Introduction

A photo-induced phase transition (PIPT), resulting from cooperative electron–lattice interactions through transiently changing the electronic states of the solid by photoexcitations1, is completely different from thermally or pressure-induced phase transitions. A PIPT not only gives access to different phases in the solid to explore anomalous properties absent in the ground-state phase2 but also enables precisely controllable phase transitions towards target structures with desired physical properties at high speeds3. Thus, the initial discovery of a PIPT in organic charge transfer crystals has triggered great interest in a variety of fields4. Compared with the vast number of materials exhibiting thermodynamic phase transitions, there are still very few solids undergoing a PIPT, and many investigations currently focus on bulk crystals possessing one-dimensional (1D) correlated electron chains in which PIPTs may be easily triggered due to inherent instabilities caused by electron–electron and electron–lattice interactions in these quasi-1D systems1,5.

As an emerging platform for PIPTs, two-dimensional (2D) and layered transition-metal ditellurides exhibit polymorphisms with distinct physical properties6,7,8. Recent experimental evidence for a PIPT in MoTe2 and WTe2 shows that structural phase transitions often involve abrupt changes in the electronic structure such as the emergence of novel topological states9,10,11. For instance, in few-layer MoTe2, an irreversible transition from a semiconducting hexagonal 2H phase to a topological distorted octahedral 1T′ phase occurs under laser irradiation, which can be used to fabricate an ohmic heterophase homojunction with accurate control of micrometer-patterning in a desired area9. The phase transition is irreversible, because the 1T′ phase formed in the electronically excited state is metastable, and to return to the ground-state 2H phase, the system has to overcome a potential barrier of around 0.71 eV12,13. The laser-induced 1T′ MoTe2 is stable for more than 1 week in ambient conditions without any protection14. Moreover, the structural distortion from the 2H to the 1T′ phase results in an intrinsic band inversion between Te p and Mo d bands15,16, enabling ultrafast manipulation of the topological character of MoTe2. The topological phase also displays gate-tunable superconductivity, providing a new potential platform to realize Majorana bound modes17,18.

Despite all this progress, the microscopic nature of the PIPT remains unclear. Triggered by external stimulation by light, the system undergoes changes in temperature, strain, electronic excitation, chemical state, and lattice vibrational modes. The transition may depend on one of these factors or on a combination of them9,19. One proposal is that Te vacancies created by irradiation trigger the local phase transition9,20,21. Other theoretical and experimental studies have argued that accumulated heat is a main driving force for the phase transition14,20. Moreover, a strain-induced phase transition has been observed in monolayer MoTe222,23; thus, laser-induced thermal strain may also contribute to the observed phase transition. Yet, another explanation is that it is the electronic excitation that plays a critical role in the phase transition12,13. Overall, the transition mechanism is still debated.

In this work, we demonstrate that the phase transition of monolayer MoTe2 can be triggered by photoexcitation of carriers alone. Using first-principles calculations, we study the excited-state properties of 2H MoTe2 at photoexcitation energies E of 1.58 eV (785 nm), 1.96 eV (633 m), 2.34 eV (532 nm), 2.42 eV (514 nm), and 2.63 eV (473 nm) by exciting all available electrons consistent with these energies. We find that a soft-mode displacive phase transition occurs for E > 1.96 eV. Photoexcitation modifies the electronic potential, resulting in a complete softening of the lattice vibrations that leads to spontaneous structural distortions with new equilibrium positions for the atoms. This structural transition takes place within one picosecond, shorter than the timescale for the photoexcited electrons to transfer their energy to the lattice. We also rule out a thermally driven or a strain-induced phase transition under laser irradiation by comparing the thermodynamic stability of 2H and 1T′ MoTe2 monolayers. Our findings not only reveal the potential origin of the PIPT in 2D transition-metal ditellurides but also provide new insight into the observed dynamic transitions in their three-dimensional (3D) counterparts, another question that remains unclear10,24,25.

Results and discussion

Lattice mode softening

We start by examining atomic displacements in the excited state to see whether (and how) a phase transition may be triggered. With D3h point group, the irreducible representations of the vibrational modes in the 2H phase at the Γ point are expressed as26

$${\Gamma }_{{\rm{2H}}}={\rm{E}}^{\prime\prime} +{{\rm{A}}}_{1}^{\prime}{\rm{+E}}^{\prime} +{{\rm{A}}}_{2}^{\prime\prime}.$$
(1)

The calculated phonon dispersion is shown in Fig. 1 and the calculated lattice mode frequencies are consistent with previous reports27,28.

