Abstract
The demand for disordertolerant quantum logic and spin electronics can be met by generating and controlling dissipationless spin currents protected by topology. Dirac fermions with helical spinlocking surface transport offer a way of achieving such a goal. Yet, surfacebulk coupling can lead to strong Dirac electron scattering with bulk carriers and phonons as well as impurities, assisted by such dissipative channel, which results in “topological breakdown”. Here, we demonstrate that coherent lattice vibrations periodically driven by a singlecycle terahertz (THz) pulse can significantly suppress such dissipative channel in topological insulators. This is achieved by reducing the phase space in the bulk available for Dirac fermion scattering into during coherent lattice oscillations in Bi_{2}Se_{3}. This lightinduced suppression manifests as a remarkable transition exclusively in surface transport, absent for bulk, above the THz electric fields for driving coherent phonons, which prolongs the surface transport lifetime. These results, together with simulations, identify the critical role of spin–orbit coupling for the “phase space contraction” mechanism that suppresses the surfacebulk coupling. Imposing vibrational quantum coherence into topological states of matter may become a universal light control principle for reinforcing the symmetryprotected helical transport.
Introduction
Recently, there is increasing evidence that coherently driven states can protect and enhance the stability of quantum systems. A pedagogical example for such dynamic stabilization is the periodically driven Kapitza pendulum^{1} where an inverted, yet stable, orientation can be achieved by a sufficiently high frequency vibration of its pivotal point. Applied to topological protected states (TPS), such as those realized in topological insulators (TIs),^{2,3,4,5,6,7} coherent lattice vibrations can have direct and profound effects on surface transport of Dirac fermions, via periodic modulation of electronic states, as illustrated in Fig. 1a. This effect of coherent phonons is in stark contrast to that of incoherent phonons from thermal excitations, which diminishes topological enhancement of surface transport via random lattice scattering, heating, surfacebulk charge transfer and coupling. Ultrafast phononics has been explored as a new avenue to manipulate properties of superconductors,^{8} oxides,^{9,10} semimetal^{11} and photovoltaic semiconductors.^{12} Although experimental realizations of coherent phonon generation have been explored in TIs,^{7,13,14} the influence of such vibrational coherence on the surface helical transport has not been observed until now.
The prototype TI, such as Bi_{2}Se_{3} exhibits surface charge transport protected by spinmomentum locking, where the spin–orbit interaction connects the direction of the carrier spin to that of its momentum.^{4,15,16,17} This spinlocking gives rise to coherent transport that manifests as, e.g., lack of current relaxation and prolonged transport lifetime, which is protected against nonmagnetic disorder by symmetry. Here, we explore a nonequilibrium driven TPS, periodically modulated by coherent phonons induced by a noncontact THz push electric field, as a new control knob for further protecting surface carriers from scattering with residual bulk states and/or thermal phonons. Such THz photon driven coherence mechanism complements the spontaneous symmetry protection mechanism in the ground state. However, its observation requires intense THz pump and THz conductivity probe spectroscopy measurements^{18,19,20,21,22} of the coherent phonondressed TPS, which has never been demonstrated so far.
In this article, we create a periodically driven topologically protected state via coherent lattice vibrations that significantly suppress the surfacebulk coupling in Bi_{2}Se_{3}. We demonstrate two regimes of postTHzpump nonequilibrium states, obtained by tuning E_{THz}. In this way we show evidence of nonthermal quantum control of the Dirac fermion transport lifetime τ_{Dirac}, by inducing a transition from incoherent carrier heating to a coherent driving regime. This transition exclusively appears in surface transport and is absent in bulk. It occurs above electric field strengths required for observing coherent phonon oscillations. Together with theoretical simulations, our results reveal a “phase space contraction” mechanism assisted by spin–orbit coupling that is responsible for coherent phononenabled suppression of the surfacebulk coupling in dressed topological states out of equilibrium.
