## Introduction

Collective behavior of microorganisms is often achieved by the emission and detection of extracellular signaling molecules which regulates their motility1,2,3. One of the most intensively studied examples of such biochemical communication are amoebae, e.g. Dictyostelium discoideum, which can spontaneously reorganize from a dispersed population into a multicellular macroscopic organism4,5. This transition is triggered by few leader cells periodically emitting symmetric pulses of cyclic adenosine 3′,5′-monophosphate (cAMP), which travel as dissipation-free waves by a self-enhancing cell-to-cell relay over large distances6. When Dictyostelium amoebae are hit by cAMP-waves, they move counter to the wave traveling direction, which eventually leads to the formation of dense aggregates7.

Such behavior is an integral part of their survival strategy in nutrient-deprived environments. Interestingly enough, in static cAMP gradients, Dictyostelium exhibit positive chemotactic behavior, i.e. it moves towards larger chemical concentrations8,9. Therefore, one expects them to follow the concentration maximum which should hinder their aggregation10,11. This seemingly inconsistent behavior, which has been recently also confirmed with motile bacteria12, is usually referred to as chemotactic wave paradox5,13. Only recently, it has been demonstrated that it results from the finite adaptation time of the organisms to variations of the surrounding chemical concentration11,14,15,16. Such time-delayed response to spatio-temporal stimuli leads to a slightly different motional response of amoebae to the front and back of entirely symmetric cAMP waves17. This explains their aggregation into multi-cellular collectives, but also their astonishingly effective migration within complex cellular tissues18 and artificial mazes11,19.

The directed motion induced by spatio-temporal cues would be also attractive for active particles (APs), i.e. the synthetic counterpart of living microorganisms. Such systems hold potential as microrobots to carry and sense, e.g. drugs in complex environments20,21,22,23. Similar to motile cells, APs can harvest energy from their environment and convert it into locomotion23. In addition, they can be spatially directed by chemical24,25,26, optical27,28, flow29,30, or gravitational31,32 fields, and thus resemble basic cellular behavior. Contrary to microorganisms, the simple structure of APs does neither allow for intricate signal processing nor a time-delayed response to external stimuli33. Instead, APs respond strictly local to their environment27. Given these limitations compared to living systems, it is surprising that numerical simulations suggest the principle possibility of AP motion against and along a traveling pulse34,35,36.

Here, we experimentally study the response of phototactic microparticles to slowly traveling optical light pulses, which are created by a scanned elongated focus of a laser beam. By analyzing the particles’ translational and orientational motions, we demonstrate that APs indeed move either along or counter to a propagating optical pulse depending on its velocity and width. In addition to single pulses, we also investigated the particle response to periodic pulse trains. With increasing time interval between consecutive pulses, directional particle motion decreases, which is due to the diffusive decorrelation of particle orientations. Since the orientational decorrelation time strongly depends on the particle size, this effect can be promoted as a sorting mechanism, which allows directing particles of different sizes into opposite directions. Our results are supported by numerical simulations which yield good agreement with the experimental data.

## Results

### Experimental characterization of the aligning torque

APs are fabricated from colloidal spheres with diameter σ = 3.25 μm, which are half-coated by carbon cap with 50 nm thickness. When suspended in a critical mixture of water–2,6-lutidine and homogeneously illuminated with laser light, they begin to self-propel. The magnitude and directionality of the propulsion velocity vp can be controlled by the illuminating laser intensityI (further details are provided in the section “Methods”)37,38. Below and above a threshold intensity Ir particles propel with the carbon cap in the back and the front, respectively. As a result of Brownian rotational motion, the direction of the propulsion fluctuates on a time scale 1/Dr5 s set by the inverse rotational diffusion coefficient Dr. Under homogeneous light illumination, the APs perform an isotropic persistent random walk which is confined to two dimensions due to gravity and hydrodynamic interactions with the walls of the sample cell37,39. In the presence of a light gradient I, however, the APs motion is no longer isotropic but exhibits a pronounced phototactic behavior. Depending on whether the illumination intensity is below or above Ir, APs will propel opposite or along I (“Methods”)27,37.

