Atomically sharp oxide heterostructures exhibit a range of novel physical phenomena that are absent in the parent compounds. A prominent example is the appearance of highly conducting and superconducting states at the interface between LaAlO3 and SrTiO3. Here we report an emergent phenomenon at the LaMnO3/SrTiO3 interface where an antiferromagnetic Mott insulator abruptly transforms into a nanoscale inhomogeneous magnetic state. Upon increasing the thickness of LaMnO3, our scanning nanoSQUID-on-tip microscopy shows spontaneous formation of isolated magnetic nanoislands, which display thermally activated moment reversals in response to an in-plane magnetic field. The observed superparamagnetic state manifests the emergence of thermodynamic electronic phase separation in which metallic ferromagnetic islands nucleate in an insulating antiferromagnetic matrix. We derive a model that captures the sharp onset and the thickness dependence of the magnetization. Our model suggests that a nearby superparamagnetic–ferromagnetic transition can be gate tuned, holding potential for applications in magnetic storage and spintronics.
In recent years the extensive efforts to create new types of heterostructures based on transition metal oxides have come to fruition1,2,3,4,5,6,7,8. The strong interactions characterizing these materials are an appealing feature as they provide a nurturing platform for new phases9. Interestingly, in the most extensively studied LaAlO3/SrTiO3 (LAO/STO) system, the non-magnetic insulator parent compounds give rise to conductivity1,7, magnetism10,11,12,13,14,15 and superconductivity2,14,15,16,17, which are sharply tuned by the number of LAO layers in the heterostructure. Motivated by the complex physics arising at the interfaces of band insulators, we studied LaMnO3 (LMO)/STO heterostructures, in which one parent compound (LMO) exhibits a very diverse phase diagram already in the bulk18. In undoped bulk LMO, orbital order due to Jahn–Teller distortions of the MnO6 octahedra sets in at high temperatures of ∼750 K. Subsequently, magnetic exchange between Mn3+ ions leads to formation of A-type antiferromagnetic (AFM) phase with Néel temperature of ∼140 K in which ferromagnetic (FM) planes are aligned antiferromagnetically19,20. At high doping or at high oxygen content, bulk LMO undergoes a phase transition into a FM metallic state19,21,22,23. The nature of the magnetic phases in thin films is, however, more controversial. While stoichiometric LMO is AFM in the bulk, a number of studies describe the appearance of FM behaviour even in stoichiometric thin films24,25,26,27,28,29,30. In addition, while FM state in the bulk is metallic, an insulating FM behaviour was reported for thin films25,26,27. Hence, the interplay between charge, orbital and spin degrees of freedom combined with low dimensionality and the fact that LMO has a polar structure similar to LAO, offers exciting potential for new emergent phenomena in superlattices and heterostructures20,27,31,32. In particular, since the existence of magnetism and its possible origins in LAO/STO remain controversial5,33, the prospect of realization of tunable magnetic order in LMO/STO is of high fundamental and technological interest.
We report here the observation of an abrupt transition from an AFM phase to a highly inhomogeneous magnetic state when more than five unit cells (u.c.) of LMO are epitaxially grown on the STO. Using a scanning superconducting quantum interference device (SQUID) microscope we probed the nature of the magnetic state. The imaging measurements reveal well separated and weakly correlated superparamagnetic (SPM) islands. These nanoscale magnetic puddles account for the entire magnetization of the LMO/STO heterostructure as observed in global measurements. We interpret the experimental findings as electronic phase separation leading to the nucleation of metallic nanoscale ferromagnetic islands embedded in an insulating antiferromagnetic matrix. We propose a theoretical model based on electronic reconstruction due to the polar nature of the interface that captures the essential part of our experimental results.
