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Dielectric collapse at the LaAlO3/SrTiO3 (001) heterointerface under applied electric field

Scientific Reportsvolume 7, Article number: 9516 (2017) | Download Citation

Abstract

The fascinating interfacial transport properties at the LaAlO3/SrTiO3 heterointerface have led to intense investigations of this oxide system. Exploiting the large dielectric constant of SrTiO3 at low temperatures, tunability in the interfacial conductivity over a wide range has been demonstrated using a back-gate device geometry. In order to understand the effect of back-gating, it is crucial to assess the interface band structure and its evolution with external bias. In this study, we report measurements of the gate-bias dependent interface band alignment, especially the confining potential profile, at the conducting LaAlO3/SrTiO3 (001) heterointerface using soft and hard x-ray photoemission spectroscopy in conjunction with detailed model simulations. Depth-profiling analysis incorporating the electric field dependent dielectric constant in SrTiO3 reveals that a significant potential drop on the SrTiO3 side of the interface occurs within ~2 nm of the interface under negative gate-bias. These results demonstrate gate control of the collapse of the dielectric permittivity at the interface, and explain the dramatic loss of electron mobility with back-gate depletion.

Introduction

Since the discovery of a variety of interfacial electronic states between insulating and non-magnetic (001)-oriented LaAlO3 and SrTiO3, such as high-mobility metallic states1, superconductivity2, 3, and magnetism4,5,6,7, the origin of these properties has been widely discussed8, 9. Given the robust insulating character of LaAlO3, it is generally understood that the electron gas forms on the SrTiO3 side of the interface10,11,12,13,14,15,16,17. Indeed, an in situ photoemission spectroscopy (PES) study revealed downward band bending toward the interface in the SrTiO3 17. Notable in this system is the dramatic tunability of the interfacial conductivity using external electric fields, attracting considerable attention for fundamental studies, as well as device applications18, 19. The application of a back-gate voltage V g tunes multiple parameters in the system simultaneously, including the superconducting transition temperature, the carrier density, the Hall mobility and the confining electric field3, 18, 20,21,22,23. In order to understand how these changes are inter-related, especially the dramatic loss of Hall mobility with back-gate depletion20, knowledge of the band alignment and potential profile changes with gating is essential.

In this study, we analyze the depth profile of the potential on the SrTiO3 side of LaAlO3/SrTiO3 (001) heterojunctions using synchrotron radiation PES for various V g. A schematic of the experimental setup is shown in Fig. 1. Depth resolution was achieved by varying the energy of the synchrotron-radiation light source - both soft x-ray PES (SX-PES) and hard x-ray PES (HAX-PES) were utilized - combined with precise tuning of the incident and emission angles24. Analysis of the SX-PES and HAX-PES core-level spectra with negative V g reveal an abrupt downward shift of the potential, narrowing the electron confinement to within ~2 nm of the LaAlO3/SrTiO3 interface. These results explain why back-gate depletion modulates the mobility far more strongly than the carrier density, and suggests this is a generic feature of nonlinear dielectrics that can be utilized in device structures.

Figure 1
Figure 1

Experimental setup for measurements of PES spectra for LaAlO3/SrTiO3 heterostructures with applied electric field at the back of the SrTiO3. Ground contact is made to the electron gas at the heterointerface using Al wire bonding. The photoelectron emission angle (θ) is defined as the angle from the surface normal.

Results

Photoemission core-level spectroscopy of LaAlO3/SrTiO3

The measured Ti 2p core-level spectra of the LaAlO3/SrTiO3 heterostructures at V g = 0 V and a bare SrTiO3 (001) substrate are shown in Fig. 2. The characteristic probing depth λ, based on the theoretical study of Tanuma et al.25, was tuned by changing the irradiation photon energy () and the photoelectron emission angle (θ) with respect to the surface normal. was 1.2 keV (λ = 2.0 nm for θ = 0 degree) and 7.9 keV (λ = 10 nm for θ = 0 degree), θ was varied from 0 to 80 degrees (also see Fig. 1). The Ti 2p core-level spectra from the LaAlO3/SrTiO3 sample are shifted towards more positive relative binding energy from that of the bare SrTiO3 substrate with no observable Ti3+ component, as previously found17. As the probing depth becomes shallower (λ < 10 nm), no significant peak shift or broadening characteristic to potential variation, was observed within the experimental resolution of 50 meV. These results together with the gate-tunable transport properties20 imply that the potential profile varies on the scale of 10 nm or more in the SrTiO3 from the LaAlO3/SrTiO3 heterointerface. By assuming that all carriers detected from Hall effect under no applied bias (n 2D ~2 × 1013 cm−2) reside within 0.4 nm of SrTiO3 surface and fully contribute to the Ti3+ signal, the estimated total volume of Ti3+ is still below its practical detection limit of 2~3 at. %. Moreover, the possible carrier distribution, which is interrelated with the potential profile, experimentally prohibits the observation of any Ti3+ states present.

