Enhanced electron dephasing in three-dimensional topological insulators

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Abstract

Study of the dephasing in electronic systems is not only important for probing the nature of their ground states, but also crucial to harnessing the quantum coherence for information processing. In contrast to well-studied conventional metals and semiconductors, it remains unclear which mechanism is mainly responsible for electron dephasing in three-dimensional topological insulators (TIs). Here, we report on using weak antilocalization effect to measure the dephasing rates in highly tunable (Bi,Sb)2Te3 thin films. As the transport is varied from a bulk-conducting regime to surface-dominant transport, the dephasing rate is observed to evolve from a linear temperature dependence to a sublinear power-law dependence. Although the former is consistent with the Nyquist electron-electron interactions commonly seen in ordinary 2D systems, the latter leads to enhanced electron dephasing at low temperatures and is attributed to the coupling between the surface states and the localized charge puddles in the bulk of 3D TIs.

Introduction

Three-dimensional topological insulators (TIs) have emerged as an important class of materials that are characterized by an insulator-like bulk and gapless surface states protected by time-reversal symmetry1,2. TIs and their derivative structures have been predicted to possess many fascinating properties and attracted a great deal of attention1,2,3,4. Recent progresses in improving the quality and electrical gating of TI materials5,6,7,8,9,10,11 have led to remarkable observations of the quantum anomalous Hall effect12, the quantum Hall effect13,14, as well as many quantum coherent transport properties, such as weak antilocalization (WAL)15,16,17, Aharonov-Bohm and Aharonov-Aronov-Spivak effects18,19 and universal conductance fluctuations20,21. It has also been proposed that quantum interference experiments can be used to probe Majorana zero modes formed on the TI surfaces due to superconducting proximity effect22,23. A full understanding of the dephasing processes is thus important for utilising various phase-coherent properties in TIs4,24. Such insight is also crucial to addressing many fundamental questions regarding TI surface states, for instance, the nature of their ground states under the influence of disorder and electron–electron interactions25,26,27,28. However, the electron dephasing rates obtained in experiments exhibit a variety of temperature-dependent behaviours. Some groups reported the linear temperature dependences19,20,29,30 that are often encountered in conventional 2D electron systems31,32,33, whereas others found much weaker or stronger temperature dependences even in TI samples with presumably insulating bulk34,35,36. The lack of consistency in the temperature dependences has precluded clear identification of the dephasing mechanisms, and brings an obstacle to the quantum coherent experiments that require long electron dephasing lengths4,22,23,24.

Measurement of the magnetoresistance due to weak localization or WAL has proven a reliable technique to study the electron dephasing in diffusive electron systems of various dimensions31,32,33. Similar magnetotransport measurements have been carried out on many types of TI thin films or microflakes10,11,15,16,17,29,30,34,35,36,37,38. The low field magnetoconductivity is usually described very well with the Hikami-Larkin-Nagaoka (HLN) equation39 at the strong spin-orbit coupling limit:

where ψ(x) is the digamma function, is the dephasing field, D is the diffusion constant, and lφ is the dephasing length. For a single-channel WAL-type transport, prefactor α would be equal to 1/2. In case of multi-channel WAL, the α value can vary from 1/2 to nc/2, where nc=2α is the number of parallel conduction channels. The nc value obtained from the HLN fit is, however, often far from integers due to the difference in the dephasing fields or the coherent coupling between these channels40. When the inter-channel coupling is not negligible, determination of the dephasing rate τφ−1 becomes very challenging because the parameter Bφ extracted from the HLN fit is no longer a simple quantity proportional to τφ−1. An ideal scenario is the surface-dominant transport with two symmetric channels (corresponding to α=1, see Supplementary Note 1). It allows for straightforward extraction of the dephasing rate with a fit to Equation (1). This transport regime, however, requires not only the bulk is insulating, but also the top and bottom surfaces are decoupled and have identical dephasing fields. Unfortunately, most of the dephasing measurements reported so far have not fulfilled these conditions owing to inadequate control of the surface and bulk conductivities.

In this work, we present the measurements of electron dephasing rates in 3D TI thin films with highly tunable chemical potential. The phase coherent transport related to the WAL can be tuned continuously from a bulk-conducting regime with α=1/2 to a decoupled surface-transport regime with α=1 in a single device. Whereas the common Nyquist dephasing behaviour41 is observed in the former regime, the dephasing rate is found to have a sublinear power-law temperature dependence in the surface-transport regime. We propose that the coupling between the surface states and localized bulk states in a variable range hopping (VRH) regime is responsible for the enhanced electron dephasing and the sublinear temperature dependence in the surface-transport regime.