All measurements presented in the following were carried out for illumination intensities I > Ir, i.e. the particles are propelling with the cap ahead and are aligned towards increasing light intensity (positive phototaxis) (“Methods”). This is demonstrated in Fig.1a, b, where we plotted the trajectory of an AP within a one-dimensional triangular light profile. The intensity pattern is created by a scanned line-shaped laser beam, whose scanning motion is synchronized with an electro-optical modulator, the latter modulating the laser intensity (“Methods”). For I > Ir, the propulsion velocity vp depends almost linearly on I (“Methods”), therefore it increases towards the intensity maximum (see color code of the trajectory). Because the particle reorientation dynamics is not instantaneous but limited by viscous friction, this leads to visible overshoots across the intensity maximum before the AP’s orientation reverses (Fig.1b). As a result, it becomes effectively localized (motility trap) near the intensity maximum where it performs an almost periodic back-and-forth motion (Supplementary Movie 1).

The aligning torque of a positively phototacting AP within a gradient I is given by27,40,41

$${\it{M}} \propto - \nabla I \times {\bf{n}}$$
(1)

The corresponding reorientation dynamics can be expressed by the angular velocity.

$$\dot \phi = \omega _{{\mathrm{max}}}\,{\mathrm{sin}}\,\phi ,$$
(2)

where the amplitude ωmax grows with increasing I but eventually saturates27 (“Methods”). In our experiments, all light gradients were above this saturation threshold, which results in a constant particle reorientation time τ = 3.3 ± 0.75 s being much shorter than 1/Dr (see the section “Methods” for further details).

### Particle response to traveling light pulses

Apart from oscillations around the intensity maximum, no drift motion of APs is observed in a static triangular light profile. When interacting with a traveling light pulse (Fig. 2a), however, they are translated during each encounter with the pulse. Each pulse is characterized by its traveling velocity u, its width w and the light pulse amplitude Imax, the latter being kept constant in all our experiments at Imax = 0.625 μW/μm2. The value of Imax sets the largest particle velocity to$$v_{\mathrm{p}}^{{\mathrm{max}}}$$ = 2 μm/s. Figure 2b–d show experimental snapshots of a dilute suspension of APs prior (top) and after (bottom) interacting with a single light pulse traveling from left to right with different velocities. At low pulse speeds $$u \ll v_{\mathrm{p}}^{{\mathrm{max}}}$$ all APs are displaced to the right, at $$u \approx v_{\mathrm{p}}^{{\mathrm{max}}}$$ APs are transported in both directions (mostly to the left resembling the diffusing wave paradox) and for $$u \gg v_{\mathrm{p}}^{{\mathrm{max}}}$$ no significant changes in the position of the particles are observed. To quantify the APs response to a traveling pulse, we calculated their averaged displacement $$x = \frac{1}{N}\mathop {\sum}\nolimits_{i = 1}^N {x_{\mathrm{{f}}}^i - x_0^i}$$, where $$x_0^i$$ and $$x_{\mathrm{{f}}}^i$$ are the initial and final positions of the ith particle prior and after interaction with the pulse. While at low pulse velocities, the particle displacement is along the pulse traveling direction, a motion counter to the pulse is observed for $$u \approx v_{\mathrm{p}}^{{\mathrm{max}}}$$ (Fig. 2e). As will be shown later below, such behavior is in quantitative agreement with numerical simulations of APs exhibiting positive phototaxis. It should be mentioned that in absence of aligning torques the opposite behavior, i.e. displacement counter (along) the pulse direction at low (high) pulse velocities is observed34,36. The saturation of the displacement at small u in Fig. 2e is due to our finite field of view, which provides an upper bound of Δx = 100 µm. With increasing pulse width, the displacement counter to the pulse motion becomes weaker and eventually vanishes.

To understand the AP motion in more detail, we analyze their time-resolved positional and orientational response to a passing traveling pulse. At small pulse velocities $$u/v_{\mathrm{p}}^{{\mathrm{max}}} \ll 1$$, the situation resembles the static case discussed above because the AP will almost instantaneously align parallel with intensity gradient I of the slowly traveling pulse (Fig. 1). Since the pulse travels to the right, the positively phototactic APs spend more time in the back than in the front of the pulse, which causes an effective AP motion to the right (Fig. 3a). Since APs can easily catch up with the slow pulse, a similar oscillatory trajectory as shown in Fig. 1b with almost periodic particle reorientations is superimposed to the drift motion.