Results
We apply a singlecycle THz pulse E_{THz} with amplitude up to ~500 kV cm^{−1}, which selectively excites coherent oscillations of \({E}_{u}^{1}\) phonons, shown in Fig. 1b. For E_{THz} = 0, the real part of the static conductivity, σ_{1}(ω), at the ground state shows a Drude lineshape superimposed to a welldefined oscillator feature centered at ~8 meV as shown in Fig. 1c. This lineshape has been established as arising from joint carrier conductivity responses from both bulk and surface states plus a \({E}_{u}^{1}\) phonon mode, consistent with prior THz electrodynamic studies of Bi_{2}Se_{3}.^{23} For THz excited states, i.e., E_{THz} ≠ 0, the spectraltemporal characteristics of the complex conductivity response functions are measured by our THz pump–THz probe conductivity spectroscopy that allows us to differentiate surface from bulk contributions as shown in ref. ^{23}. In this way we measure the transport lifetimes of Dirac currents, τ_{Dirac}, and bulk ones, τ_{Bulk}, which reveals the interaction between topological states and bulk coherent phonons.
We study 50 quintuple layers of ntype Bi_{2}Se_{3} with bulk insulating bandgap ~310 meV and Fermi energy ~60 meV above the conduction band edge. This Bi_{2}Se_{3} film is grown by molecular beam epitaxy on top of a 0.5 mm thick sapphire substrate with caxis perpendicular to surface. The sample is cooled down to 5 K in a He flow cryostat in order to maximize the surface responses by reducing thermal phonons.
Figure 1d shows phonon emission after THz pump at 5 K as a function of electric field E_{THz}, up to ~500 kV cm^{−1}. The broadband THz pulses used here are centered at ω_{pump} ~ 4 meV (Fig. 1c) and can excite the \({E}_{u}^{1}\) phonon mode. Interestingly, the phonon emission clearly shows a pronounced multicycle oscillation for high driving fields ~180 kV cm^{−1}. The Fourier transform (FT) spectra of these coherent oscillations displays a resonant peak centered at ~8 meV, which is consistent with the \({E}_{u}^{1}\) phonon mode (inset, Fig. 1e). The integrated spectral weight (SW) clearly shows a “thresholdlike” buildup at E_{THz} ~ 180 kV cm^{−1} (Fig. 1e). Below E_{th} ~180 kV cm^{−1}, the coherent phonon THz emission SW is vanishingly small. This nonlinear emergence of the coherent phonon oscillations is most likely due to the multiphoton excitation of coherent \({E}_{u}^{1}\) phonons ~8 meV. The THz pump spectra is broad, from 2 to 6 meV with center ~4 meV (Fig. 1c). Therefore, the excitation will be a combination of multiple processes that mainly include two and threephoton nonlinear processes. This is consistent with the fitted data (Supplementary Note 6), which shows a power law with exponent ~2.7 in the Efield dependence. Most intriguingly, this transition in lattice displacement driven outofequilibrium distinguishes two different THz pumping regimes controlled by the THz electric field: (1) weak pumping can mainly excite incoherent phonons, averaging to zero lattice movement, and mainly accesses a lattice heating regime; (2) intense THz driving allows the establishment of a macroscopic lattice vibration and accesses a periodically driven TPS. The latter regime gives rise to the observed THz radiation, as shown in Fig. 1d. Note that THz pulses will also excite charge carriers by intraband transitions at surface and bulk because of finite doping.
