Abstract
Excitonpolaritons are lightmatter mixed states interacting via their exciton fraction. They can be excited, manipulated, and detected using all the versatile techniques of modern optics. An excitonpolariton gas is therefore a unique platform to study outofequilibrium interacting quantum fluids. In this work, we report the formation of a ringshaped array of same sign vortices after injection of angular momentum in a polariton superfluid. The angular momentum is injected by a ℓ = 8 LaguerreGauss beam. In the linear regime, a spiral interference pattern containing phase defects is visible. In the nonlinear (superfluid) regime, the interference disappears and eight vortices appear, minimizing the energy while conserving the quantized angular momentum. The radial position of the vortices evolves in the region between the two pumps as a function of the density. Hydrodynamic instabilities resulting in the spontaneous nucleation of vortexantivortex pairs when the system size is sufficiently large confirm that the vortices are not constrained by interference when nonlinearities dominate the system.
Introduction
Quantized vortices have been extensively investigated in different fields of physics, such as superconductivity^{1}, matterwave superfluids^{2} and nonlinear optics^{3}. In this context, halflight, halfmatter polariton fluids offer an unprecedented opportunity to study the quantumfluid aspects of interacting photons, a rich field at the interface of condensed matter and quantum optics. The recent discovery of polariton BoseEinstein condensation in semiconductor microcavities^{4,5,6} has renewed the possibilities of observing superfluidity in quantum fluids of light^{7}. As a consequence, the understanding of the mechanism of vortex nucleation and vortex dynamics in such systems becomes particularly important. Vortices are natural topological solutions in interacting photonic systems^{8,9}. Indeed, the nucleation of vortices^{10,11,12,13,14} and halfvortices^{15,16} in polariton fluids have been reported in several experiments.
Several schemes to produce vortices and vortex lattices have been proposed and implemented. Liew et al^{17} predicted the formation of regular triangular lattices and of Penrose triangular lattices with coherently pumped polariton condensates, while Gorbarch and coworkers^{18} proposed to create robust halfvortex lattices in the optical parametric oscillator (OPO) scheme. Spontaneous selfordered vortexantivortex pairs have been recently reported in Refs. 19, 20 and Hivet et al^{21} experimentally demonstrated the formation of vortexantivortex lattices in square and triangle trapping potentials. Nevertheless, none of these schemes allow the effective transfer of a global angular momentum, therefore preventing the spontaneous nucleation of samesign vortex lattices.
In this work, as a first step towards the physics of rotating polariton quantum fluids, we theoretically propose and experimentally implement a scheme that generates stable chains of samesign vortices in a coherently driven polariton superfluid. The global angular momentum is injected by mean of a LaguerreGauss (LG) laser beam with orbital angular momentum ℓ. Note that selfordered, samesign vortex lattices have been theoretically predicted in Ref. 22. However, in this ideal, disorderfree scheme, an important experimental limitation arises, as the lattice rotates at very high angular velocities, therefore making timeresolved interferometry measurements a very difficult task. To circumvent the issue of fast rotation in our scheme, an additional Gaussian beam (G) with zero angular momentum is added at the center of the LG beam. The central Gaussian beam allows to lock the azimuthal position of the vortices. We use a Spatial Light Modulator (SLM) to produce the spatial profile of the resonant pumps. This hologrambased optical technique is very versatile and can be used to generate a wide variety of pumping schemes for polaritons. Based on a variational analysis of the generalized GrossPitaevskii equation, we then show that the vortex chain is a consequence of the quantization of the total angular momentum transferred to the superfluid, thus different from a trivial interference pattern imposed by the pumps. The quantum nature of the fluid is also confirmed by the appearance of hydrodynamical instabilities, resulting in the nucleation of vortex–antivortex pairs.
These characteristics are close to those of cold atom condensates^{29,30,31,33}, where the angular momentum can be externally transferred either by stirring^{32} or via rotation of the trapping potential. In this case, the vortices nucleate and selforganize into an Abrikosov lattice. In our case, the ring geometry is imposed by the pumps, resulting in an additional constraint. In the context of atomic BECs, the method consisting in transferring angular momentum from photons to atoms was studied as well. In particular Dutton and Ruostekoski^{28} theoretically studied the formation of vortex lattices upon illumination with LG beams, and the injection of angular momentum into atomic BECs with LG beams was achieved^{26,27}. Interestingly, in the case of polariton fluids the injection method is not strictly identical since the rotating polaritons are directly created by the LG pump, as opposed to injections of angular momentum into a preexistent, nonrotating superfluid.