Fig. 1: Lattice dynamics in the ground states.
figure 1

Phonon dispersion of 2H MoTe2 monolayer and vibrational modes for optical phonons at the Γ point. The phonon occupation number is determined from the Bose–Einstein distribution function at 300 K.

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The three modes E″, \({\rm{E}}^{\prime}\), and \({{\rm{A}}}_{2}^{\prime\prime}\) correspond to the three primary lattice distortions along the pathway from the 2H to the 1T′ phase, so could play a role in triggering the phase transition (for the three primary lattice distortions, see “Crystal Structures” in Supplementary Information). We calculate the potential energy as a function of displacement amplitude of these vibrations under different photoexcitation energies and corresponding carrier densities to investigate potential structural instabilities. The results are summarized in Fig. 2a-c, with the energy of the excited 1T′ phase set to zero for comparing the relative stability between the 2H and 1T′ phases. In the ground state, the energy of the 2H phase is 80 meV lower than that of the 1T′ phase. However, as the system is optically excited, the 2H phase becomes energetically less favorable than the 1T′ phase due to population inversion12,13.

Fig. 2: Lattice dynamics in the excited states.
figure 2

Potential energy surface at different excitation energies along the eigenvectors of (a) E″, (b) \({\rm{E}}^{\prime}\), and (c) \({{\rm{A}}}_{2}^{^{\prime\prime} }\) modes, and their corresponding structures (d–f) at the minima of the potential energy surface at 2.63 V.

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For the E″ mode (corresponding to the opposite in-plane motion of top and bottom Te layers), the Te atoms vibrate harmonically around their equilibrium positions before photoexcitation. With increasing excitation energy (and corresponding excited carrier density), the potential energy surface gradually flattens, and a double-well potential forms at E > 1.96 eV. Thus, a distorted octahedral structure can form as atoms move to new equilibrium positions (Fig. 2d). A similar situation occurs for the \({{\rm{A}}}_{2}^{^{\prime\prime} }\) mode (an out-of-plane displacement of Mo atoms and an opposite-direction displacement of Te atoms). For E > 1.96 eV, the Mo atoms can bounce up or down to the two minimum energy sites of the new double-well potential, whereas the Te atoms move in opposite directions, leading to an out-of-plane distorted variant of 2H MoTe2 (Fig. 2f). The evolution of the \({\rm{E}}^{\prime}\) mode under irradiation is slightly different. This mode is composed of in-plane displacements with the single Mo layer and the two Te layers moving opposite to each other. Increasing E lowers the energy barrier for positive displacements along the eigenvector of the \({\rm{E}}^{\prime}\) mode. The barrier becomes a deep well at 2.63 eV, leading to the atomic distortion shown in Fig. 2e, with distorted in-plane atomic positions yielding a twisted octahedral coordination around Mo atoms. It should be noted that at 2.63 eV this mode dominates, but at lower energies the potential along the \({\rm{E}}^{\prime}\) mode still exhibits a barrier, whereas both E″ and \({{\rm{A}}}_{2}^{^{\prime\prime} }\) modes show double-well potential energy surfaces, and therefore the latter two dominate in that regime. All three distortions of the corresponding mode eigenvectors are along the phase transition pathway from 2H to 1T′ MoTe2. The full transition from 2H to 1T′ MoTe2 probably occurs along a higher-dimensional path in configuration space in which photoexcitation lowers the energy barrier from 0.77 eV to 0.08 eV13, but our results suggest that the softening of these key modes can initiate the PIPT with a purely electronic mechanism.

Critical excitation energy E C

The transition from a single-well potential to a double-well potential shown in Fig. 2a–c indicates a displacive phase transition, which involves a phonon frequency that falls to zero at a critical excitation energy EC and corresponding excited carrier density. These zero-frequency soft modes drive the crystal instability along the displacements of the corresponding mode eigenvectors, leading to spontaneous symmetry breaking29,30. We examine the soft-mode behavior under optical excitation in the framework of Landau theory for the E″ and \({{\rm{A}}}_{2}^{^{\prime\prime} }\) modes that soften at lower energies. For a soft-mode displacive phase transition, the order parameter can be chosen as the amplitude of the distortion of the soft-mode eigenvector u29. The lattice potential energy, equivalent to the free energy in the Landau theory31,32, can be expressed by a fourth order even polynomial expansion of the order parameter u