We characterize the ultrafast THz conductivity by measuring the THz fields in the time domain, shown in the inset of Fig. 2a, b. In the inset, we show E(t) after transmission through (i) a reference substrate, E_{ref}(t) (gray) and (ii) the unexcited sample, E_{Sample}(t) (blue). We also compare the above to the pumpinduced change ΔE(t) after pump–probe delay Δt_{pp} = 0.5 ps (red, inset). Using FT and Fresnel equations, the full THz dielectric response is obtained and expressed as the real parts of the conductivity, Δσ_{1}(ω), Fig. 2a, and the dielectric function, Δε_{1}(ω), Fig. 2b. These response functions characterize the change in transport properties of surface Dirac electrons and bulk carriers following THz driving. We observe a clear bipolar frequencydependence of Δσ_{1}(ω), with transition from strong bleaching (Δσ_{1} < 0) to enhanced absorption (Δσ_{1} > 0) for frequencies between 2 and 10 meV. We also observe a decrease of Δε_{1} with increasing probe frequency in the same range. In our previous study of intraband photoexcitation responses in Bi_{2}Se_{3}, mainly using midinfrared pulses,^{23} we identified a similar bipolar spectral shape of Δσ_{1}(ω) dynamics, which arises from the combined responses due to competing surface and bulk states. There we showed that the above behavior can be used to distinguish the intrinsic transport properties of Dirac fermions and bulk electrons. The lineshape can also be explained by quantitative simulation as applied below.
The observed spectral lineshapes as a function of pumpprobe time delay can be fitted by using a composite model with two Drude terms and one Lorentz oscillator. These three contributions account for the THz response functions of surface and bulk carriers and phonons, respectively
where ε_{∞} is the background electrical permittivity. The plasma frequencies \({\omega }_{\,\text{p}\,}^{2}=n{e}^{2}/{\varepsilon }_{0}{m}^{* }\) are proportional to the densities of surface (n_{S}) and bulk (n_{B}) free carriers. The subscripts j = S and B in the equation stand for surface and bulk states, respectively. ω, e, and ε_{0} denote the frequency, electron charge, and vacuum electrical permittivity, respectively. m* and γ are the effective mass and scattering rates of surface or bulk carriers. The THz response functions measured in the experiment are well reproduced for all time delays by varying the surface and bulk scattering rates γ_{j}, the phonon oscillator strength F, and the phonon damping coefficient Γ. At the same time, we keep the surface and bulk carrier densities fixed, consistent with a physical picture of subgap photoexcitation that is decoupled from interband transitions.^{23} A unique set of model parameters is obtained by simultaneously fitting conductivity and permittivity in the measured broad frequency range. By only varying the surface τ_{S} and bulk τ_{B} scattering times (i.e., 1/γ), we are able to consistently reproduce the timedependent experimental results, as shown in Fig. 2a, b, and extract the Dirac (purple line) and bulk (green line) transport properties. This fitting implies that the THz pumping used here gives rise to much smaller changes of surface and bulk quasiparticle densities as compared to the scattering time changes, unlike for high frequency pumping as discussed in ref. ^{23}. We can thus separate the intrinsic surface and bulk transport properties in both time and frequency domains.
The distinct spectraltemporal characteristics observed here can be used to characterize how THz driving influences carrier transport. In Fig. 2c–f, complete 2D false color plots of Δσ_{1} and Δε_{1} spectra are presented as a function of THz pump electric field E_{THz} up to 500 kV cm^{−1}, at short pump–probe delay t_{pp} = 0.5 ps after excitation. The pumpinduced THz conductivity spectra Δσ_{1}(ω) exhibit a bipolar behavior, demonstrated by the two THz fieldcut spectra in Fig. 2c taken at the black dashed lines in Fig. 2d. We observe a pump fielddependent nonlinear negative growth and then decay of Δσ_{1}(ω) at 5 K. As shown in Fig. 2, the low frequency negative signals from 2 to 4 meV become dominant for driving fields above ~180 kV cm^{−1} and then progressively decrease with increasing THz pump field. To analyze this behavior, we fit the 2D THz response functions Δσ_{1}(ω) and Δε_{1}(ω) shown in Fig. 2d, f by using the composite model discussed above. Excellent agreement between this model and the measured transient THz response is achieved for all THz pump fluences, similar to the exemplary fitting in Fig. 2a, b. As we discuss next, these results indicate that the transport properties of Dirac fermions arise from two competing effects: coherent phonon periodic modulation and incoherent phonon heating of the Fermi sea.