Within increasing pulse velocity particles spend less time within the pulse. For $$u \approx v_{\mathrm{p}}^{{\mathrm{max}}}$$, the residence time tres of APs in the front and back of the pulse (horizontal arrows in Fig. 3b, c) are below 2 s each which is below the particle’s reorientation time τ. Therefore, APs have not enough time to align their orientation parallel to the light gradient of the traveling light pulse. As a consequence, their spatial displacement by a pulse becomes strongly dependent on their initial orientation θ0 (cf. Fig. 2c). Exemplarily, we show trajectories for two initial AP orientations, i.e. θ0 ≈ 0 (Fig. 3b) and θ0 ≈ π (Fig. 3c), which demonstrate particle displacement along and counter to the pulse propagation direction. For a qualitative understanding, we provide a sketch at the bottom of Fig. 3b, c. For θ0 ≈ 0, the particle initially points antiparallel to the gradient I of the pulse front and will start to propel in the direction of pulse propagation. Any deviation from θ0 = 0 (e.g. due to thermal noise) causes a torque acting on the particle (Eq. (1)). Since tres < τ, parallel alignment between n and I is not achieved; instead, particles tumble between θ0 ≈ 0 and π/2. This tumbling motion is at the expense of the translational particle drift which is significantly smaller compared to Fig. 3a. On the opposite, particles having an initial orientation θ0 ≈ π are aligned parallel to I and propel counter to the pulse until reaching the intensity maximum (Fig. 3c). The torque M is stabilizing AP orientations θ0 ≈ π (Eq. (1)), therefore particles maintain their orientation while propelling towards the pulse maximum. Once the AP is in the back of the pulse, n becomes antiparallel to I resulting in particle reorientation. Since tres < τ, however, the particle essentially maintains its original alignment counter to the pulse traveling direction which then leads to the diffusing wave paradox (Supplementary Movie 2). The influence of the initial particle orientation θ0 to their response to a traveling pulse is also seen in Fig. 2f where we have replotted the data of Fig. 2e but now resolved according to θ0.

Finally, when $$u/v_{\mathrm{p}}^{{\mathrm{max}}} > 1$$, the particles’ residence time become further reduced, which leads to a strongly weakened phototactic response and thus to a decreasing displacement an agreement with Fig. 2e.

The observed disappearance of the diffusing wave paradox with increasing pulse width (Fig. 2e) is easily understood by considering that tres increases with w. For larger w particle alignment parallel to I becomes more likely and thus facilitates particle motion along the pulse traveling direction.

As shown in Fig. 3b, c the particle orientation before and after interacting with a light pulse with θ0 ≈ 0 hardly changes (note that considerable reorientations occur when the pulse is running over the particle). Therefore, when subjecting APs to a train of N identical pulses with period T (Fig. 4a), at first glance one expects that the displacement is enhancement by a factor N. Figure 4b shows the averaged particle displacement $${\mathrm{\Delta }}x_{}^{N = 10}$$(N = 10) with $$u/v_{\mathrm{p}}^{{\mathrm{max}}} = 1$$, as a function of T/Dr, i.e. time T in units of the AP’s rotational diffusion time. Again, we have independently analyzed the data for different initial AP orientations (before encountering the first pulse) and exemplarily show the results for θ0 = 0 ± 0.2 andπ ± 0.2. For small T, indeed the displacements are about 10 times larger than for a single pulse (Fig. 2f and Supplementary Movie 3). With increasing T, however, the total displacement decreases and almost disappears. This is caused by the particles’ rotational diffusion time 1/DR, which determines their orientational dynamics between the pulses and leads to an increasing randomization, i.e. decorrelation of the particle orientation with increasing T. The orientational decorrelation between single pulses is shown as insets in Fig. 4b. While the particle orientation prior to each pulse remains rather preserved at small T, particles are almost isotropically aligned when T/(1/Dr)  1 and, thus, explains why eventually no net particle transport is achieved. With decreasing pulse velocity, the time APs spend within a pulse finally exceeds their reorientation time. Accordingly, they will perfectly (parallel) align to the local gradient of pulses and the displacement becomes independent of the time interval of pulses. This is shown in Fig. 4c for $$u/v_{\mathrm{p}}^{{\mathrm{max}}}$$ = 0.875 and demonstrates that transport of active particle by pulse trains is rather robust regarding parameter variations.