Results

Characterization of (Bi1-xSbx)2Te3 field-effect devices

Our measurements were carried out in a set of field-effect devices based on 15–30 nm thick (Bi1-xSbx)2Te3 (BST) films grown on SrTiO3 substrates with molecular beam epitaxy. A high Sb composition (x>0.9) was chosen to prevent the Dirac point being buried inside the bulk valence band8,9. The ungated BST films have a conducting bulk with p-type carriers. As illustrated in Fig. 1 with a 15 nm thick BST film (Sample #1), the Hall-bar shaped device is equipped with both the top and bottom gates, which enable a large range tuning of the chemical potential. When a positive gate voltage is applied, the hole density is reduced and correspondingly the magnitude of Hall coefficient RH decreases. When the gate voltage is sufficiently high, the Fermi level passes the charge neutral point, which is manifested as a reversal of the sign of RH and appearance of a maximum in longitudinal resistivity ρxx. At large positive gate voltages, the Fermi level is shifted into the bulk band gap and the surface-dominant transport is achieved. For instance, with back-gate voltage VB=210 V and top-gate voltage VT=25 V, surface carrier densities as low as n1=3.3 × 1011cm−2 and n2=4.0 × 1012cm−2 can be obtained from a two-band fit of the Hall effect data. Such low electron densities indicate that the Fermi level in the BST film resides in the bulk band gap (See Supplementary Fig. 2 and Supplementary Note 2 for more details), consistent with angular resolved photoemission studies of similar BST films9.

Figure 1: Tunable electron transport in a 15 nm thick (Bi1-xSbx)2Te3 topological insulator (TI) thin film (Sample #1).
figure1

(a) Sketch of the Hall bar-shaped device with a back gate and a top gate. The width of the current path is 50 μm. (b,c) Hall coefficient RH and longitudinal sheet resistivity ρxx rendered in a 2D map in top-gate voltage VT and bottom-gate voltage VB. The thin dashed line in b marks the gate voltages for RH=0. The sign of RH is set to positive for electrons throughout this work. (d) Gate-voltage dependence of zero-field ρxx and Hall coefficient RH. The open circles represent the data for VT=0, whereas the solid symbols stand for the case of dual-gating, in which the corresponding (VT, VB) values are shown in b with solid diamonds. (e) Hall resistance curves for several set of top and bottom gate voltages. Data in be were taken at T=1.6 K. (f) Schematic band diagrams for the top and bottom surface states for the decoupled surface-transport regime (A) and the bulk-conducting regime (B).

High tunable phase-coherent transport

Figure 2a shows the magnetoconductivity curves of the BST film at several gate voltages at T=1.6 K. All of them can be satisfactorily fitted with the HLN equation. Shown in Fig. 2b are the α and Bφ values extracted from the fits. For small gate voltages, α is close to 1/2, in agreement with previous measurements of TI thin films with conducting bulk10,11,15,16,37. This can be attributed to strong surface-bulk coupling, which makes the sample, behaving like a single-channel system in the phase coherent transport despite the coexistence of multiple conduction channels40. This transport regime is realized when the inter-channel scattering rate is much higher than the dephasing rates in individual channels (See Supplementary Note 1). It is also noteworthy that in this work the dephasing length extracted from the fit to Equation (1) is always much longer than the corresponding film thickness. Therefore, even in the bulk-conducting regime, the phase coherent transport is two dimensional, justifying the application of the HLN equation for the data analysis. As the positive gate voltage increases, the depletion of hole carriers in the bulk leads to gradual decoupling between the top and bottom surfaces and accordingly the α value becomes greater15,16,17,38. When these two surfaces are fully decoupled and their dephasing fields are brought into equality, α=1 is observed. For the BST thin films studied in this work, both α1/2 and α1 can be maintained for a wide range of temperatures at fixed gate voltages, as depicted in Fig. 2d,e. Such a good tunability in the phase coherent transport provides a solid foundation for studying the temperature dependence of dephasing rate in TIs.

Figure 2: Tunable surface-bulk coupling in the BST thin film (Sample #1) revealed in the magnetotransport.
figure2

(a) Low field magnetoconductivity and the best fits to the Hikami-Larkin-Nagaoka (HLN) equation. (b) Gate-voltage dependence of prefactor α and dephasing field Bφ extracted from the HLN fits. The gate voltages used for the dual-gating are same as those in Fig. 1. The error bars denote s.d.s of Bφ determined from various fitting ranges. (c,d) Temperature dependence of the prefactor α in both decoupled surface-transport regime (α≈1) and bulk-conducting regime (α≈1/2). Slight differences between different cool-downs were caused by exposure of the sample to atmosphere during the measurement intervals.