Figure 3a compares the THz driving field (E_{THz}) dependence of the transport lifetimes of the surface, τ_{S}, and bulk, τ_{B}, electrons extracted from Fig. 2d, f. It shows a clear correlation with the amplitude of coherent phonon emission. τ_{S} undergoes a clear transition at ~180 kV cm^{−1} and saturates at 400 kV cm^{−1}. Below ~180 kV cm^{−1}, there is a reduction in τ_{S} with increasing field, marked by the black dashed line, which we assign to increased surface electron scattering due to THz heating of the Fermi sea and incoherent thermal phonons. Above ~180 kV cm^{−1}, this reduction in τ_{S} clearly slows down, which indicates suppression of Dirac fermion scattering compared to what is expected for thermal effects. The observation of a clear transition between two excitation regimes indicates the emergence of additional protection absent in the ground state. This stops further suppression of τ_{S} even with increasing THz field pumping, which finally saturates at the highest THz field used. The most salient feature is the coincidence between the transition field observed in the Dirac fermion transport lifetime changes and the nonlinear threshold for emergence of coherent phonon oscillations at E_{th}. This coincidence suggests a strong correlation between the two phenomena, i.e, the emergence of prolonged, new nonequilibrium transport lifetimes when the THz field drives ordered lattice positions via coherent phonon oscillations, instead of disordered lattice positions due to thermal fluctuations. At the same time, the THz pump field dependence of the bulk transport lifetime τ_{B} (inset, Fig. 3a) does not show any transition across E_{th} (Fig. 3b). Instead, τ_{B} displays an opposite field dependence, i.e., an increase in τ_{B} at low pump fields followed by a decrease at high pump fields. This behavior can be understood as a transition from impurity to phonondominated scattering with increasing THz pumping, which is consistent with conventional behaviors seen in the temperature dependence of bulk carrier scattering in a doped semiconductor.^{24,25} Figure 3c illustrates our interpretation of these experimental observations as signatures of suppression of the surfacebulk coupling by THz driving, which leads to a nonequilibrium topological state protected and stabilized further by a new dynamic channel from coherent phonon excitations.
Discussion
To explore how coherent lattice displacements driven by E_{THz} influence the topological electronic state, we use firstprinciples calculations in combination with a microscopic theory of surfacebulk coupling as discussed in details in the Supplementary Note 3. Bi_{2}Se_{3} has a rhombohedral structure (space group R3m) with five atoms in the primitive unit cell (Fig. 4a). These atoms are arranged in a quintuple layered structure, with each layer consisting of five planes of Se2–Bi–Se1–Bi–Se2, with lattice parameters a = 4.142 Å and c = 28.635 Å. The details of our firstprinciples calculation are discussed in the Supplementary Notes 3 and 4. The most important scattering mechanisms of the surface electrons in Bi_{2}Se_{3} at low temperature are electron–electron (e–e) and electron–impurity (e–imp) scattering. On the one hand, the e–e scattering rate Γ_{e−e} for normal Fermiliquids is proportional to T^{2}. In our THz pump experiment, the surface electronic temperature increases due to intraband scattering after THz excitation, therefore we expect that \({\Gamma }_{ee}\propto {({E}_{\text{THz}})}^{4}\) leads to reduced carrier transport lifetimes when heating dominates. On the other hand, the e–imp scattering in the surface is weakly temperaturedependent. Next we explore how the e–imp scattering, assisted by surfacebulk coupling, can be reduced nonthermally by intense THz driving of coherent phonons that will compete with Γ_{e−e} above the threshold as demonstrated in Fig. 3a.