Figure 2
Figure 2

Ti 2p core-level spectra of LaAlO3/SrTiO3 heterostructures without bias gate voltage. The relative binding energy is given with respect to the Ti 2p core-level spectra of a bare SrTiO3 substrate as reference (black line). λ is the probing depth controlled by photon energy and emission angle; λ = 1.6 and 10 nm are obtained by HAX-PES ( = 7.9 keV) with θ = 80 and 0 degrees, respectively, while others (λ = 2.0, 1.4 and 1.0 nm) are SX-PES ( = 1.2 keV) results with varied angles at θ = 0, 45, and 60 degrees, respectively.

Figure 3 show the measured Ti 2p core-levels using (a) SX-PES and (b) HAX-PES with −100 V ≤ V g ≤ 100 V. For all V g, the gate leakage current through the SrTiO3 during the PES measurements was less than 10 nA. The binding energy of the SrTiO3 core-level spectra were normalized to those of the LaAlO3 spectra, which minimizes possible artifacts from the PES measurements, such as fluctuations of the photon energy. For negative V g, the Ti 2p core-level first shifts to more positive relative binding energy from V g = 0 V before saturating at +0.1~+0.2 eV in the case of SX-PES, while it remains unchanged for the HAX-PES. Both SX-PES and HAX-PES measurements show no Ti 2p core-level shift for positive V g. Similar results were also obtained in the Sr 3d core-level measurements. The change of the Ti 2p core-level peak position are plotted as a function of V g in Fig. 3(c) and (d), showing a total energy shift ~+0.15 eV for V g < 0 V for the SX-PES without any hysteresis.

Figure 3
Figure 3

Ti 2p core-level spectra of LaAlO3/SrTiO3 heterostructures measured using (a) SX-PES ( = 1.2 keV, θ = 0 degree) and (b) HAX-PES ( = 7.9 keV, θ = 0 degree) with applied gate voltage. Plots of relative binding energy (B.E.) shift between (c) Ti 2p and La 4d core-level spectra (filled circles), Ti 2p and Al 2p (open triangles) for SX-PES data, and (d) Ti 2p and La 4d core level spectra (filled circles) from HAX-PES data. The error bars in (c,d) were obtained from the accuracy of the peak fitting. The two sets of data points correspond to the forward and backward voltage sweeps to evaluate a possible hysteresis.

Qualitatively we can examine these results by considering the simultaneous tuning of the sheet carrier density and the potential profile due to the application of negative V g. Considering the SrTiO3 substrate as a capacitor dielectric between the back gate contact and the interface conducting layer, V g < 0 V corresponds to depletion of carriers at the interface resulting in a downward shift of the Fermi energy (E F) towards the conduction band bottom. At the same time however the band-bending is enhanced by the gating. This shifts the center of the electron distribution closer to the interface. For fixed sheet carrier density, n 2D, the increased confinement shifts E F upwards in energy, opposite to the effect of depletion. Since the SX-PES Ti 2p core-level shifts to higher binding energy for V g < 0 V the band-bending induced upshift in E F is dominant. Indeed the dielectric constant of SrTiO3 at room temperature ε r(T = 300 K)~350, gives a total carrier density change of ~2 × 1010 cm−2 for V g = −50 V. This is just 0.14% of the measured total Hall sheet carrier density in this sample20. The magnitude of the energy shift clearly depends on the probing depth of the PES measurement compared to the characteristic length scale of the confinement potential narrowing. Hence the lack of an observable shift in the HAX-PES data suggests that the most significant changes in the confining potential occur in the topmost layers of the SrTiO3.