$$V(u)=a+\frac{b}{2}{u}^{2}+\frac{c}{4}{u}^{4},$$
(2)

where the harmonic prefactor b is equal to the square of the soft-mode phonon frequency ω229,33. Before the phase transition, there is a single-well potential, corresponding to b > 0 (c is a small positive value with a much weaker E dependence). When b becomes negative, V(u) becomes a double-well function with minima at \(u=\pm \sqrt{-b/c}\) and a local maximum value at u = 0. Therefore, the phonon softening can be described quantitatively by calculating the phonon frequencies of the two symmetric E″ and \({{\rm{A}}}_{2}^{^{\prime\prime} }\) modes as a function of photoexcitation energy. As shown in Fig. 3a, at 1.58 eV both modes soften slightly and drop significantly at 1.96 eV. The phonon frequency becomes imaginary for E > 1.96 eV, confirming again that a soft-mode phase transition occurs at E > 1.96 eV. It should be noted that at EC = 1.96 eV, the potential energy surface of the \({\rm{E}}^{\prime}\) mode is still a single well. The energy surface in the subspace spanned by both soft modes is calculated to further evaluate the spontaneous lattice distortions. Figure 3b shows the energy surface mapped on the plane spanned by the two soft modes E″ and \({{\rm{A}}}_{2}^{^{\prime\prime} }\) at the photoexcitation energy of 2.34 eV. These results suggest that the \({{\rm{A}}}_{2}^{^{\prime\prime} }\) mode dominates the distortion; thus, the PIPT is probably triggered along that distortion.

Fig. 3: Analysis of the E″ and \({{\rm{A}}}_{2}^{^{\prime\prime} }\)modes.
figure 3

a Phonon frequency of the E″ and \({{\rm{A}}}_{2}^{^{\prime\prime} }\) modes as a function of laser excitation energy. b Energy surface in the plane spanned by the two soft modes. Each contour line represents an energy increase of 0.02 eV.

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In the Landau theory, the phase transition occurs at b = 0. For temperature-driven ferroelectric/magnetic phase transitions, b ∝ (T − T0), giving the well-known Curie–Weiss law31. In the detailed analysis of the potential well of the \({{\rm{A}}}_{2}^{^{\prime\prime} }\) mode, we find \(b\propto {({E}_{C}-E)}^{\gamma }\), where EC = 1.96 eV and γ = 0.24. As b = ω2, we fit the mode frequencies as a function of E by \(\omega \propto {({E}_{C}-E)}^{\gamma /2}\), as shown in Fig. 3a. The obtained EC = 1.96 eV is in good agreement with the change of electron distribution (Fig. 4b), from which one can see that the electron localization function also changes completely by E ≥ 1.96 eV. A similar EC is also predicted for the E″ mode in Fig. 3a. Thus, our results suggest that the lattice distortions occur spontaneously after photoexcitation. Our prediction of photo-induced lattice mode softenings, marked by clear changes in both Raman and infrared spectra (E″ is Raman active and \({{\rm{A}}}_{2}^{^{\prime\prime} }\) is infrared active), can be verified experimentally by ultrafast coherent phonon spectroscopy24 or second harmonic generation34.

Fig. 4: Microscopic mechanism for PIPT.
figure 4

a 3D and b top view (Mo layer) of the electron localization function of 2H MoTe2 at different excitation energies. The electron localization function from 0 to 1 is shown by colors from navy to red. The isosurface for the electron localization function in a is 0.2. Static lattice DOS (gray) compared with the DOS along the eigenvector of the (c) E″ (green) and (d) \({{\rm{A}}}_{2}^{^{\prime\prime} }\) (pink) phonon modes, with the displacement amplitudes corresponding to the potential minimum at 2.34 eV.

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For a thermally induced phase transition, \(b=\tilde{b}(T-{T}_{0})\), where \(\tilde{b}\) is a positive constant29, the potential well changes gradually with temperature towards the phase transition. In contrast, in a PIPT, the potential well change is determined by the number of excited carriers, which is related to the excitation energy E and the density of states (DOS). For instance, when E is only slightly larger than the band gap, few electrons are excited to the conduction bands, leading to a negligible change of the potential well. Thus, in the PIPT, b has a much weaker E dependence than the T dependence in a thermally induced phase transition, leading to a much smaller γ.

