The strong coupling of excitons to optical cavities has provided new insights into cavity quantum electrodynamics as well as opportunities to engineer nanoscale light–matter interactions1,2,3,4,5,6. Here we study the interaction between out-of-equilibrium cavity photons and both neutral and negatively charged excitons, by embedding a single layer of the atomically thin semiconductor molybdenum diselenide in a monolithic optical cavity based on distributed Bragg reflectors. The interactions lead to multiple cavity polariton resonances and anomalous band inversion for the lower, trion-derived, polariton branch—the central result of the present work. Our theoretical analysis reveals that many-body effects in an out-of-equilibrium setting result in an effective level attraction between the exciton-polariton and trion-polariton accounting for the experimentally observed inverted trion-polariton dispersion. Our results suggest a pathway for studying interesting regimes in quantum many-body physics yielding possible new phases of quantum matter7,8,9,10,11 as well as fresh possibilities for polaritonic device architectures12,13,14,15.
Coupled harmonic oscillators are ubiquitous in physics and an exemplary platform to observe them is with cavity exciton-polaritons1,2. Pioneering work reported planar cavity photon and quantum well exciton-polariton formation3,4. Since then a wide range of optical resonances have been coupled to excitonic resonances5,6. Studies have ranged from studying polariton amplification, condensation and interactions with a two-dimensional electron gas7,8,9,10,11,16 to leveraging these quantum matter coherences for light generation17,18,19. But, in almost all the previous work, the focus has been on polaritons formed out of neutral excitons and photons, with little work on other exciton complexes20,21.
The past decade has witnessed the emergence of atomically thin transition metal dichalcogenides (TMDCs) that support strongly bound neutral22, charged exciton resonances23 and defect excitons24. TMDC materials exhibit large exciton binding energies, stabilizing them at room temperature25,26. Recent work demonstrated polariton formation27, and shortly thereafter negatively charged excitons (trions) and polarons were coupled to cavity photons28,29. In this work we study cavity polariton physics with a device that supports dispersing and mutually interacting, out-of-equilibrium, cavity photons, neutral excitons and negatively charged excitons.
Figure 1a presents an illustration of our device architecture (see Methods) containing the single-layer TMDC, molybdenum diselenide (MoSe2), at the cavity anti-node. Natural doping levels are such that the device supports both neutral excitons and trions that can couple with the cavity photon. A conventional approach to describe the above excitations in the system would involve modelling them in terms of bosonic oscillators, as shown in Fig. 1b. We would expect to observe three polariton branches, an upper, middle and lower polariton branch (UPB, MPB, LPB). Such theoretically expected dispersions are presented in Fig. 1c using known energy detunings from our experiments, and this was indeed observed in recent experiments21.
The previous are in contrast to our observation shown in Fig. 1d. Figure 1d is a measurement of our device’s polariton dispersion. The dispersion of the lower trion-polariton branch is completely inverted (compare to Fig. 1c), which translates to a negative mass for the trion-polaritons in the neighbourhood of k∥︀ = 0. This is the central observation of our work. In what follows we describe the physics resulting in this spectrum and find it depends on the fermionic nature of the trions and how they interact with cavity photons, the strong interaction between the trions, the MPB and electrons, and the out-of-equilibrium regime of the experiment. Note that the fundamental difference between the earlier observation30 of negative polariton mass and this work is that many-body interactions result in an anomalous trion-polariton dispersion, resulting in charged cavity polaritons exhibiting negative mass in the neighbourhood of k∥︀ = 0.
In our system, the constituent resonances are the MoSe2 exciton, trion and the cavity photon. The bottom panel of Fig. 2a presents the measured photoluminescence (PL) spectrum of the single-layer MoSe2 flake on a SiO2 substrate. We observe a stress-induced redshift of 8 meV for both the neutral and charged excitons when the monolayer is embedded inside the microcavity. The exciton (trion) linewidth is 7 meV (9 meV). Reflectance spectroscopy of the unloaded cavity (top panel, Fig. 2a) identifies the spectral location of the cavity resonance and reveals a quality factor of 600 and a linewidth of 3 meV. A PL spectrum of the loaded cavity is presented in Fig. 2b.
To unmask the polariton dispersion an angle resolving measurement set-up was constructed that images the objective (numerical aperture, NA 0.7) Fourier plane onto a spectrometer (Fig. 3a). The raw angle-resolved spectrum is shown in Fig. 3b, where the colour represents the differentiated intensity of PL in log (the raw PL data are shown in the Supplementary Section 2). As shown in Fig. 3c, it is possible to measure PL spectra at specific values of in-plane momentum. Fits to each of the polariton resonances in the spectra of Fig. 3c map the full polariton dispersion relation as reported in Fig. 1d. We observe a large Rabi splitting of ∼25 meV at zero in-plane momenta when the cavity photon and exciton are resonant (see Supplementary Section 1a).
To understand the microscopic mechanism responsible for the observed inverted dispersion relation and the negative trion mass, we introduce the following Hamiltonian written in momentum space where ck† (ck), ak† (ak), ψk† (ψk), and Γl, k† (Γl, k) are the electron, photon, trion, upper (l = 1) and middle (l = 2) polariton creation (annihilation) operators, respectively; Δkel, ωktr, Ek1, Ek2, are the bare electron, trion, upper, and middle polariton resonance energies. v2 quantifies the interaction strength of the cavity photon, electron and trion and v3 quantifies the interaction strength of the middle polariton, the electron and the trion (see Supplementary Fig. 1). In equation (1) we have neglected the interaction between the upper polariton and the trion as they are detuned from resonance. In this experiment, we have a small relative detuning between the cavity photon and the uncharged exciton and the trion is detuned by 30 meV below the cavity resonance.