Self-consistent simulation for the core-level spectra and potential profile

In order to quantitatively analyze these scenarios, we simulated the potential profile in SrTiO3 as a function of the depth (z) from the interface based on a modified Thomas-Fermi screening model, using the PES data to constrain the results. The scheme of self-consistent calculation is as follows: for a trial potential Φ(z), the carrier density profile n(z) is calculated using

$$n(z)={\int }_{{\epsilon }=0}^{\infty }D({\epsilon })f({\epsilon })d{\epsilon },$$
(1)

where D(\({\epsilon }\)) is the density of states at electron energy \({\epsilon }\) from the conduction band minimum which is calculated via \(D({\epsilon })={(2{m}^{\ast }/{\hslash }^{2})}^{3/2}{\epsilon }{(z)}^{1/2}/2{\pi }^{2}\), where \({m}^{\ast }\) is the effective mass of SrTiO3, \(\hslash \) is Plank’s constant divided by 2π, and \(\,{\epsilon }(z)\) is based on Φ(z)16, and f(\({\epsilon }\)) is the Fermi-Dirac function. Following ref. 16, we use the three-dimensional form of the density of states. The potential is obtained by solving Poisson’s equation

$$\frac{\partial }{\partial z}({\varepsilon }_{0}{\varepsilon }_{r}({\mathbb{E}})\frac{\partial {\rm{\Phi }}(z)}{\partial z})=-{e}_{0}n(z).$$
(2)

ε 0 is the vacuum permittivity, ε r(\({\mathbb{E}}\)) is the electric field (\({\mathbb{E}}\)) dependent relative permittivity of bulk SrTiO3, and e 0 is the elemental charge. Here, we assumed other sources of charge, e.g. holes, extrinsic donors and acceptors, are negligible. Equations (1) and (2) were solved self-consistently with a convergence criterion of 0.01% throughout the whole depth region. For each V g, the two boundary conditions used are Φ(z = 0) and \(\frac{\partial {\rm{\Phi }}(z)}{\partial z}|\,\) z=∞ . The former is equal to the energy shift of the Ti 2p core-level peak position in the SX-PES spectra at the appropriate V g 24, and the latter is 0 V/m and 1 × 105 V/m, for V g = 0 and −50 V respectively, given the 0.5 mm SrTiO3 substrate thickness. In order to compare the experimentally obtained spectra with our model, we introduce an evaluation function known as the core-level intensity spectrum I(E). This is generally computed according to

$$I(E)\propto {\sum }_{z=0}^{\infty }\exp (-z/\lambda \,\cos \,\theta )C[E-{E}_{0}-{\rm{\Phi }}(z)],$$

where C(E) represents a core-level spectrum described by a Voigt function peaked at E 0, which in this case we set to zero as we are interested only in the relative change in the spectrum at different V g, not in the absolute value of E 0 24. The final best fit result is determined by minimizing the sum of the squares of the difference between the measured and calculated forms of the I(E) for both the SX-PES and HAX-PES measurements.

The electric field (\({\mathbb{E}}\)) dependent local nonlinear permittivity of SrTiO3, ε r(\({\mathbb{E}}\), z), must be considered as discussed in previous reports16, 20, 26. First we attempted to utilize the reported form of ε r(\({\mathbb{E}}\)) in our simulation (Fig. 4(c) inset)27. However when n 2D was constrained to the measured value from Hall effect20, satisfactory agreement with the PES spectra was not possible. Even allowing n 2D to be a free parameter (allowing for the possibility of localized charge not contributing to the Hall measurement), no value could reasonably fit the spectra and other features such as the core-level shift in Fig. 3(c) (see supplementary materials). The key point is that the reported bulk form of ε r(\({\mathbb{E}}\)) did not accurately reproduce the nonlinearity of the dielectric permittivity inferred from the data.

Figure 4
Figure 4

The calculated self-consistent potential and carrier density profiles. (a) Simulated potential depth profiles of the electron gas, for V g = 0 and −50 V. Inset of Fig. 4(a) shows the magnification around the interface. (b) Self-consistent carrier profile and (c) the resultant ε r(\(z)\) for V g = 0 and −50 V. The inset of Fig. 4(c) shows the comparison between the extracted form of ε r(\({\mathbb{E}}\)) (symbols and dashed line) and the reported ε r(\({\mathbb{E}}\)) (solid line)27. Measured and simulated SX-PES and HAX-PES Ti 2p core-level spectra for (d) V g = 0 V, and (e) V g = −50 V. Open circles are the experimental data, and solid lines are the best-fit simulations. Dashed lines correspond to the Ti 2p core-level spectrum of a bare SrTiO3 substrate. (f) The calculated electric displacement field from the inset of Fig. 4(c). Solid line is calculated by fitting the extracted form of ε r(\({\mathbb{E}}\)) in the inset of Fig. 4(c) using a sigmoid function.