The e–imp scattering can proceed via surface–surface (SS) and surface–bulk (SB) channels, whose contribution depends on the available final states, i.e., the surface electron may scatter to either surface or bulk states. According to the microscopic theory of impurity and phononinduced SB coupling in TIs,^{26} in ndoped Bi_{2}Se_{3} samples with Fermi level at ~60 meV above the conduction band minimum (CBM) similar to ours, the SB scattering channel dominates over the SS one. The SB impurity scattering rate is shown to be proportional to the bulk density of states (DOS) at the Fermi level and is also sensitive to the relative orientation of the surface and bulk orbital pseudospin 〈τ^{z}〉.^{26} Using a model Hamiltonian derived to describe the lowenergy electronic structure of Bi_{2}Se_{3} up to O(k^{2}),^{27} we computed the low energy electronic bands and corresponding surface and bulk expectation values of the orbital pseudospin 〈τ^{z}〉. The results are plotted in Fig. 4b. It can be seen that, at 60 meV above the CBM, the surface and bulk states have parallel orbital pseudospin orientation. Thereby, the SB scattering rate is enhanced and dominates over other channels, consistent with ref. ^{26}. Since \( {\langle {\tau }^{z}\rangle }_{\text{S}} \le 1\), \( {\langle {\tau }^{z}\rangle }_{\text{B}} \simeq 1\), the SB scattering rate of the surface electron at the Fermi level near the conduction band edge takes the following simplified form^{26} (Supplementary Note 4)
where the summation includes all bulk bands \({\alpha }^{\prime}\). \({g}_{\alpha ^{\prime} }^{\,\text{imp}\,}\) is proportional to the effective electron–impurity coupling and is dependent on the overlap between the surface and the \({\alpha }^{\prime}\) bulk band wavefunctions. \({v}_{\alpha ^{\prime} }({E}_{\text{F}})\) is the DOS of the bulk band \(\alpha ^{\prime}\) at the Fermi level. The SB scattering rate \({\Gamma }_{\,\text{SB}}^{\text{imp}\,}\) is therefore proportional to the bulk DOS at the Fermi level.
Next we analyze the variation of the bulk DOS at the Fermi level, \({v}_{\alpha ^{\prime} }({E}_{\text{F}})\), during the lattice vibration under the \({E}_{u}^{1}\) mode. To determine the lattice dynamics, we calculate the phonon properties with a supercell approach and harmonic approximation using the Phonopy code.^{28} In the calculations, a supercell containing 135 atoms, i.e., 3 × 3 × 3 of the primitive unit cell, and a kpoint grid of 2 × 2 × 2 are used. The force constants are computed without and with spin–orbit coupling (SOC) using the VASP code.^{29,30} Our results show that the frequency of the \({E}_{u}^{1}\) mode is 2.57 THz from the GGA calculation, while the GGA + SOC calculation gives 2.30 THz, closer to the experimental measurement (~2.0 THz). The directions of the lattice vibrations under the \({E}_{u}^{1}\) modes are schematically plotted in Fig. 4c, where the two inequivalent \({E}_{u}^{1}\) modes are illustrated from different views. Note that a hexagonal plane is used to represent all atoms in the quintuple layer without losing generality. The atomic displacement of each layer is determined to be r = (−0.30, 0.40, −0.70, 0.40, −0.30) Å in the GGA calculation and r = (−0.31, 0.44, −0.65, 0.44, −0.31) Å in the GGA + SOC calculation, which allows us to track the atomic positions in each plane of the quintuple layer during the harmonic vibration of lattice. Subsequently, the electronic properties are calculated for each snapshot captured during the \({E}_{u}^{1}\) lattice vibration under the Born–Oppenheimer approximation. Further details are outlined in the Supplementary Notes 3 and 4 and the main results are shown in Fig. 4d, e. Here, the bulk DOS at the Fermi level \({v}_{\alpha ^{\prime} }\)(E_{F}) is plotted as a function of the lattice vibration amplitude (in units of r) from GGA and GGA + SOC calculations, respectively, i.e., without (Fig. 4d) and with SOC (Fig. 4e). We note that the results obtained for the two inequivalent \({E}_{u}^{1}\) modes are not the same, thus an average curve is also computed and plotted in Fig. 4d, e (black solid circles).
