align the (pusher) Stokes dipole in the direction parallel to the interface. This result was previously shown in the case of a solid wall,Berke et al. (2008) and is thus generalized here to any fluid-fluid interface.

The stable orientation is therefore a microorganism swimming parallel to the interface, . In that case, the induced velocity along the vertical axis reads

(50)

We see thus that a swimming pusher will be attracted by a nearby liquid interface for any value of the viscosity ratio. In the limits of a free surface () and a solid wall (), standard results are recovered.Berke et al. (2008); Spagnolie and Lauga (2012)

iv.2.2 Partial slip boundary

In the presence of a partial slip boundary, the flow due to the boundary is equivalent to that generated by a continuous distribution of singularities along the vertical axis on the other side of the surface.Lauga and Squires (2005) Taking derivatives of higher-order solutions is not straightforward in real space, but is easily carried out in Fourier space. It is interesting to note that is a symmetry plane for the first two singularities of the decomposition shown in Eq. (48), namely and . As a result, these terms do not contribute to any rotation rate through vorticity, only the stresslet does. However, all terms contribute to the total rotation rate, as the swimmer’s orientation breaks the symmetry, acting on the strain contribution to the rotation rate, Eq. (76).

The three singularities necessary for describing a tilted Stokes dipole are derived with a particular choice for the different velocity fields , so that corresponds to the solution in the presence of a free surface. This limit is reached in the partial slip model when tends to infinity. For the stresslet , we choose therefore ; the no-slip solution reads

(51)

Following the procedure outlined above we determine the solution in the presence of a partial slip boundary in Fourier space

(52)

Similarly we have for the parallel Stokes dipole Lauga and Squires (2005)

(53)

with the no-slip solution . For the perpendicular Stokes dipole , we have

(54)
(55)

The rotation rate of the cell along is then computed in Fourier space for the three singularities, and the total rotation rate on a tilted Stokes dipole close to a partial slip boundary finally reads

(56)

evaluated at the singularity position, where index SDX stands for parallel Stokes dipole, SDZ for perpendicular Stokes dipole, and SS for the stresslet contribution. The technical difficulty in this problem is the inverse Fourier transform of the rotation rate and we refer to Appendices B and C for the details related to the inversion problem and solution of the resulting differential equations. The final solution in real space is given analytically by

(57)

where the functions , and derive from the exponential integral function of order , , as

(58)

with

(59)
Figure 4: (a) Interface-induced rotation rate along, , characterizing the alignment of the bacterium with the boundary, as a function of the orientation angle and for different values of the dimensionless slip length (0.1, 1, and 10, thin solid lines). Bold dashed lines correspond to the limits of vanishing slip length (no-slip condition) and infinite slip length (no shear). (b) Qualitative physical picture for interface alignment and attraction; streamlines are thin dashed lines, thin arrows (dark blue online) show local effects while thick arrows (light red online) show global effect on the swimming microorganism.

The dependence of the rotation rate induced by a partial slip boundary on a tilted Stokeslet dipole is shown in Fig. 4a, as a function of the tilt angle , for different values of the slip length. We see that the slip length, similarly to the viscosity ratio in the case of a clean liquid interface, does not modify qualitatively the reorientation dynamics and alignment rate with the boundary and a pusher micro-swimmer will always tend to align parallel to the boundary. The limit of infinite slip length, in Eq. (49), leads naturally to the free surface limit. Furthermore, using the asymptotic properties of the exponential integral functions, we have and when tends to infinity, which can then be used to recover quantitatively the reorientation dynamics in the no-slip limit.

We then compute the velocity induced on a micro-swimmer parallel to the boundary, modeled by a parallel Stokes dipole, Eq. (53). The integration can be done in a similar way as for the rotation rate, and using integration by parts we get a simple expression for the vertical velocity as

(60)

A partial slip boundary will always attract a pusher swimmer for any value of the slip length, generalizing therefore the known results for (no-slip) and (no-shear).

iv.2.3 Surfactant-covered interface

We finally consider the case of a Stokes dipole close to a liquid interface covered with incompressible surfactants. From the Stokeslet solution presented in Sec. III.2, it is possible to derive higher-order solutions. Using Eq. (46), the flow generated by a tilted Stokeslet dipole is therefore given by

(61)

with

(62)

Using the same methodology as that described in the previous section and Appendix B, we get that , where is the solution in the presence of a no-slip boundary, given by Eq. (49) with , and (resp. ) is the contribution from the flow (resp. ). The resulting rotation rate is given by

(63)

where and the functions are defined in Eqs. (58)-(59). For any value of the parameters and orientation angle, the sign of the rotation sign is that of the prefactor . As a result, a surface covered with incompressible surfactants tends to always align a swimming microorganism with the surface, similarly to the no-slip and no-shear cases.

Furthermore, since the additional velocity field does not have a vertical component, we see immediately that the vertical velocity induced by the interface is the same as that in the presence of a no-slip boundary, and again a surface covered with surfactants will attract a pusher toward the interface.

In summary, the leading-order singularity modeling a swimming microorganism allowed us to generalize results known for both a solid wall and a free surface. The interface, be it a clean fluid-fluid interface, a partial slip boundary, or surface covered with surfactants always induces alignment parallel to the nearest surface and attraction toward it. The only common boundary conditions to these three types of interfaces is impermeability, which strongly confines the fluid in the vertical direction. This confinement provides a qualitative argument for explaining alignment and attraction of pushers near any type of boundary, as sketched in Fig. 4b. When tilted, a pusher will experience a higher vertical fluid force on the part of the cell closer to the interface, inducing a reorientation in the parallel direction. When swimming parallel to the interface, fluid is attracted towards the cell on its side, leading to attraction toward the surface. From a mathematical point of view, impermeability on the surface is enforced by a symmetric singularity as an image in the second fluid. At leading order it is therefore as if there were two symmetric micro-swimmers, which tend to align and attract each other when they are pushers.Berke et al. (2008); Lauga and Powers (2009)

iv.3 Circular motion: rotlet dipole close to an interface

We turn now to a higher-order representation of a swimming bacterium in order to account for its circular motion near interfaces. Given the results above concerning the leading-order effect of the interfaces, we will assume that the the microorganism is swimming parallel to it. The micro-swimmer is now modeled by a rotlet dipole along the swimming direction, , which can be written as a combination of Stokes quadrupoles,

(64)

As a result, the flow generated by a rotlet dipole close to a boundary can be obtained from that of the Stokeslet, one only needs to consider the parallel Stokeslet along rather than . In this section, in order to perform dimensional analysis, we write the strength of the rotlet dipole as (units of N.m).

iv.3.1 Clean interface

In the case of a clean fluid-fluid interface, we start by considering the problem using dimensional analysis. In a far-field approach, the bacterium geometry plays a role only through the non-dimensional aspect ratio appearing in Faxén’s law (13). The dimensional quantities involved in the rotation rate are then the rotlet dipole strength , the two viscosities and , and the distance to the interface. A straightforward dimensional analysis then yields a rotation rate normal to the interface given by

(65)

where we recall that . The non-dimensional function needs to be determined analytically, but we can already see from Eq. (65) that the sign of , and thus the direction of rotation of the circular motion, will be determined by a comparison between the viscosity ratio and the swimmer geometry, and will be independent of the distance to the interface . Moreover, within the context of our far-field approach, we observe that this rotation rate decays as . The circular motion is therefore likely to occur very close to the interface.

Starting from the image system of a Stokeslet in the presence of an interface, we derive the image system for a rotlet dipole along , and get