As an alternative, we then assumed a smoothly varying dielectric constant as a function of distance from the interface ε r(z) for V g = 0 and −50 V, based on a simple sigmoid function, which was used as a physically reasonable qualitative form. The self-consistently solved potential and carrier density profiles are shown in Fig. 4(a) and (b). Here the errors of the simulated parameters were estimated with a threshold of 3% increase in the total squared error from the minimum value, except for the error in Φ(0) which was directly taken from the experimental error in the PES spectra. The comparison between the experimental spectra (open symbols) and the best-fit simulated spectra (solid lines) from the obtained potential profiles are shown in Fig. 4(d) and (e). Good agreement is observed for both the SX-PES and HAX-PES data. The main panel of Fig. 4(c) shows the best fit ε r(z) for V g = 0 and −50 V in these simulations, and the insets of Fig. 4(c) shows the extracted ε r(\({\mathbb{E}}\)).

From these simulations, close to the interface, we find a relatively abrupt potential shift of ~0.15 eV inside the SrTiO3 for V g = −50 V compared to V g = 0 V. As shown in the inset of Fig. 4(a), the potential crosses E F around z = 6 nm and 2 nm for V g = 0 and −50 V, the former is in good agreement with previous experimental and theoretical estimates of the electron gas thickness being < 10 nm13, 15, 16, 28, 29.

Discussion

Experimentally a significant change of the potential around the interface occurred only for V g < 0 V, and not V g > 0 V. Based on these calculation results, we can explain this asymmetry by considering the magnitude of \({\mathbb{E}}\) around z = 0. For V g = 0 V, \({\mathbb{E}}\) is not large enough to significantly reduce ε r, and positive V g only tends to decrease the interfacial electric field. The resultant changes in the band-bending and position of E F are therefore relatively small and below the PES resolution. This is in stark contrast to the case of V g < 0 V, where \({\mathbb{E}}(z=0)\) is large enough to reduce ε r, which self-consistently enhances the confinement leading to significant changes in the potential which are measurable by SX-PES.

Quantitatively, the collapse of ε r with \({\mathbb{E}}\) obtained in the analysis above is more rapid than reported for non-doped SrTiO3 16, 30,31,32 and Nb doped SrTiO3 27; the latter being somewhat more strongly affected for a given \({\mathbb{E}}\) than the former one. This has important implications for calculations of electron accumulation layers in any SrTiO3–based heterostructure. We note that our self-consistent approach is the same as the one of Copie et al., who utilized the literature form of ε r(\({\mathbb{E}}\))16. The ε r(\({\mathbb{E}}\)) relationship reported by Yamamoto et al.27 has also been successfully used to model the depletion layer in metal/SrTiO3 Schottky junctions33. An important difference between the Schottky depletion layer and the LaAlO3/SrTiO3 is the existence of free electrons in the latter, which can screen applied electric fields in addition to the lattice polarization which is the only possibility in the former. Indeed, a recent theoretical study has noted the interplay between electron density changes and lattice polarization34. In order to clarify these points, direct microscopic investigations of the lattice polarization with gate voltage are essential. Noting the large changes in potential over just a few lattice parameters, the failure of the prior experimental measurements of ε r(\({\mathbb{E}}\)) to capture our data likely reflect the need to explicitly consider ε r on short length scales, and include nonlocal effects35, 36. In this sense, our model employing ε r (z) is one of the approximations implicitly incorporating the effect of k-dependence of ε r . Despite the flexibility in the functional form of ε r , an abrupt drop in the potential at the interface is an essential feature required to reproduce our spectroscopic results.

Finally we note the intriguing point that when the electric displacement field D(\({\mathbb{E}}\)) is calculated using the new functional form of ε r(\({\mathbb{E}}\)), \({\mathbb{E}}\) is multi-valued for 0.02 ≤ D ≤ 0.08 Cm−2, as shown in Fig. 4(f). Although the underlying physics and effects of such an electrostatic instability are currently not clear, it is possible that the presence of multiple metastable dielectric states in SrTiO3 close to the interface could induce local structural phase transitions37 and associated effects in resistive switching properties38, in addition to creating an unstable potential profile at the interface. The collapse of ε r around the interface, simultaneously enhancing the electron confinement and impurity scattering, especially at low temperatures, explains the substantial decrease in the mobility20 and enhanced localization37 that has been previously observed for back-gating. The strong contrast with top-gating39 suggests that this nonlinear dielectric response provides new device switching approaches in oxide heterostructures.

