## Abstract

Self-accelerating optical beams form as a direct outcome of interference, initiated by a predesigned initial condition. In a similar fashion, quantum mechanical particles exhibit force-free acceleration as a result of interference effects following proper preparation of the initial Schrödinger wave function. Indeed, interference is at the heart of such wave packets, and hence it is implied that self-accelerating wave packets must be coherent entities. Counter to that, we demonstrate theoretically and experimentally spatially incoherent self-accelerating beams, in both the paraxial and the nonparaxial domains. We show that in principle, the transverse correlation distance can be as short as a single wavelength, while a properly designed initial beam will give rise to shape-preserving acceleration for the same distance as a coherent accelerating beam propagating on the same trajectory. These findings expand the understanding of the relation between coherence and accelerating beams, and may have implications for the design of self-accelerating quantum wave packets with limited quantum coherence.

© 2015 Optical Society of America

## 1. INTRODUCTION

The field of accelerating wave packets has attracted extensive research interest in the last several years, since the concept of Airy wave packets (first formulated in quantum mechanics [1]) was introduced into optics [2,3]. This acceleration, or self-bending—in the case of spatial acceleration—is first and foremost an effect of wave interference. In the regime of small angles (the paraxial domain), proper design of the initial amplitude and phase can generate a beam that propagates along a parabolic trajectory while maintaining a shape-preserving Airy profile. Such self-bending beams have led to many intriguing applications in the past several years, including particle manipulations [4,5], curved plasma channels [6], Airy plasmons [7 –9], single-molecule imaging using the curved point-spread function [10], light-sheet microscopy using Airy beams [11], and even accelerating electron beams in electron microscopes [12]. The concept of accelerating beams was generalized to curved beams following arbitrary convex trajectories [13 –17], and accelerating beams were shown to allow additional functional forms besides the Airy function [18]. Accelerating wave packets were also proposed [2] and demonstrated [19,20] in the temporal domain, where shape-preserving pulses accelerate for long distances in dispersive media (fibers) until causality causes their breakup [21]. Importantly, this concept was recently generalized to the full Maxwell equations [22], thereby enabling large bending angles close to 180° and features on the scale of a single wavelength [23 –26]. This beyond-paraxiality generalization introduces a wealth of additional accelerating trajectories [27 –29]. Likewise, shape-preserving paraxial [30 –32] and nonparaxial [33,34] self-accelerating beams were also found in nonlinear media, such as Kerr, saturable, and quadratic nonlinearities [31,35], and even in nonlocal nonlinear media [36]. Finally, accelerating beams were also found in nonhomogeneous landscapes such as waveguide arrays [37] and photonic crystals [38]. The past seven years of research on accelerating optical beams, together with the recent demonstration of accelerating electron beams that took the concept to the quantum domain [12], has proved that accelerating wave packets exist in a very broad range of wave systems.

In all of these systems where accelerating wave packets were explored, the underlying principle is wave interference, since the entire effect of acceleration is the direct outcome of this most basic property of waves of any kind. However, waves are not necessarily fully phase coherent. In fact, natural light sources are generally incoherent—because in most cases the emission of electromagnetic radiation results from spontaneous emission. In the quantum domain, incoherence is introduced by coupling to the environment, which inevitably causes dephasing and is generally perceived as disruptive to any quantum process. Can shape-preserving accelerating wave packets also occur in wave systems that are only partially coherent? Can they occur in systems where the coherence length is extremely short, comparable to a single wavelength?

Thus far, research on accelerating wave packets was focused on coherent beams. The most common method for creating paraxial accelerating beams (Airy beams) is by shining the light through a cubic phase mask. Thus, the natural extension beyond coherent light would be to shine partially incoherent light through the same cubic phase mask, as indeed has been studied theoretically [39,40] and experimentally [41]. However, these few papers discussing self-accelerating beams using light that is not fully spatially coherent have treated imperfect coherence as a disruptive effect, claiming that the more incoherent a beam is, the shorter the range of its acceleration [39,41]. Those papers did not attempt to explain whether incoherence is indeed a fundamental limitation, but left the impression that incoherent shape-preserving accelerating beams are altogether impossible, due to the diminutive effects incoherence has on the propagation of such beams. Likewise, for other wave systems—from classical to quantum [12]—the lack of perfect coherence was always perceived as disruptive, and incoherent shape-preserving accelerating wave packets were thought to be impossible altogether.