Photo-induced changes in the electronic state

We next investigate the electronic state to rationalize the phonon softening upon photoexcitation discussed above. When a solid undergoes a structural phase transition, the ionic positions change because the symmetry of the electronic potential changes35. Light-induced electronic excitations in the 2H lattice may be responsible for such a change in the electronic potential. Figure 4a shows the 3D electron localization function of 2H MoTe2 at different photoexcitation energies. As shown in Fig. 4b, the electron distribution around Mo atoms changes from isolated triangles (dashed red line) at 0 eV to connected hexagons (dashed red line) at 1.58 eV. As the excitation energy increases further to 1.96 eV, the electrons in the Mo layer gather between top and bottom Te atoms, and the in-plane triangles around Mo atoms appear once again, but with a reversed orientation compared with the ground state, indicating an electronic potential change. As the excitation energy increases to 2.34 eV, the inverted-triangle region of the electron density shrinks.

Figure 4c, d show a comparison of the DOS calculated for the static lattice and for the lattice distorted along the E″ and \({{\rm{A}}}_{2}^{^{\prime\prime} }\) phonon modes, with the displacement amplitudes corresponding to the potential minimum at 2.34 eV. As expected from the discussion in Figs. 2 and 3, the \({{\rm{A}}}_{2}^{^{\prime\prime} }\) mode distortion leads to a larger change in the DOS: there is a significant redistribution of DOSs in the conduction band towards lower energies. A similar picture emerges for the E″ mode, but in that case the changes are small. In the ground state the conduction band is empty and therefore a redistribution of the DOSs towards lower energies does not affect the total energy of the system. However, upon photoexcitation, the conduction bands become occupied and it then becomes energetically favorable to undergo a lattice distortion to red shift the conduction bands and lower the overall energy of the system. This is analogous to the Peierls mechanism and provides a microscopic picture for the driving force behind the mode softening induced by photoexcitation. We note that the DOS around the valence band maximum also changes, and when those states are occupied in the ground state, the distortion leads to an energy increase as expected. However, under photoexcitation those states are unoccupied (holes), and the DOS redistribution has a minor effect on the total energy.

Excited carrier concentrations

As discussed above, for a given photoexcitation energy we consider that the number of incoming photons is as large as necessary to excite all available electrons that can be excited at the given laser energy. Therefore, the excited carrier concentration becomes a function of the excitation energy. Table 1 shows the excited carrier concentrations n under different excitation energies. The excited carrier density at 1.96 eV is 3.4 × 1014 cm−2, corresponding to an excited carrier density of 2.9%. We also estimate the maximum amount of electron-hole pairs generated by a femtosecond laser with a fluence of 100 mJ/cm2 assuming that no saturation occurs (for the calculations of the maximum amount of electron-hole pairs, see “Within 20 fs of Laser Excitation” in Supplementary Information). At 1.96 eV, excitation of up to 10.2% is possible for a laser pulse with a fluence of 100 mJ/cm2 (see Table 1) and thus the excited carrier concentrations in our calculations are experimentally accessible. As a PIPT can take place for excitations over 2.9%, a laser pulse with a minimum fluence of 28 mJ/cm2 is needed to induce a phase transition at 1.96 eV. This is consistent with the experimental fact that with insufficient laser fluence, the phase transformation cannot take place even for long irradiation times9,14.

Table 1 Excited carrier concentration n and the maximum amount of excitation N.
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The excited carrier population is related to the DOS36. Optical transitions are dominated by peaks in the DOS, and the dominant peaks in MoTe2 are marked by arrows in Fig. 5c, where the optical transitions correspond to the excitation energies of 2.52, 2.74, and 2.96 eV. In 2D materials, reduced electronic screening typically leads to strong excitonic effect. The Coulomb interaction of excited electrons and holes redistributes oscillator strength, giving rise to tightly bound excitons with eigenvalues lower than the band gap. By including electron-hole interactions, the optical transition energies between the DOS peaks are reduced to 2.22, 2.45, and 2.68 eV (shown in parentheses in Fig. 5c). With laser energies larger than 2.22 eV, the concentrations of excited carriers become higher, corresponding to strong optical excitation.