The DOS dependence on phonon amplitude is markedly different with or without SOC, which identifies its critical role for determining the phase space available for the SB scattering rate \({\Gamma }_{\,\text{SB}}^{\text{imp}\,}\). Figure 4d shows that \({v}_{\alpha ^{\prime} }\)(E_{F}) gradually increases in the regular GGA calculations without SOC, which implies increased Dirac electron scattering. In contrast, the calculations in Fig. 4e with SOC show that \({v}_{\alpha ^{\prime} }\)(E_{F}) rapidly decreases for initial decrease of lattice vibrations (<0.2 Å from the equilibrium position), and then slowly increases and saturates. The Dirac fermionimpurity scattering rate \({\Gamma }_{\,\text{SB}}^{\text{imp}\,}\), Eq. (2), changes similarly to \({v}_{\alpha ^{\prime} }\) (E_{F}) as a function of the lattice vibration amplitude, which is proportional to the THz pump field. The simulated behavior clearly explains the slow down in τ_{S} decrease with this new surface protection channel against bulk scattering and saturation at the highest THz field used (Fig. 3a). Therefore, the good agreement between the calculated results when SOC is included and the experimental observations clearly underpins the importance of spin–orbit coupling for the “phase space contraction” mechanism that suppresses the surfacebulk coupling in Bi_{2}Se_{3} during coherent phonon oscillations. Note that the observed nonequilibrium τ_{S} in Fig. 3a (black circles) is always smaller than the unexcited one mainly due to the unavoidable heating of bulk Fermi sea in highly doped samples like ours. However, the “phase space contraction” mechanism demonstrated in Fig. 4 indicates that further increase in τ_{S} can be achieved, e.g., in samples with the doping below the bulk band edge to remove heating effects of bulk carriers. Our data for the bulk conducting state clearly shows the roadmap and it will be interesting to extend the demonstrated coherentdriving scheme to bulk insulating samples and other systems including semimetals and semiconductors to increase coherent transport.^{11,12,31}
We expect two major changes with elevated temperature: (1) decrease of coherent phonon amplitude for the same pump field and (2) much stronger surfacebulk coupling, assisted by the population of incoherent phonons. Figure 5 shows these expected behaviors. First, Fig. 5a, b compare THz pumpinduced phonon emission at 5 and 300 K for two selected pump fields, above and below E_{th} ~180 kV cm^{−1}. One clearly sees coherent phonon oscillation at low temperature above E_{th}, as discussed above. In contrast, the phonon oscillation strength is significantly suppressed at high temperature, due in part to enhanced scattering and thermal population. This result is consistent with our conclusion that the incoherent phonons dominate the THzdriven state at high temperature, unlike for low temperature. This interpretation naturally leads to the conclusion that strong surfacebulk coupling and charge transfer exist at high temperatures as discussed next. Second, THz spectra of Δσ_{1}(ω) and Δε_{1}(ω) measured at 300 K (red circles) are shown in Fig. 5c, d, which could not be fitted with our composite model (green solid lines) consisting of two Drude contributions with only the scattering rate changes. This is in contrast to the 5 K data, which are fitted very well with the proposed model. This clearly shows that surface and bulk are strongly coupled by the incoherent phonon with charge transfer in this high temperature case,^{32} which can only be accounted beyond a linear combination of their individual responses.