Results
Experimental setup
We consider a planar semiconductor microcavity in the strong coupling regime, where excitonphoton coupled states (i.e. polaritons) are created by a laser excitation. We make use of a CW single mode, frequencylocked Ti:Sa laser to resonantly excite the cavity. Resonant pumping creates a lowdensity exciton gas, which allows us to neglect interactions between polaritons and the exciton reservoir, in contrast with experiments performed under nonresonant pumping^{20}. The laser is tuned to be quasiresonant with the ground state of the lower polariton (LP) branch (~837 nm), so that the detuning with respect to the bottom of the LP branch is given by Δ = ω_{laser} − ω_{pol}, where ω_{laser} and ω_{pol} are respectively the pump and bare polariton energies at normal incidence k = 0 μm^{−1}. A singlemode, polarizationpreserving fiber selects the TEM_{00} mode. The polarization is linear (vertical) after the fiber and the remaining polarization fluctuations are cut by a polarizing beam splitter (PBS). As visible in Fig. 1 (a), the collimated laser beam is then sent to a SLM, which allows us to arbitrarily modify the spatial phase profile of the beam.
By programming a specifically designed phase hologram on the SLM, we can create beams with welldefined intensity and phase profiles. We create a coherent superposition of a ringshaped LaguerreGauss (LG) beam of orbital momentum ℓ = 8 and a Gaussian (G) beam of zero orbital momentum at the center. Both the spot size and the intensity of the laser beams are fully determined by the hologram. The LGbeam diameter is chosen to be larger than the waist of the Gbeam. As a result, their spatial overlap is small, allowing for the interference to be very weak. To avoid spindependent phenomena, the () polarization is set to circular with a quarterwave plate, before being focused on the sample by an aspherical condenser. In Ref. 23, a SLM was used to create a ring shaped condensate, but using nonresonant optical excitation. As a result, the condensate created was in a superposition of two states with opposite angular momentum without the formation of a vortex lattice.
Sample
The sample is a 2λGaAs planar microcavity containing three GaAsInGaAs quantum wells, with a polariton Rabi splitting of 5.1 meV. The cavity finesse is F = 3000, which results in a polariton linewidth of about 0.1 meV. The cavity is wedged in one direction, providing a large choice of cavityexciton detunings by pumping at different positions in the sample. In order to enhance the polaritonpolariton interactions, we use a cavityexciton detuning of δ = ω_{C} − ω_{X} = 1 meV (ω_{X}_{(C)} is the excitonic (cavity) energy at normal incidence, k = 0 μm^{−1}), thus increasing the exciton fraction of polaritons and, consequently, the nonlinear effects. The microcavity is cooled down to 5 K in a cryostat and the measurements are taken in transmission. Above a critical value of Δ, a bistable behavior appears^{24}. By increasing Δ and working within the upper bistability branch, we increase the polariton density. This is necessary to reach the regime where nonlinearities dominate. We therefore use the polariton bistability to control the density as follows: in the upper bistability branch, at constant pump power I_{p} = 300 mW, we modify Δ. We consider three different cases: low density (Δ_{1} ≈ 0 meV, point (i) in Fig. 1 (b)), high density far from the bistability threshold (Δ_{2} = 0.4 meV, point (ii) in Fig. 1 (b)) and near the bistability threshold (Δ_{3} = 0.7 meV, point (iii) in Fig. 1 (b)).
Detection
The detection is simultaneously made in energy and in real and momentum space. An objective collects the sample emission. CCD cameras are used for direct imaging of the real and the momentum space, while the energy (wavelength) is measured with a spectrometer. We only collect circularlypolarized light, therefore filtering out any residual spinflip effect. The polariton phase is measured with an offaxis interferometry setup: a beam splitter divides the realspace image into two parts, one of which is expanded to generate a phase reference beam. The selection of the Gaussian part at the center of the image ensures a flat phase reference, which is used to make an offaxis interference pattern. With this method, the vortex position in the image is independent of the phase of the reference beam^{25}. The actual phase map is then numerically reconstructed with a standard offaxis phase detection method.