Fig. 5: Electronic properties of 2H MoTe2.
figure 5

a Electronic structures, b quasiparticle relaxation time, and c DOS of monolayer MoTe2. The red circles in a denote the first exciton. The radius of circles represents the electron-hole coupling coefficient of excitonic wave functions. The larger the radius, the more an electron-hole pair contributes to the exciton eigenstate. The arrows in c indicate optical transitions with different electronic excitation energies. The parentheses in c show the exciton excitation energies.

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Timescale of the phase transition

The timescale after laser excitation is divided into three regimes: (1) excited electrons thermalization (in 20 fs), (2) soft-mode phase transition (117–292 fs), and (3) lattice heating (within hundreds of ps).

In the first stage, the temperature of the electronic system increases by photoexcitation and the excited electrons thermalize within 20 fs at a high electronic temperature, whereas the lattice remains cold. In photoexcited MoTe2, carrier-carrier scattering is responsible for redistributing carrier energy, resulting in a thermalized distribution function of carriers37. The carrier relaxation time can be calculated from the quasiparticle self-energy38,39. The excited electrons thermalize in 20 fs (Fig. 5b), whereas the electron-hole recombination occurs on the order of picoseconds (see “Within 20 fs of Laser Excitation” in Supplementary Information). Thus, all the excited electrons are in thermal equilibrium before recombining or interacting with phonons.

In the second stage, the symmetry breaking displacements in 2H MoTe2 take place within 292 fs. As the laser pulse creates electronic excitations, the new potential energy surfaces in Fig. 2a–c are formed immediately. The photo-induced lattice distortions, as a result of phonon softening, occur within the timescale of lattice vibrations. This can be estimated by the lattice vibration periods from 117 fs (\({{\rm{A}}}_{2}^{^{\prime\prime} }\) mode) to 292 fs (E″ mode). Such an estimate agrees well with previous molecular dynamics simulations12 and pump-probe spectroscopy24. The structural distortion can take place before the electrons transfer their energy to the lattice by carrier-phonon interaction (1– 100 ps37).

In the third stage, the hot carriers are cooled by transferring energy to the lattice, converting electronic photoexcitation energy to heat in hundreds of picoseconds through interaction with various phonons.

Competing mechanisms

One proposed mechanism for the PIPT in MoTe2 is that after the excited electrons transfer their energy to the lattice through electron–phonon coupling, atomic reorganization toward the 1T′ phase may occur as a result of local heat20 or thermal strain22,23. We next demonstrate that these thermal effects alone cannot trigger the phase transition.

As the thermalized electronic system transfers its energy to the lattice, local heat is generated. The estimated local temperature during the laser irradiation is 670 K9. As the temperature increases, the phonons in the 1T′ MoTe2 phase are more highly excited than the phonons in the 2H MoTe2 phase, because the 1T′ phase has more low-energy phonons than the 2H phase (Fig. 6a). Thus, the entropy of the 1T′ phase becomes higher than that of the 2H phase as temperature increases (the entropy increases with the occupancy). It is thereby possible for the 2H structure to transform into 1T′ MoTe2.

Fig. 6: Thermodynamic stability of 2H and 1T′ MoTe2 monolayers.
figure 6

a Phonon dispersion of 1T′ MoTe2 monolayer. The phonon occupation number is determined from the Bose–Einstein distribution function at 300 K. b Helmholtz free energy difference between 2H and 1T′ MoTe2 monolayers as a function of temperature with and without thermal strain.

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Thermodynamic stability at finite temperature can be described by the difference in Helmholtz free energy40,41,42 (for the calculations of thermodynamic stability, see “Thermal Effects (about hundreds of ps)” in Supplementary Information). At 0 K, the free energy difference between the 2H phase and the 1T′ phase is just 72 meV per rectangular unit cell, indicating that the stability of the 1T′ phase is quite close to that of the 2H phase. As shown by the blue curve in Fig. 6b, at temperatures higher than 930 K, 1T′ MoTe2 becomes thermodynamically more stable than 2H MoTe2. This is consistent with the fact that the pure 1T′ phase appears in a temperature range between 930 K (for Te deficiency) and 1170 K (for Te excess)43. However, the temperature to facilitate the phase transition, 930 K, is significantly higher than the laser-induced temperature of 670 K9. Even after taking thermal strain into consideration [red curve in Fig. 6(b)], the phase transition temperature of 810 K is still higher than the laser-induced temperature (for the role of thermal strain, see “Thermal Effects (about hundreds of ps)” in Supplementary Information). Therefore, the laser-induced thermal effect on the phase transition has probably been overestimated in earlier studies9,20.