Electron dephasing rates in surface-transport regime

Figure 3a shows the temperature dependence of the dephasing field Bφ extracted from the HLN fits for the case of α1. In this decoupled surface-transport regime, the transport takes place in two independent, equivalent channels and the dephasing rate τφ−1 is simply proportional to Bφ (See Supplementary Note 1). Figure 3b depicts that Bφ has a sublinear power-law dependence: BφTp with p=0.55 for a wide range of temperatures (0.1–10 K). Similar results have also been obtained from other BST samples with various thicknesses (15–30 nm), in which p is distributed in a range of 0.45–0.60 when the prefactor α is tuned close to 1 (See Supplementary Fig. 6, Supplementary Table 1 and Supplementary Note 5). These values are substantially lower than the p=1 that is corresponding to the linear dependence commonly observed in conventional 2D electron systems31,32.

Figure 3: Enhanced electron dephasing in the decoupled surface-transport regime.
figure3

(a) Temperature dependence of dephasing field Bφ for a dual-gating case with α≈1. The data can be well fitted to BφTp with p=0.55. (b) T-dependences of Bφ and the corresponding power-law fits for three cool-downs with single-gating. The extracted exponent p is same as the dual-gating case. (c) Dephasing time τφ of the bottom surface states as a function of temperature. The dashed line shows the estimated dephasing times due to the Nyquist electron–electron interactions.

Crossover to linear dependence in bulk-conducting regime

In contrast to the surface-transport regime, the dephasing field in the bulk-conducting regime has qualitatively different temperature dependences. As depicted in Fig. 4a, Bφ exhibits a nearly perfect linear temperature dependence when α is tuned close to 1/2. Figure 4b,c (see Supplementary Fig. 4 for more details) further show that reducing the bulk conductivity by increasing the gate voltage can induce a crossover from the linear T-dependence to sublinear ones by varying the gate voltage. The variation of p from 1 to 0.55 is correlated well with the increase of α from 1/2 to 1, as the bulk-mediated coupling between the top and bottom surfaces become stronger with increasing bulk conductivity. Observation of such a crossover in a single device rules out the possibility of extrinsic mechanisms, such as magnetic impurities4, environmental microwave radiation42 or interfacial interaction with the STO substrates, for the sublinear T-dependences in the decoupled surface-transport regime. Otherwise, similar deviations from the linear dependence would also be observed in the bulk-conducting regime.

Figure 4: Tunable power-law temperature dependence of the dephasing rate.
figure4

(a) Temperature dependence of dephasing field Bφ, which is proportional to the dephasing rate τφ−1, in the bulk-conducting regime (symbols) and the corresponding linear fit (line). (b) T-dependences of Bφ for several gate voltages. The transport is tuned from the bulk-conducting regime (α≈1/2) to the decoupled surface-transport regime (α≈1) as the gate voltage VB increases. The Bφ values obtained from the HLN fits are shown in symbols and the lines are the fits to BφTp. (c) Prefactor α and exponent p for the same set of gate voltages as (b). (d) Schematic diagram of the TI bulk bands with strong fluctuations due to the compensation doping. The filled areas denote nanoscale electron and hole puddles43. (e) Cartoon illustration of electron dephasing in the surface states owing to strong coupling to the localized charge puddles in the bulk.

Discussion

For a weakly disordered conventional 3D electron system, electron–phonon interactions are the dominant source of electron dephasing, which gives rise to a power-law temperature dependence of the dephasing rate: τφ−1Tp, with p=2–4 (ref. 32). In low dimensional systems, the dominant dephasing mechanism at low temperatures is usually associated with small energy transfer processes owing to electron–electron interactions31. This so-called Nyquist dephasing, first proposed by Altshuler et al.41, also leads to a power-law T-dependence, but with a smaller exponent: p=2/3 and 1 for 1D and 2D electron systems, respectively. The Nyquist mechanism has been confirmed by numerous magnetotransport experiments on low dimensional metals or semiconductors31,32. As shown above, the p values for the decoupled surface-transport regime in TIs are in a range of 0.45–0.60, substantially lower than those of the known dephasing mechanisms for weakly disordered, nonmagnetic 2D electron systems31,32,33. Figure 3c further shows that dephasing times estimated for the surface states are considerably shorter than the theoretical values for the Nyquist dephasing. This indicates the existence of an additional dephasing source in the topological transport regime.