Magnetic structure in zero-field cooled state
Here we use a scanning probe microscope based on a nanoscale SQUID that resides on the apex of a quartz tip (SQUID-on-tip (SOT))34,35 for imaging of the local magnetic structure in stoichiometric LMO films grown epitaxially on TiO2-terminated (001) STO substrates (see Methods section). Figure 1a–f show images of the out-of-plane magnetic field Bz(x,y) in LMO films of various thicknesses acquired at a height of ∼100 nm above the sample surface at 4.2 K after zero-field cooling (ZFC). A highly inhomogeneous Bz(x,y) is observed in all the films with a characteristic scale of 100–200 nm, comparable to the size of our SOTs (90–230 nm diameter, Supplementary Table 1). Remarkably, even though the Bz(x,y) structures look similar, the span of the local field varies by more than three orders of magnitude between the samples (see colour bars). Figure 1g shows the quantitative analysis of the r.m.s., , and peak-to-peak, (inset), values of Bz(x,y) versus the thickness N (in u.c.) of the LMO film. For N≤Nc=5, and remain very small. However, at N=6 a discontinuous change in their values by more than an order of magnitude occurs. A similar behaviour, although on a much larger length scale, was recently reported by Wang et al.27 and interpreted as a phase transition from AFM to FM state driven by the polar electronic reconstruction. Interestingly, the saturation value Ms obtained from global magnetization measurements at elevated fields (Supplementary Fig. 1) shows similar N dependence (Fig. 1g, blue dots), further suggesting a sharp onset of FM order in LMO/STO. It is worth noting the same features were found everywhere across the sample (see Supplementary Note 1 and Supplementary Fig. 2).
Magnetization reversal process
Since global measurements show that LMO/STO films have an in-plane magnetization27 (Supplementary Note 2), we have studied Bz(x,y) while progressively increasing the in-plane magnetic field (Supplementary Movies 1 and 2). For each set value of , Bz(x,y) was acquired either in the presence of or after reducing back to zero (to minimize noise and drift), with similar results. Figure 2a,b shows an example of two consecutive Bz(x,y) images from Supplementary Movie 2 in N=12 u.c. sample for and 161 mT, which appear to be identical. To uncover the underlying magnetization process, we numerically subtract Fig. 2a from Fig. 2b, revealing small isolated dipole-shaped features in the differential image ΔBz(x,y) in Fig. 2c and in the corresponding Supplementary Movie 3. Figure 2d presents the numerical fit (see Methods section) of ΔBz(x,y) demonstrating that the dipole-shaped features are magnetization reversals of isolated nanoscale islands with in-plane magnetic moment m. As is increased, isolated islands undergo moment reversals at random locations, as presented in Fig. 3i and Supplementary Movie 4, indicating weak inter-island interactions. We did not observe magnetization reversal events for sample with N≤Nc=5 u.c. (Supplementary Fig. 3).
The observed magnetic behaviour is profoundly different from that expected for a FM state. A FM film after ZFC is composed of macroscopic domains with different magnetization orientations separated by domain walls (DW). As the field is increased, a magnetization process occurs through motion of DW: domains aligned along the magnetic field expand while oppositely aligned ones shrink, until a homogeneous state is achieved. Thus, the process of local microscopic magnetization reversal is highly correlated in space as DWs propagate through the sample. In the LMO/STO heterostructures, in contrast, there is no DW motion as seen in Supplementary Movies 1 and 2. Instead, the sample behaves as if it was composed of a sparse array of weakly interacting single-domain FM nanoparticles or islands. Since each nanoparticle has a different coercive field, the magnetization process occurs through uncorrelated reversal events of the individual islands at random locations (Supplementary Movie 4). This behaviour is analogous to slow magnetization dynamics in a two-dimensional array of SPM nanoparticles at temperatures below their blocking temperature TB, leading to a hysteretic magnetization loop36. Moreover, if the SPM islands are densely packed with a complete areal coverage, the resulting field distribution in the fully magnetized state should be uniform like in a fully polarized FM film. In contrast, Fig. 3a–d shows that the LMO films display highly non-uniform Bz(x,y), that is similar to the ZFC Bz(x,y), even in the fully magnetized state at fields much larger than the coercive field Hc. This finding shows that the SPM islands are well separated from each other with substantial gaps between the islands that are nonmagnetic or only weakly magnetic. This physical separation renders the magnetic islands to form an essentially non-interacting SPM system rather than an interacting spin glass state37.
Analysis of the SPM islands
The statistical analysis of N=8 u.c. sample in Fig. 3j shows that the magnetic islands have a typical moment of m≅1.5 × 104 μB, comparable to magnetic moments of common SPM nanoparticles36. By summing all the moments m of the flipped islands as a function of magnetic field, we find that the total in-plane moment and its saturation value Ms measured microscopically over a very small area (∼8 × 10−8 of the 5 × 5 mm2 sample area) well account for the global magnetization of the sample as shown in Fig. 3k. The reversal process of the individual nanoscale islands thus provides a quantitative description of the macroscopic magnetization behaviour of LMO/STO heterostructures.