### Sorting mechanism

Apart from steering phototactic particles by trains of light pulses, this approach can be also employed for sorting APs. Since torques subjected by light gradients increase with the particle diameter σ27,40, the AP’s response to laser pulses becomes size-dependent. Exemplarily we discuss this for a binary mixture of APs with σsmall = 3.25 μm (rotational diffusion time 1/Drsmall 50 s and reorientation time σsmall = 3.3 ± 0.75 s) and σbig = 4.9 μm ($$1/D_r^{big}$$ 115 s and τbig = 1.83 ± 0.55 s) subjected to a periodic pulse train. It should be noted that the propulsion velocity only depends on the cap thickness but not on σ37. Figure 5a shows typical trajectories of big (red) and small (blue) APs, relative to their initial position x0 at t = 0 s. The data were obtained for u = 2 μm/s ($$u/v_{\mathrm{p}}^{{\mathrm{max}}}$$ = 1) and T = 5 s. As a result of the faster orientational response of the large APs (red trajectories), they can follow the propagating wave (thereby performing a similar back-and-forth motion as shown in Fig. 3a) and move to the right. On the opposite, small particles (blue trajectories) travel on average counter to the pulse train. Note that also motion along the pulse train becomes possible when θ ≈ 0, but then with much smaller displacements compared to θ ≈ π (compare Fig. 4b). Figure 5b shows the corresponding time-dependent probability distributions of small and large APs. With increasing time, we observe a broadening but also a shift of the mean values in opposite directions (Supplementary Movie 4).

## Discussion

In addition to our experiments, we also performed numerical simulations where we considered that (i) the AP propulsion velocity linearly increases with the local light intensity (Fig. 1b) and that (ii) an additional angular velocity is imposed on the APs in the presence of a light gradient (Eq. (2)). Since the light pulses travel along to the x-direction, the propulsion velocity and the orientational dynamics depend on space and time (the orientational dynamics additionally depends on the particle orientation ϕ relative to the local light gradient). For sake of simplicity, we approximated the intensity profile of a single pulse by two identical segments with constant and opposite gradients I. Thus, the vectorial translational and rotational Langevin equations can be written as

$${\dot{\mathbf{r}}} = v_{\mathrm{p}}\left( x \right){\mathbf{n}} + {\mathbf{\xi }}_{\mathbf{r}},$$
(3)
$${\dot{\boldsymbol{\theta }}} = \omega _{{\mathrm{max}}}{\mathrm{{sin}}}\phi \left( {x,t} \right) + {\mathbf{\xi }}_{\mathbf{\theta }},$$
(4)