There are distinguishing features and robust analysis that show the presence of two transport channels, i.e., both surface and bulk, and reliably determine their transport lifetimes, as shown in Fig. 3a. We have addressed them extensively in our prior THz conductivity study using ultrabroadband, wavelengthselective pumping that extends from midIR to nearIR and visible.^{23} Applied to the THz pump data, for example, one distinguishing feature is the observation of frequencydependent cooling times that directly distinguish the faster surface channel from the slower bulk one as shown in the Supplementary Note 5. This cannot be explained by a single state with fixed carrier density. The only physical picture that one can propose to consistently explain this unusual behavior is that there are two relaxation channels, i.e., surface and bulk, with different cooling times.^{23}
In summery, intense THzdriven coherent phonon modulations provide a previously inaccessible tuning knob for suppressing surfacebulk scattering channels. Our results provide compelling implications of exploring “phononic engineering” of phase space, by modulation of electronic DOS, toward achieving persistent coherent transport in topological device applications.
Methods
Experimental schemes
Broadband quasisinglecycle THz pulses were generated by optical rectification in a MgOdoped LiNbO_{3} crystal using the tilted pulse front method. The crystal was pumped by 2 W and 35 fs pulses from a Ti:Sapphire based regenerative amplifier with a 1 kHz repetition rate. A portion of the amplifier beam was used to generate THz probe pulses via optical rectification in a 110cut 1 mm ZnTe crystal. The probe THz waveforms were measured using electrooptic sampling in another 110cut 1 mm ZnTe crystal. The pump THz electric field was varied using three wiregrid polarizers placed in the THz beam path. The pump THz and probe THz spot sizes were 1.2 and 0.8 mm, respectively. A 2 mm aperture was placed in front of the sample to ensure uniform illumination of the probed area. The sample was mounted in an optical cryostat along with a bare substrate which served as a reference. More information can be found in Supplementary Note 1.
Sample preparation
The Bi_{2}Se_{3} thin film sample, 50 quintuple layers (~50 nm thick), is grown by molecular beam epitaxy on a 0.5 mm thick sapphire substrate. The sample is mounted together with a 0.5 mm thick pure sapphire substrate, used as a reference, into a cryostat with temperatures down to T = 5 K. Two copper mounts with the same aperture are placed directly in front of the sample and reference to ensure uniform photoexcitation and accurate comparison of their THz transmission. The sample studied has a Fermi energy E_{F} ~60 meV from the bulk conduction band edge, as estimated from the measured plasma frequency in the static THz conductivity spectra. Please note that the exact value of the gap size is not critical for our scheme, nor does it change our conclusion, as long as the interband transition gap in our sample is larger than our pump photon energy ~4 meV. Other details can be found in the Supplementary Note 2.
Data availability
The data that support the findings of this study are available from the corresponding author upon reasonable request.
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Acknowledgements
This work (scientific driver, THz spectroscopy and theory) was supported by the U.S. Department of Energy, Office of Basic Energy Science, Division of Materials Sciences and Engineering (Ames Laboratory is operated for the U.S. Department of Energy by Iowa State University under Contract No. DEAC0207CH11358). Sample development was supported by National Science Foundation DMR 1400432. Terahertz instrument was supported in part by National Science Foundation EECS 1611454. I.E.P. (data analysis) at the University of Alabama, Birmingham was supported by the US Department of Energy, Office of Science, Basic Energy Sciences under award no. DESC0019137.
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X.Y., C.V., and L.L. performed the experimental measurements and collected the data. D.C., Z.L., and R.H.J.K. helped to set up experimental instrumentation. The calculation and some data analysis was done by X.Z., Y.Y., I.E.P., C.Z.W., and K.M.H. Samples were developed by X.L., M.D.; and J.K.F. J.W., and X.Y wrote the paper with help from all authors. J.W. supervised the study.
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Correspondence to Jigang Wang.
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Yang, X., Luo, L., Vaswani, C. et al. Light control of surface–bulk coupling by terahertz vibrational coherence in a topological insulator. npj Quantum Mater. 5, 13 (2020). https://doi.org/10.1038/s4153502002157
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