Methods

The LaAlO3/SrTiO3 was fabricated on TiO2-terminated SrTiO3 (001) substrates by pulsed laser deposition as described elsewhere20. During LaAlO3 depositions, the substrate was kept at a temperature of 800 °C, and the ambient oxygen pressure was maintained at 1 × 10−5 Torr. The LaAlO3 thickness is 10 unit cells (~4 nm), which is the identical sample used in our previous transport study using back-gate20. SX-PES and HAX-PES synchrotron radiation measurements were carried out under applied V g at beamline BL2C of the Photon Factory, KEK, Japan and beamline BL47XU of SPring-8, Japan, respectively. The SX-PES and HAX-PES spectra were recorded using a Scienta SES-2002 electron energy analyzer, and a Scienta R-4000 electron energy analyzer, respectively. All PES measurements were performed at room temperature. A schematic of the experimental setup is shown in Fig. 1. V g was applied from the back of the 0.5 mm thick SrTiO3 substrate during the PES measurements, with the LaAlO3/SrTiO3 interface grounded using Al wire bonding via a gold-coated copper plate. The back of the SrTiO3 substrate was electrically contacted to this copper plate using silver epoxy.

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Acknowledgements

The authors are grateful to R. Yasuhara, and S. Toyoda for experimental support, M. S. Bahramy, R. Takahashi, and M. Lippmaa for the useful discussions. This work was supported by the Department of Energy, Office of Basic Energy Sciences, Division of Materials Sciences and Engineering, under contract DE-AC02-76SF00515 (experimental work of M.M., Y.H., C.B., H.I., M.H., H.K.S. and H.Y.H.); and by ONR-MURI number N00014-12-1-0976 for modeling and simulations. The experiments with synchrotron radiation were carried out under the approval of Photon Factory Program Advisory Committee (Proposal Nos. 2010G503, and 2008S2-003) and SPring-8 Japan Synchrotron Radiation Research Institute (Proposal No. 2010B1696).

Author information

Author notes

    • M. Minohara

    Present address: Photon Factory, Institute of Materials Structure Science (IMSS), High Energy Accelerator Research Organization (KEK), Tsukuba, Ibaraki, 305-0801, Japan

    • C. Bell

    Present address: H. H. Wills Physics Laboratory, University of Bristol, Tyndall Avenue, Bristol, BS8 1TL, UK

Affiliations

  1. Stanford Institute for Materials and Energy Sciences, SLAC National Accelerator Laboratory, Menlo Park, California, 94025, USA

    • M. Minohara
    • , Y. Hikita
    • , C. Bell
    • , M. Hosoda
    • , H. K. Sato
    •  & H. Y. Hwang
  2. Geballe Laboratory for Advanced Materials, Department of Applied Physics, Stanford University, Stanford, California, 94305, USA

    • H. Inoue
    •  & H. Y. Hwang
  3. Department of Advanced Materials Science, The University of Tokyo, Kashiwa, Chiba, 277-8561, Japan

    • M. Hosoda
    •  & H. K. Sato
  4. Photon Factory, Institute of Materials Structure Science (IMSS), High Energy Accelerator Research Organization (KEK), Tsukuba, Ibaraki, 305-0801, Japan

    • H. Kumigashira
  5. Department of Applied Chemistry, The University of Tokyo, Bunkyo-ku, Tokyo, 113-8656, Japan

    • M. Oshima
  6. Japan Synchrotron Radiation Research Institute (JASRI), SPring-8, Sayo, Hyogo, 679-5198, Japan

    • E. Ikenaga

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Contributions

M.M., Y.H., and M.H. performed PES measurements. Samples were fabricated by C.B., and H.K.S. and H.I. assisted with the simulation of the PES spectra and potential profile. H.K., M.O., and E.I. assisted with the PES measurements at beamlines. Y.H., C.B., and H.Y.H. assisted with the planning, measurements and analysis of the study.

Competing Interests

The authors declare that they have no competing interests.

Corresponding author

Correspondence to M. Minohara.

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https://doi.org/10.1038/s41598-017-09920-9

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