where θ is the angle between the x-axis and particle orientation (inset Fig. 1b). The prefactor ωmax has been obtained from the theoretical fit in Fig. 6b (see the section “Methods” for further details). Brownian fluctuations are included by means of zero-mean Gaussian noise terms ξr and ξφ defined by the variances $$\left\langle {{\mathbf{\xi }}_{\mathbf{r}}\left( {t_1} \right) \otimes {\mathbf{\xi }}_{\mathbf{r}}\left( {t_2} \right)} \right\rangle = 2D_{{\mathrm{tr}}}1\delta (t_1 - t_2)$$) and $$\left\langle {{\mathbf{\xi }}_\theta \left( {t_1} \right){\mathbf{\xi }}_\theta \left( {t_2} \right)} \right\rangle = 2D_{\mathrm{r}}\delta (t_1 - t_2)$$), where denotes the dyadic product, 1 is the unit tensor, and Dt and Dr are the translational and rotational diffusion coefficients of a spherical Janus particle, respectively. Our numerical results (cf. Figs. 2 and 4) show excellent agreement with our experimental data and confirm that a spatio-temporal variation of the propulsion velocity in combination of an aligning torque is sufficient to understand particle motion along and counter to the direction of a traveling light pulse. Contrary to experimental trajectories which are limited by the field of view, we obtained simulated trajectories with total lengths up to 2000 μm. This allowed us also, to investigate the behavior of APs in pulse trains at much larger particle propulsion velocities compared to our experiments. In Fig. 6a, we show computed trajectories x(t) for different $$v_{\mathrm{p}}^{{\mathrm{max}}}$$. For $$u \ll v_{\mathrm{p}}^{{\mathrm{max}}}$$, the pulse is traveling too fast, so the particle comes almost immediately to rest when hitting the pulse, i.e. no net transport. In the optimal case, $$v_{\mathrm{p}}^{{\mathrm{max}}}$$ slightly larger than u, the particles are able to be reoriented within the pulse, which increases dramatically the directed particle motion. When $$v_{\mathrm{p}}^{{\mathrm{max}}} \gg u$$, the particles overcome the pulse without being reoriented. The long steady-state trajectories enable to extract the AP’s mean velocity of the V by doing a linear fit (see inset Fig. 6a), which is shown in Fig. 6b. As expected V increase when $$v_{\mathrm{p}}^{{\mathrm{max}}} \simeq u$$, that is when the mean residence time in the pulse becomes larger. Consequently, this protocol offers promising opportunities for sorting.

Our results show a complex response of APs to traveling light pulses. Contrary to amoebae, where a similar response results from the organisms capability to integrate and adapt to external signals6,7, APs respond strictly local and do not display memory. Instead, the APs response is due to the interplay of a modulation of their propulsion velocity and their phototactic properties. Because changes in the AP’s propulsion direction require their rotation which is limited by viscous friction with the solvent, this enables their motion towards or opposite to the direction of the pulse depending on the pulse velocity. This allows for a novel bidirectional steering strategy of APs which is contrast, to e.g. topographical structures42,43 or static optical landscapes12,27,44,45,46, where only unidirectional particle motion is observed. Apart from particle steering, the use of traveling pulses may be employed for effective sorting of APs according to their size, shape but also swimming velocity. Finally, it should be pointed out that the observed behavior does not only apply to the specific propulsion mechanism discussed here, but is also applicable to APs powered by chemotactic23,26,47, catalytic48,49,50,51, or thermophoretic52,53,54 forces.

## Methods

### Fabrication of APs and quantification of phototactic response

Active colloids were made from spherical silica particles (diameter σ = 3.25 μm) half-coated with 50 nm carbon caps. As solvent, we used a binary critical mixture of water–2,6-lutidine having a lower critical point at Tc = 34.1 °C. The entire sample cell is kept at a temperature of T0 = 31 °C using a bath cryostat. When the particles are homogeneously illuminated, the carbon cap becomes evenly heated by absorption of the laser light and its temperature will increase. When the cap’s temperature exceeds Tc, the solvent near the cap will demix resulting in the appearance of a droplet nucleating around the particle. As a result of local body forces and the wetting properties of the particles, this leads to a self-propelling particle motion. At low illumination intensities I < Ir the particle moves with the cap in the rear but reverses its direction of motion for I > Ir37 (Fig. 7a). Independent of the intensity, the AP performs a persistent random walk with a transition from a short-time ballistic to a long-time effective diffusive behavior38. Contrary to homogeneous illumination, the AP motion is no longer isotropic in the presence of a light gradient I. Under such conditions, the cap becomes unevenly heated leading to the nucleation of asymmetric droplets. This results in a torque which aligns the cap always (independent of I) towards larger intensities, i.e. the particle orientation n becomes parallel to I37. This eventually leads to a negative and positive phototactic behaviors for I < Ir and I > Ir, respectively (Fig. 7a). All experiments in this paper have been performed for intensities larger than Ir, i.e. under condition where the AP exhibits positive phototactic behavior, and where the propulsion velocity almost linearly increases with I (Fig. 7).