Theory
In order to describe the configuration under study, we numerically solve the drivendissipative GrossPitaevskii equation, which in the parabolic approximation readsHere, P(r) = P_{LG}(r) + P_{G}(r) with and ; A_{1} and A_{2} are the amplitudes of the pumping lasers, with σ_{1} = 5.0 μm and σ_{2} = 3.0 μm. Direct comparison with the experiments is then performed by extracting the steadystate density ψ^{2} and phase arg(ψ).
Results
In the linear regime (Δ = Δ_{1} ≈ 0 meV), we observe  both experimentally (Fig. 2 a),b)) and theoretically (Fig. 2 c),d))  a pattern resulting from the optical interference between the LG and G beams. This interference pattern consists in an eightlobbed spiral (Fig. 2 a),c)) with eight phase singularities (Fig. 2 b),d)). The annular phase singularity chain visible in Fig. 2 is thus imposed by the pump phase. As the density increases, the nonlinear behavior of polaritons is unveiled, with a deformation of the interferences. For Δ = Δ_{2} = 0.4 meV (point (ii) in Fig. 1 (b)), the calculated pattern shown in Fig. 3 (c) is reduced to roundshaped dips of quasizero density containing the phase singularities: the eight elementary vortices carrying the injected angular momentum, with a homogeneous density around the dips. In the experiment we observe a ring of samesign vortices with a density distribution much more uniform than in the linear case, with some residual variations. The vanishing of the interference pattern means that the polariton phase is no more imposed by the pump and is modified through the nonlinear interactions, generating specific features compared to an optical interference pattern. Our observations are consistent with other resonant and nonresonant pumping experiments done in absence of angular momentum^{20,21}. The formation of a ring of ℓ singlecharged vortices from a pump with angular momentum ℓ is a manifestation of the quantum nature of the polariton fluid, in analogy to the formation of the Abrikosov lattice from a single highlycharged vortex.
It is important to remark that the spatial freedom of the vortices provides a quantitative test of the model given below. As predicted by our model, we observe that the vortices in the nonlinear case exhibit a radial phase freedom, while their azimuthal position is locked by the pump phase. Their radial position is modified as the density ρ = ψ^{2} increases. In order to quantify the dependence of the ring radius R_{0} on the relevant experimental parameters, we employ a variational method. We describe the vortex chain solution with the variational ansatzwhere ψ_{TF}(r) = ρ^{1/2}[P_{1}(r)/A_{1} + P_{2}(r)/A_{2}] is the ThomasFermi density profile induced by the pump, r_{i} = R(cosθ_{i}, sinθ_{i}) is the position of each vortex in the chain, and is the average healing length. In Fig. 4 a), we plot the variational profile given by Eq. (2). The value of R that minimizes the energy, R_{0}, can then be extracted by minimizing the total energy E[R] = E_{kin} + E_{int} and taking the physically relevant solution of the condition δE/δR = 0, whereIn Fig. 4 b), we plot the energy E as a function of R for different values of ξ ~ ρ^{−1/2}. We observe that R_{0}, the value of R that minimizes the energy, increases as the value of ξ (ρ) is decreased. Since ρ increases with Δ, ξ decreases with Δ; it follows that R_{0} increases with Δ. Fig. 4 c) shows R_{0} as a function of ρ calculated by this method and the comparison with experimental data. As expected, the higher the density, the further from the center the vortices migrate. This behavior and the agreement between the variational method and experiment are a clear indication of the phase freedom obtained when interactions dominate, a feature that is independent from the optical interference.
In the upper bistability branch, the polariton energy is renormalized through selfinteraction to the pump energy, so that the pumping is resonant and yields high polariton densities. This is not the case in the lower bistability branch, where the pumping is not resonant and thus inefficient. For large Δ, the low pump intensity regions in the lower bistability branch are offresonant, as can be seen in Fig. 1 (b). In these regions, nonresonant pumping yields a negligible polariton population and can be considered as a pumpfree region. For example, near the threshold, for Δ = Δ_{3} = 0.7 meV (point (iii) in Fig. 1 (b)), a large area between the LG and G pumps is not pumped. Although no polariton is directly injected in this area, the density is not zero due to polaritons propagating from the pumped to the nonpumped area. In this region, the phase is free to evolve, which explains the radial chain expansion. Moreover, when the density in this pumpfree area is large enough and when the size of this region is at least of the order of the vortex core ~ ξ, we observe the spontaneous nucleation of vortexantivortex pairs. Four pairs are experimentally visible in Fig. 5 and eight in the theoretical figure. This discrepancy between theory and experiment for the number of pairs is due to the cavity wedge making the experimental cavity anisotropic, a property that is absent in the simulations. The vortexantivortex pairs form a lowdensity ring inside the vortex chain described above. This is due to a hydrodynamic instability of the same nature as the one observed in the ℓ = 0 case^{14}, but here each pair formation is stimulated by the presence of a vortex which acts as a defect. The disorderfree model confirms that the vortexantivortex pairs are generated by the vortices of the main chain and not by the disorder. This feature also proves that the vortex distribution is not due to optical interference in the superfluid regime, but that it rather evolves with the density.