Assuming that the free electron concentration is such that the majority of free electrons form trions with the optically excited excitons31, we integrate out the electronic contribution in the model. To the leading order in perturbation theory in v2 and v3 (see Supplementary Section 1b), this generates interaction between the photons and the trions, between the middle polariton branch and the trions, as well as mutual interaction among the photons, middle polariton branch and the trions. In addition, it also renormalizes the bare dispersion of the trion. Now, to account only for the dispersion, we make a mean-field approximation by introducing mean-field occupation numbers for the trions and the polaritons: 〈ψk′ †ψk〉 = δk′kntk and 〈Γak†Γbk′〉 = δkk′δabnΓa, k, where ntk and nΓa, k are the respective out-of-equilibrium occupation numbers for the trion and upper (a = 1) and middle (a = 2) polariton modes. Since such out-of-equilibrium occupancy is expected to be very different from the equilibrium Bose–Einstein (for polaritons) or Fermi–Dirac (for trions) distributions, within mean-field theory we take the ratio of occupancies of the MPB and UPB as a k-independent fitting parameter. The data in Fig. 1d are fitted by a ratio of ∼1.3 in accordance with the PL data (see Fig. 2b).
The mean-field Hamiltonian (see Supplementary Section 1d) can be diagonalized to yield the dispersion relation. The data in Fig. 1d are fitted by our model (seen Supplementary Table 1). In particular, for the trion-polariton branch our mean-field calculations yield the following dispersion where αk and βk (see Supplementary Section 1c) are two matrix elements that transform the exciton–photon basis to the polariton basis, Etr0 is the bare trion energy and E(αk, βk) captures the many-body effects present in our device. The sign of E(αk, βk) is determined by the relative sign of the coupling constants v2 and v3, and we find the relative sign of v2 and v3 has to be opposite to give the hybridization.
We can understand the above inverted trion-polariton dispersion as resulting from an electron-mediated interaction between the exciton-polariton branch and the trion-polariton that overwhelms the weak trion cavity repulsion, leading to level attraction. The origin of such an interaction may be understood in terms of exchange of an electron between a neutral exciton and the negatively charged trion, and thus gaining delocalization energy of the trion’s electron. Note in ref. 32 that the combination of increased sample doping and zero cavity–trion detuning overwhelms the many-body-interaction-induced inverted dispersion observed in Fig. 1d.
To demonstrate the level attraction is controllable we vary the device temperature. Figure 4a shows data for the temperature-dependent trion-polariton dispersion branch (T = 6 K, 25 K and 45 K). In this temperature range the bare exciton is first red-detuned from the cavity (T = 6 K), brought into resonance near 25 K, and then becomes blue-detuned from the cavity for higher temperatures (above 55 K the trion becomes unstable). The tunability of the LPB negative mass, determined via meff−1 = ℏ︀−2(d2E/dk2), in the vicinity of low k∥︀ for different temperatures is presented in Fig. 4b (see Supplementary Section 3). In Fig. 4c, the trion-polariton zero momentum energy Etr(0) is plotted. The solid (open) circles present the raw data (model). As the temperature is increased, the exciton is brought into resonance with the optical cavity and the level hybridization between the exciton-polariton and the trion-polariton is enhanced. This is again seen in Fig. 4d, where the energy difference at zero in-plane momentum between the UPB and MPB (ΔEUPB–MPB) and MPB and LPB (ΔEMPB–LPB) is plotted as a function of temperature.
The ease with which atomically thin materials can be doped and incorporated in photonic devices will provide many opportunities to study Fermi polaritons in the solid state. Future work will involve controlled in situ doping and resonant, angle-sensitive polariton pumping. Further, the combination of the magnitude and sign of the lower polariton branch effective mass and its extra charge provide a unique opportunity to build responsive current-carrying polaritonic circuitry that exhibits anomalous dissipative behaviour. We intend to explore how the negative mass influences the effect of disorder on the flow of the observed negative mass charged polaritons.
We deposit silicon dioxide (SiO2) and tantalum pentoxide (Ta2O5) as two dielectrics with refractive indices of 1.45 and 2.10, respectively, by electron beam evaporation to fabricate the distributed Bragg reflector (DBR). The thickness of each layer of oxide film (controlled by the thickness monitor) is λ/4n, where λ and n are the resonance wavelength of the cavity and the refractive index of the dielectric. First, a λ/4n thick (half of the total cavity thickness) SiO2 film is deposited on top of the bottom mirror, then we deposit a mechanically exfoliated monolayer of MoSe2 layer by a dry transfer technique. Subsequently, we deposit the other half of the cavity and the rest of the top mirror. A 675 nm (1.836 eV) continuous wave laser was used to excite the sample from the top mirror in a microscopy cryostat. An empty cavity was used to calibrate the charge-coupled device (CCD) pixel to sample momentum in-plane via the relation k∥︀ = k0 sin(θ). The reflectivities of the top and bottom mirrors were designed to have a slight asymmetry by choosing a different number of pairs for the top (7.5) and bottom (10.5) mirrors.
The data that support the plots within this paper and other findings of this study are available from the corresponding author upon reasonable request.
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This work was supported by NSF EFRI EFMA-1542707, NSF CAREER DMR 1553788, AFOSR FA9550-16-1-0020 and the University of Rochester University Research Award and the Leonard Mandel Faculty Fellowship in Quantum Optics. S.D. also acknowledges support from a Ramanujan Fellowship research grant, SERB, and ISIRD project SRIC, IIT Kharagpur. S.B. acknowledges the Max-Planck-Gesellschaft for funding though MPI partner group at ICTS.