Given the fact that decreasing the bulk conductivity in TIs can induce the crossover from the Nyquist dephasing to the sublinear power-law temperature dependence, it is reasonable that the evolution of bulk states with gating are involved in the crossover of the dephasing behaviour. As revealed by previous studies, TIs in the family of bismuth chalcogenides do not have truly insulating bulk3. Even in the state-of-the-art materials, such as (Bi,Sb)2(Te,Se)3 single crystals5,6,7,13, the bulk conductivity does not freeze out completely at low helium temperatures (typically on the order of Ω·cm). This was first explained by Skinner et al.43, who pointed out that the narrow band gaps and electrostatic fluctuations from the compensation doping result in the formation of localized nanometre-sized charge puddles in the bulk, and consequently the VRH of charge carriers between these puddles is energetically favoured over the thermal activation. In addition to the estimated bulk resistivities from the transport measurements of thick TI single crystals, the existence of surface and bulk charge puddles has been supported by scanning tunnelling microscopy44 and optical conductivity measurements45, respectively. In addition, the VRH transport has been directly observed in ultrathin BST films, in which the surface conductivity is suppressed by a hybridization gap46.

For the BST films with the bulk layer in the VRH regime, the transport is dominated by the diffusive Dirac fermions on the surfaces. If the films are sufficiently thick, the top and bottom surfaces do not couple to each other coherently owing to the lack of direct tunnelling. The phase coherent transport can be modelled as a decoupled two-channel system. Even though the localized charge puddles carry little electrical current due to the high resistivity, they can couple to the surface states via tunnelling. As the hopping transport is an inelastic process, the surface-bulk coupling makes the charge puddles working as an environmental bath with very low energy excitations and thus opens a new avenue for the dephasing in surface states. In the VRH regime, the dephasing length is believed to be set by the hopping distance and hence follows lφ,VRHTp/2, with p=2/3 and 1/2 for 2D and 3D systems, respectively47 (See Supplementary Note 3). At sufficiently low temperatures, lφ,VRH becomes shorter than that for the Nyquist dephasing, namely lφ,eeTp/2 with p=1. Therefore, the surface-bulk coupling can reduce the dephasing length significantly, leading to the enhanced dephasing rates shown in Fig. 3c. In case of lφ,VRH<<lφ,ee and strong surface-bulk coupling (that is, τφ,SB<<τφ,ee), the dephasing rate follows with 1/2≤p≤2/3. This is consistent with the p values (p=0.45–0.60) obtained from the dephasing field measurements as well as the temperature dependence of conductivity (Fig. 4, Supplementary Figs 3–6 and Supplementary Notes 4–6).

In addition to the dephasing induced by the hopping between the localized bulk states, the inelastic coupling between the surface states and individual charge puddles might also cause dephasing. For 2D TIs, Väyrynen et al.48,49 showed theoretically that electron tunnelling between edge states and individual charge puddles in the bulk can cause electron backscatterings and hence a decrease in conductivity. An earlier theoretical work by Jiang et al.50 showed that similar deviation from the quantized conductance in 2D TIs can be understood as an electron dephasing effect. However, a direct link between the dephasing and the charge puddles in 2D TIs has been established neither in theory nor in experiment51. To the best of knowledge, previously reported works on charge puddles in 3D TIs were focused on the conductivity of the bulk43,44,45, and the possible influence on electron dephasing has never been investigated. Even though it is reasonable that the strong coupling between the charge puddles and the edge/surface states could exist in both 2D and 3D TIs, there could be some qualitative differences between these two systems. It was pointed out in ref. 50 that only the dephasing scatterings with spin flips can cause electron backscatterings in 2D TIs. In contrast, all types of electron dephasing, including those without spin flips, are expected to cause a suppression of the WAL effect in 3D TIs. It is also interesting to note that a recent theoretical work showed that the energy transport in the VRH regime is much more efficient than the charge transport due to Coulomb interaction between the localized states52. It is likely that the Coulomb interaction of the TI surface states with the charge puddles in the bulk can potentially be an additional source of dephasing. Obviously, further theoretical efforts are needed to gain deeper insight into the electron dephasing or more generally the quantum transport properties related to the charge puddles in both 2D and 3D TIs.