Discussion
In the present work, we resonantly inject polaritons with a given total angular momentum and observe the formation of a ring of quantized singlecharged vortices. For the first time, a regular ring pattern of elementary vortices of the same sign is reported in a polariton superfluid. In the superfluid regime, the radial position of each vortex is not determined by the pump but rather depends on the polariton density. Experimental and theoretical indications of this behavior, due to strong nonlinear interactions, are provided through the system hydrodynamical characteristics. The mechanism leading to the creation of vortex chains results from the combination of the saturation of the radial counterflow instability with the injection of angular momentum in a limited region of space. Let us note that this general behavior was experimentally and theoretically verified to be the same if the number of injected vortices is changed, whether odd or even. We expect that the present scheme will pave the stage to study a series of new vortex collective phenomena that have been observed in cold atom BEC^{2}. It is also a first step towards a new class of experiments investigating selfarranged samesign vortex lattices, unveiling the physics of vortexvortex interactions in polariton superfluids. In particular, the collective dynamics of the vortex chain (Tkachenko modes)^{34,35,36}, for which the polariton lifetime is expected to play a central role in the mode damping, can be of great interest.
Methods
Collimated LaguerreGauss beams are a class of modes possessing a simple phase profile with radial invariance. The phase profile of a mode is given by the function φ_{LG}(r, φ) = ℓφ [2π], where (r, φ ∈ [0, 2π]) are the polar coordinates in the SLM plane. However, imposing this phase on the SLM produces a superposition of and weak higher modes in the condenser lens focal plane. Since the higher modes are spatially more extended, they can be cut with an iris placed before the condenser lens, which solves the problem. The result is a good quality beam. Adding the central Gaussian pump is straightforward as the mode imprinted on the SLM is Gaussian: we simply need to impose a flat phase in the hologram. This has been done by using the phase function φ_{LG + G}(r, φ) = ℓφH(r − r_{0}) + π(1 − H(r − r_{0})), where H(r) is the Heaviside distribution and r_{0} is a constant determining the LG/G intensity ratio. The resulting hologram is presented in Fig. 6 (a).
A small fraction of the light is not modified by the SLM, for which it acts like a mirror. To separate this from the desired mode a grating hologram (, where d controls the separation angle) is added to the LG + G hologram (mathematical sum modulo 2π). This vertically deviates the first order reflection forming the pump, allowing us to block the zeroorder reflection. The final hologram is presented in Fig. 6 (b).
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Acknowledgements
We acknowledge the financial support of the ANR Quandyde (ANR11BS10001), ANR Labex GANEX (ANR11LABX0014) and IRSES POLAPHEN (246912).
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Affiliations
Laboratoire Kastler Brossel, UPMCSorbonne Universités, CNRS, ENSPSL Research University, Collège de France, 4, place Jussieu Case 74, F75005 Paris, France
 T. Boulier
 , Q. Glorieux
 , E. Giacobino
 & A. Bramati
Institut Pascal, PHOTONN2, Université Clermont Auvergne, Blaise Pascal University, CNRS, 24 Avenue des Landais, 63177 Aubière Cedex, France
 H. Terças
 , D. D. Solnyshkov
 & G. Malpuech
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Contributions
T.B. performed the experiment, analyzed the data and wrote the manuscript. H.T. and D.S. performed the simulations and wrote the manuscript. Q.G. and E.G. participated to the manuscript. A.B. supervised the experiment. G.M. developed the theoretical model. All authors reviewed the manuscript.
Competing interests
The authors declare no competing financial interests.
Corresponding authors
Correspondence to G. Malpuech or A. Bramati.
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Further reading

Interactions and scattering of quantum vortices in a polariton fluid
Nature Communications (2018)
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