To quantify the orientational response of particles to light gradients, which is relevant for the AP’s encounter within the light pulse, we have measured their orientational response ϕ(t), i.e. the temporal change of the angle between I and the particle orientation n, when subjected to a light gradient. The inset of Fig. 7b shows the corresponding data for a particle with initial orientation ϕ = π and how it aligns parallel with I within ~2 s (in our experiments clockwise and anticlockwise rotation is observed). The AP’s reorientation dynamics in an intensity gradient I is (in absence of noise) described by the differential equation (2). Solving this equation gives $$\cos \phi \left( t \right) = {\mathrm{tanh}}(\omega _{\max }(\bar t - t))$$, where t is the time when $$\phi \left( {\bar t} \right) = \pi /2$$ and ωmax as the only fitting parameter used to obtain the theoretical fit in Fig. 7b and which strongly depends on I27. From this, one obtains the reorientation time $$\tau = \frac{2}{{\omega _{{\mathrm{max}}}}}{\mathrm{ln}}\left( {\frac{{\cos \left( {\phi _{{\mathrm{max}}}} \right) + 1}}{{\sin (\phi _{{\mathrm{max}}})}}} \right)$$, where ϕmax is the total rotation27. The reorientation times given in this paper correspond to the value for ϕmax = 3 rad, which is shown in Fig. 7b vs. I. As a result of the heat flux through the particle and its coupling to the surrounding solvent velocity at the particle surface, τ saturates at large gradients27. All gradients considered in this work (0.007 μW μm−3 < |I| < 0.04 μW μm−3) are above the saturation value and yield a constant reorientation time τ = 3.3 ± 0.75 s.

Creation of dynamical light patterns is achieved by a periodically oscillating mirror, which scans the elongated focus of a line-shaped (1 μm × 2000 μm) laser beam (λ = 532 nm) across the sample plane. For small voltages applied to the mirror (Vmirror), the displacement of the laser line is proportional to Vmirror. Synchronization of the scanning motion with the input voltage of an electro-optical modulator (VEOM) leads to spatio-temporal illumination patterns27. To generate a static light pattern, the ratio of the mirror-frequency νmirror and the EOM-frequency νEOM must yield a rational number, which determines the number of intensity maxima in the field of view. In order to create time-dependent illumination patterns, this ratio must be slightly varied (in our experiments we kept νmirror constant at 200 Hz and varied νEOM). This is schematically shown in Fig. 8a for the situation, where νmirror and νEOM are modulated according to a symmetric triangular and truncated triangular function, respectively. The time interval where VEOM ϕmax ≠ constant determines the width of the resulting traveling pulses. Figure 8b shows the dependence of the pulse velocity u on νEOM which increases linearly for small deviations from a rational number of the frequencies of the mirror and the EOM.

Due to the large thermal diffusivity of the carbon cap (~10–7 m2 s−1), the temperature and mixture’s concentration profile around the particle will respond on times scales below 10–5 s to changes in the illumination intensity37. For the given laser scanning frequencies, this leads to quasi-static illumination conditions and an immediate response of the particle propulsion to the spatio-temporal light field.

### Particle tracking

Images of the particles were acquired using video microscopy with a frame rate of 12 fps. The size of the region of interest is 300 μm × 160 μm. Particle tracking was performed using an automated tracking program developed in-house with Matlab image analysis software55. First, the background of images was removed by using an appropriate intensity threshold. The particle position r = (x,y) was approximated as the center of mass of the contours obtained after segmentation, with a spatial resolution 100 nm. Particle trajectories were calculated using Bayesian decision-making, linking every particle center with the previous closest one. Because of the optical contrast between the dark carbon hemisphere and the transparent silica, the particle orientation vector n = (cos θ, sin θ) can be obtained from the vector connecting the particle center and the intensity centroid of the particle image. The error of this detection is <5% as confirmed by comparison with stuck particles whose orientation can be precisely controlled.

### Simulated particle trajectories in a static motility gradient

To demonstrate, that the AP dynamics in light gradients are correctly described by our numerical simulations, we compared the experimentally observed dynamics of an AP in a static triangular motility profile (cf. Fig. 1). Indeed, the simulations show very similar trajectories, in particular, the oscillatory motion near the intensity maximum is reproduced very well. The results show good agreement between the point-like particles simulations (Fig. 9) and the experimental measurements (Fig. 1). For each experimental conditions, between 25 and 50 simulations were done.