As all known TIs have narrow band gaps in the bulk3, the electron dephasing caused by the localized charge puddles should not be limited to the BST thin films studied in this work. At low temperatures, the enhanced dephasing severely shortens the dephasing length, and should be detrimental to the experiments requiring long phase coherent lengths, for instance, the interferometers proposed to detect Majorana zero modes22,23,24. Therefore, it is highly desirable to search for the TI materials in which the dephasing caused by the charge puddles can be substantially suppressed. The electron dephasing measurement will play an unreplaceable role in such endeavours because it can probe the interaction between the surface and bulk states at a very small energy scale (down to the order of μeV). Such information is very difficult, if not impossible, to obtain from other transport or spectroscopic measurements. Finally, it is noteworthy that the coupling between the diffusive surface states and the bulk states in the hopping regime revealed in this work can be extended to non-topological bilayer systems. Such coupling can be utilized to offer a new method to measure electron dephasing rates in electron systems that are not in the weakly disordered regime. This could provide valuable information to the study of electron dephasing phenomena in non-diffusive systems, which have been very challenging both experimentally and theoretically53.

Methods

Thin film growth and device fabrication

TI BST thin films were grown on 500 μm thick SrTiO3 (111) substrates in a molecular beam epitaxy (MBE) system with a base pressure of 1 × 10−10 Torr or lower. The BST films are single crystalline and have large, atomically flat terraces on the surfaces, similar to those reported previously46,54. They were capped with a 10 nm thick amorphous Te layer before being taken out of the molecular beam epitaxy chamber. The samples were subsequently patterned into standard Hall bars with photolithography and chemical wet etching. A 35 nm thick AlOx thin film was deposited with atomic layer deposition onto the BST samples to serve as the dielectric material for top-gating. The SrTiO3 substrates, which have exceptionally large dielectric constants and high electrical breakdown strength, were used as the bottom-gate dielectric. Both top and bottom gate-electrodes, as well as electrical contacts were prepared by thermal evaporation of Cr/Au thin films with typical thicknesses of 5 nm/80 nm.

Electron transport measurements

The I–V characteristics of all electrical contacts and gates had been checked with Agilent source-measurement units with a current resolution of 100 fA before the electron transport measurements. All of the data presented in this manuscript were taken from the samples with good ohmic contacts and the leakage current is negligible for both top and bottom gates. The transport experiments were performed in a vapour-flow 4He flow cryostat, a 3He refrigerator and a top loading 3He/4He dilution refrigerator with magnetic fields up to 15 T. Electrical wirings of the dilution refrigerator are equipped with a variety of low pass filters at different temperature stages so that electron temperatures lower than 15 mK can be obtained. The electron temperature has been confirmed by the measurements of activation gaps of fragile fractional quantum Hall states (for instance, the 5/2 state), and dephasing phenomena in the quantum Hall plateau-to-plateau transitions in high mobility GaAs/AlGaAs 2D electron systems, as well as quantum transport properties of other systems. Standard lock-in technique with low frequency ac current (typically at 17.3 Hz and no more than 100 nA) was used for the transport measurements. The amplitude of excitation current was optimized to avoid electron heating effects while maintaining sufficient signal-to-noise ratios (see Supplementary Fig. 1 for an example of testing the measurement current). The longitudinal and Hall resistivities presented in this manuscript were obtained by symmetrization and anti-symmetrization of the raw magnetotransport data with respect to the magnetic fields.

Data availability

The data that support the findings of this study are available from the corresponding author upon request.

Additional information

How to cite this article: Liao, J. et al. Enhanced electron dephasing in three-dimensional topological insulators. Nat. Commun. 8, 16071 doi: 10.1038/ncomms16071 (2017).

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Acknowledgements

We thank P. Ostrovsky, Q. F. Sun and X. C. Xie for valuable discussions. This work was supported by the National Basic Research Program of China (Projects No. 2015CB921102, No. 2015CB921001 and No. 2012CB921703), the National Key Research and Development Program (Project No. 2016YFA0300600), the National Science Foundation of China (Projects No. 61425015, No. 11374337, No. 11325421, No. 11674028 and No. 91121003), and the Strategic Initiative Program of Chinese Academy of Sciences (Project No. XDB070200).

Author information

Y.L. and K.H. initiated the project. Y.O. carried out the MBE growth of the samples. J.L. fabricated the Hall bar devices, performed the electron transport measurements. J.L., H.L. and Y.L. analysed the data and prepared the manuscript with contributions from all authors.

Correspondence to Ke He or Yongqing Li.

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Liao, J., Ou, Y., Liu, H. et al. Enhanced electron dephasing in three-dimensional topological insulators. Nat Commun 8, 16071 (2017) doi:10.1038/ncomms16071

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