Here, we investigate spatially partially incoherent shape-preserving accelerating beams, and demonstrate them theoretically and experimentally in both the paraxial and the highly nonparaxial regimes. We find that partial spatial coherence does not diminish the acceleration properties of the beam, provided that the beam is properly designed. Moreover, we show that it is possible to design accelerating beams with spatial transverse correlation distances as short as a single wavelength, and the beams still exhibit shape-preserving acceleration for the same distance as a coherent accelerating beam propagating on the same trajectory. Such highly incoherent accelerating beams display a single, broad intensity lobe and a smooth profile, instead of the highly oscillating one characteristic of all coherent accelerating beams. We provide explicit criteria for maintaining the acceleration despite the incoherence, and suggest applications, such as particle manipulation along curved paths [4,5,26], that could benefit greatly when the bending beams are partially incoherent. Finally, these findings may be beneficial for the design of self-accelerating quantum wave packets with limited quantum coherence.

## 2. THEORETICAL BACKGROUND

#### A. Spatial Incoherence

We begin by formulating the coherent-mode representation of partially spatially incoherent quasimonochromatic beams [42]. We write the electric field as $E(\mathrm{r\u20d7},t)=\mathrm{Re}(U(\mathrm{r\u20d7},t){e}^{i\omega t})$, where $\omega $ is the optical frequency and $U(\mathrm{r\u20d7},t)$ is an envelope that fluctuates much slower than the optical frequency. In this modal theory, the field $U(\mathrm{r\u20d7},t)$ can always be decomposed into a sum of statistically independent orthogonal modes, written as

where $U(\mathrm{r\u20d7},t)$ is the randomly fluctuating field, ${\psi}_{n}(\mathrm{r\u20d7})$ are the orthogonal modes that must satisfy boundary conditions in the medium, and ${c}_{n}(t)$ are randomly fluctuating complex coefficients, obeying $\u3008{c}_{n}^{*}(t){c}_{{n}^{\prime}}(t)\u3009={a}_{n}{\delta}_{n{n}^{\prime}}$, with ${a}_{n}$ having real values representing the power associated with each mode and $\u3008\xb7\u3009$ indicating time averaging over times longer than the characteristic fluctuations time. The coherence function, defined as $W({\mathrm{r\u20d7}}_{1},{\mathrm{r\u20d7}}_{2})=\u3008{U}^{*}({\mathrm{r\u20d7}}_{1},t)U({\mathrm{r\u20d7}}_{2},t)\u3009$, can now be written as#### B. Self-Accelerating Beams

We proceed by recalling the accelerating solutions of Maxwell’s equations [22]. In vacuum, the time-harmonic electric field obeys the Helmholtz equation:

where $k$ is the wavenumber. The accelerating solution for the Helmholtz equation was shown to move along a circular trajectory [22]. For a TE-polarized electric field, $\mathrm{E\u20d7}={E}_{y}(x,z)\widehat{y}$ can be written as## 3. INCOHERENT SELF-ACCELERATING BEAMS: USING ACCELERATING MODES

#### A. Theory

Next, we construct partially spatially incoherent accelerating beams from these paraxial and nonparaxial solutions [Eqs. (6) and (4), respectively]. Based on the coherent mode representation of the coherence function [Eq. (2)], it is clearly seen that if only some of the modes are accelerating while the others do not accelerate, then the entire incoherent beam will exhibit weaker acceleration properties (i.e., weaker acceleration and shorter acceleration range). Similarly, if all the modes are accelerating but they do it along different curves, the acceleration of the entire beam will be washed out and once again the beam will exhibit weaker acceleration properties. Therefore, we reason that in order for an incoherent beam to accelerate at a rate and a range equivalent to that of a coherent beam, the incoherent beam must be comprised strictly of modes that accelerate along the same curve. In the nonparaxial regime, such an accelerating incoherent beam should be constructed from stochastically populated modes that accelerate along the same circular trajectory with the same origin, but have different values of the radius parameter $\alpha $, resulting in a beam comprised of a set of concentric rings:

#### B. Experiment

Experimental results with incoherent nonparaxial accelerating beams are presented in Fig. 3. The experimental system is depicted in Fig. 3(a). Laser light with a wavelength of $\lambda =532\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{nm}$ is used. A spatial light modulator (SLM) imposes the appropriate phase profile for generating nonparaxial accelerating beams [22], and two objective lenses (X60, $\mathrm{NA}=0.85$) focus the accelerating beam to the micrometer scale. By moving one of the objective lenses, we image the intensity pattern at different planes and thus map out the acceleration trajectory of the beam. Experimentally, we first generate a coherent nonparaxial accelerating beam, with the radius parameter $\alpha =800$. This beam bends on a circular trajectory, over an angle of approximately 65°, which is highly nonparaxial, as presented in Fig. 3(b). Next, we generate an incoherent beam where all the modes comprising it accelerate along the same trajectory, as described by Eq. (7). We do so by alternating among multiple phase profiles imposed on the SLM, each of which is properly designed to launch a single accelerating beam with a given $\alpha $ parameter. When the SLM alternates among these phase profiles (at 16 Hz) faster than the integration time of our camera (1 Hz), the camera measures only the time-averaged intensity distribution. This measured time-averaged intensity is equal to the intensity distribution of an incoherent beam constructed from exactly the same modal structure. This is due to the fact that for incoherent light the interference among modes is washed out because their fluctuating populations ${c}_{n}(t)$ are uncorrelated. Likewise, in our experimental realization the interference among modes is nonexistent because the modes alternate, never coexisting within the same time window. However, because all the modes are accelerating along the same trajectory, the lack of coherence does not hamper the acceleration. We present two examples of nonparaxial accelerating incoherent beams, both consisting of 16 modes. The first is presented in Fig. 3(c), with $\alpha $ spanning from 786 to 816. It can be seen in Fig. 3(c) that the beam bends over an angle of approximately 70°, which is even larger than the coherent case, while maintaining a beam profile that is smooth and without the oscillations that are an inherent part of any accelerating coherent beam. The coherence length at $z=0$ is calculated to be ${l}_{c}\approx 2\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{\mu m}$. The second example is presented in Fig. 3(d), with $\alpha $ spanning from 730 to 880. In this case, the main lobe is very thick, and the coherence length at $z=0$ is calculated to be ${l}_{c}\approx 0.7\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{\mu m}$, which is about $1.4\lambda $. The beam in the second example accelerates over an angle of $a$, which is the same as the coherent beam generated using similar parameters. Thus, we have experimentally demonstrated an incoherent nonparaxial accelerating beam with a coherence length on the order of a single wavelength.

## 4. INCOHERENT SELF-ACCELERATING BEAMS: USING LIGHT FROM ROTATING DIFFUSER

#### A. Theory

Having demonstrated how to engineer a highly incoherent accelerating beam, the next natural question would be: is it possible to accelerate a beam of natural incoherent light? To answer that, we analyze the features of quasimonochromatic, spatially incoherent accelerating beams generated, for example, with a rotating diffuser [43,44], or from spectrally filtered sunlight passed through a pinhole [45]. We analyze such beams in the paraxial regime, and model them using the Gaussian Schell model [42], in which the spatial coherence between two points is a Gaussian function of the distance between them. A similar treatment was presented for the case of nondiffracting incoherent Bessel beams [46]. For simplicity, we focus on one-dimensional beams, but our results apply equally well to two-dimensional cases. Using a beam with a Gaussian intensity profile, we can write the coherence function at the Fourier plane [42,43]:

#### B. Experiment

We now present the experimental results with incoherent paraxial accelerating beams. The experimental setup is sketched in Fig. 4(a). The incoherent beam is obtained by passing a 532 nm laser beam through a rotating diffuser. The beam is then reflected from the SLM, where the cubic phase pattern is imposed, thus achieving the form of Eq. (9). A Fourier transforming lens is placed to obtain the incoherent accelerating beam, such that ${x}_{0}=75\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{\mu m}$ and the truncation parameter is $a=0.075$. To enable proper comparison with coherent accelerating beams, we first present the propagation of a coherent accelerating beam. The initial beam and the beam at propagation distance $z=20\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{cm}$ are shown in Figs. 4(b) and 4(c), respectively. Figure 4(h) shows the corresponding side view of the propagation, where the bending of the main lobe is clearly visible. Next, we present two examples of accelerating beams with incoherent light. In the first example, the transverse coherence length at $z=0$ is ${l}_{c}=215\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{\mu m}$, and the initial beam and the beam at propagation distance $z=20\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{cm}$ are shown in Figs. 4(d) and 4(e), respectively. Figure 4(i) shows the corresponding side view of the propagation, where the bending of the main lobe is again clearly visible, despite the obvious fact that the intensity oscillations of the beam are smeared. The smearing is even more pronounced in the second example with ${l}_{c}=115\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{\mu m}$, which is on the order of about half the width of the main lobe of the coherent beam. The initial beam and the beam at propagation distance $z=20\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{cm}$ are shown in Figs. 4(f) and 4(g), respectively. Figure 4(j) shows the corresponding side view of the propagation. The deflection of the main lobe is again clearly visible, despite the complete lack of the intensity oscillations. That is, this incoherent accelerating beam has no sidelobes whatsoever, in sharp contrast with coherent accelerating beams where the acceleration (beam bending) is created by the oscillating structure of the beam. The results are summarized in Fig. 4(k), where the deflection of the main lobe versus the propagation distance is plotted. According to our estimates, in both the coherent and incoherent cases the acceleration dynamics breaks down at $z\approx 70\text{\hspace{0.17em}}\text{\hspace{0.17em}}\mathrm{cm}$, which is outside our experimental regimes. Nevertheless, our experimental results clearly demonstrate that despite significant incoherence and even when the transverse coherence length ${l}_{c}$ can be on the order of one half the width of the main lobe, the acceleration dynamics persists in the same way as in the fully coherent case.

## 5. CONCLUSIONS

In conclusion, we have presented, experimentally and theoretically, incoherent accelerating beams, in both the nonparaxial and the paraxial regimes. We have shown that by constructing the incoherent beam solely of modes that accelerate along the same trajectory, the incoherence does not hamper the acceleration. We demonstrated experimentally incoherent nonparaxial beams with a transverse coherence length on the order of a single wavelength, which accelerate up to the same bending angle as their coherent counterparts with similar parameters. We demonstrated how to engineer such beams using temporal modulation of the phase mask, a technique that will be useful for all applications where the natural response time is slower than the modulation speed—for example, particle manipulation along curved paths. In addition, we analyzed incoherent accelerating beams generated using natural light, and have shown, theoretically and experimentally, that for a wide range of parameters the incoherence of the beam does not hamper its acceleration properties. Our work provides a new outlook for the field of accelerating beams, no longer treating incoherence as a disruptive effect, but rather expanding the scope of beam acceleration to incoherent wave packets. Finally, the concept presented here also applies to accelerating wave packets outside the domain of optics, for example, accelerating electron beams, accelerating ion beams, and accelerating beams of cold atoms, where incoherence often poses major challenges.

## Funding

I-CORE Israeli Center of Excellence “Circle of Light”; U.S. - Israel Binational Science Foundation (BSF); Israel Science Foundation; Marie Curie (328853–MC–BSiCS); National Key Basic Research Program (2013CB328702, 2013CB632703); National Natural Science Foundation of China (NSFC) (11304165); 111 Project of China (B07013); PCSIRT (IRT0149); National Science Foundation (NSF); Army Research Office.

See Supplement 1 for supporting content.

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