In fact, previous experiments have suggested that the heating effect alone cannot induce the structural transformation14. For pure 2H MoTe2, no significant change occurs after annealing, whereas laser irradiation leads to a mixed 2H + 1T′ phase. In the laser-irradiated mixed phase, the 2H phase disappears completely after annealing, leaving a pure 1T′ crystal14. Therefore, electronic excitation may drive spontaneous lattice distortions, whereas the heating effect accelerates the phase transition via thermal displacements, in which the intermediate states decay to the 1T′ phase (for the role of thermal displacement, see “Thermal Effects (about hundreds of ps)” in Supplementary Information).

Another proposed mechanism for the PIPT in MoTe2 is that laser irradiation can create Te vacancies, which can trigger a local phase transition9,20,21. Consistent with this picture, a recent study has demonstrated that the phase transition involves a set of successive dynamics such as Te vacancy diffusion and ordering to generate the 1T′ phase44, which is similar to the Ge-Sb-Te phase-change memory materials45. A vacancy-induced phase transition is related to a change in chemical composition, which is analogous to the composition-dependent phase transition in Mo1−xWxTe246. We emphasize that our work demonstrates that a phase transition can occur even in the absence of Te vacancies, and instead be driven by photoexcited carriers alone. Indeed, a recent experimental study has reported an electric-field induced structural transition in 2H MoTe28, supporting our conclusion that changes in electron density alone can induce a phase transition without the need for Te vacancies. Similar photo-induced transitions have recently been predicted in the perovskites BaTiO3 and PbTiO347.

In summary, we demonstrate that a sub-picosecond phase transition in monolayer MoTe2 from the 2H phase to a distorted 1T′ phase can be triggered by purely electronic excitation, even when the lattice is still cold. Such electronic excitation changes the electron density, resulting in a soft-mode displacive phase transition. The phase transition from the 2H phase to the 1T′ phase can be induced by a critical excitation energy of 1.96 eV, at which 2.9% of the carriers are excited. We also show that this phase transition mechanism can be understood in the frame of Landau theory and is quite different from a temperature-driven phase transition. The microscopic picture of the phase transition is analogous to a Peierls distortion, with a red shift of the conduction bands that are occupied upon photoexcitation that lowers the overall energy of the system. Our findings shed new light on the microscopic origin of PIPT in 2D transition-metal ditellurides and are expected to motivate both fundamental and applied studies of ultrafast phase transitions in these new class of materials for topological switching and neuromorphic computing.

Methods

All calculations are performed based on density functional theory (DFT) using the Vienna ab-initio simulation package48. The exchange-correlation energy is calculated within the generalized gradient approximation in the Perdew–Burke–Ernzerhof (PBE) parameterization49. In the excited state simulations, we mimick optical excitation by promoting valence electrons from high-lying valence band states to low-lying conduction band states. This method, typically called Δ self-consistent field50,51,52, introduces noninteracting electron-hole pairs by changing the occupation numbers of the Kohn-Sham orbitals and is less computationally demanding than more advanced approaches such as constrained DFT53 and excited-state force calculations within GW + BSE54 but has been successfully used in studying PIPTs12,55,56. The occupied conduction band is determined by energy conservation at photoexcitation energies E of 1.58 eV (785 nm), 1.96 eV (633 nm), 2.34 eV (532 nm), 2.42 eV (514 nm), and 2.63 eV (473 nm) (see “Computational Details” in Supplementary Information). We choose these laser excitation energies, because the corresponding wavelengths are experimentally feasible. We keep these occupancies fixed throughout the calculations. This scenario corresponds to the time domain of interest, namely, after the laser-excited carriers populate the states near the band edges but before these carriers relax to the band edges via electron–phonon interactions. Electron-hole recombination occurs on the picoseconds timescale, which is much larger than a single phonon period and therefore the number of excited electrons can be reasonably assumed to remain constant as in the calculation. It should be noted that, for simplicity, we use the PBE band structures to determine the number of the excited electrons under optical excitation. The GW0 band structure correction is an almost rigid upshift of the PBE conduction bands of 0.69 eV, and after a simple scissor shift, the required laser excitation energies are still experimentally feasible. In subsequent work, it would be interesting to see how bound excitations (excitons) modify the picture.