Taking the experimental histogram of Fig. 3j, we simulate the ZFC and the fully magnetized state by random spatial distribution of non-overlapping islands with in-plane moments m oriented either randomly (Fig. 3e) or fully aligned (Fig. 3f–h) (see Methods section). The resulting Bz(x,y) in Fig. 3e–h closely describes the amplitude and the characteristic length scale of the ZFC state in Fig. 3a as well as of the non-uniform Bz(x,y) in the magnetized state in Fig. 3b–d, emphasizing the presence of well-separated magnetic islands.
Reversal events were observed predominantly along the horizontal and vertical axes (see Supplementary Note 3 and Supplementary Fig. 4). The in-plane magnetization thus shows fourfold anisotropy with easy axes along the LMO crystallographic direction that are locked to the underlying STO crystal structure.
Our local measurements are carried out at T=4.2 K well below the blocking temperature TB which can be estimated from the temperature dependence of the global magnetization (Supplementary Fig. 5). Therefore, the fast temporal SPM dynamics are expected to be suppressed, leading to hysteresis in d.c. magnetization measurements36 (Fig. 3k and Supplementary Fig. 1). To investigate the existence of slow dynamics, was abruptly raised and a sequence of Bz(x,y) images was acquired at 380 s intervals in N=6 u.c. sample at constant mT (Supplementary Movie 5). The corresponding ΔBz(x,y) images (Fig. 2e,f and Supplementary Movie 6) reveal the presence of a random moment reversal process following the fast field increase and leading to a slow relaxation of the overall magnetization. The rate of the moment relaxation dM/dt decays monotonically with time (Fig. 2g) as anticipated for tunnelling or thermal activation in a tilted potential. As in the case of the Bz(x,y) dependence on , the observation of the temporal process of uncorrelated nanoscale magnetization reversals is in sharp contrast with DW motion in FM films. Here the nanoscale relaxation process is a direct manifestation of the slow dynamics of SPM islands at T<TB.
Evaluation of the size of the SPM islands
Two possible doping mechanisms that may account for the magnetism in LMO/STO heterostructures will be discussed below: extrinsic bulk doping and surface charge reconstruction. We can estimate the characteristic size of the islands in these two cases assuming a magnetization of 4 μB per Mn atom and u.c. of 0.39 nm. In bulk LMO a spherical island with characteristic m=1.5 × 104 μB (Fig. 3j) should thus have a diameter of D=7.5 nm, which is larger than the thickness d=3.1 nm of the 8 u.c. sample. In thin films with extrinsic bulk doping we therefore expect the islands to have a disk-like shape extending from top to bottom surfaces resulting in characteristic island diameter of D=9.5 nm in the 8 u.c. film. In the charge reconstruction model, in contrast, the magnetism occurs only within a surface layer of thickness Ne. Taking Ne=2 u.c. for the 8 u.c. sample (see derivation below), results in characteristic diameter of D=19 nm. The top axis in Fig. 3j shows the distribution of the island diameters in this case. Since both bulk and surface mechanisms lead to island sizes that are smaller than our spatial resolution of ∼100 nm determined by the SOT diameter and the scanning height, our local magnetic imaging cannot directly discern the two models.
We now elaborate on the possible mechanisms that can lead to the formation of the observed SPM state. The Mn3+ ions, which are responsible for the LMO magnetism, have four 3d valence electrons in three low-energy t2g and one eg orbital19. The spin-aligned t2g electrons form a core spin of S=3/2, and the fourth electron, occupying the split eg orbitals, is slaved to the core spins by Hund’s coupling. The ground state is an A-type AFM Mott insulator with alternating planes of opposite magnetization of 4 μB per Mn atom19 (Supplementary Fig. 6). Hund’s coupling between the Mn core spins and eg electrons impedes hopping of any excess charges between AFM aligned sites, while FM alignment of the core spins allows excess charges to delocalize, thus lowering their kinetic energy19. Upon electron or hole doping, this double-exchange mechanism should therefore lead to a first-order phase transition from insulating AFM to metallic FM. At low doping, however, it has been shown that the energy of the system can be lowered by an electronic phase separation in which nanoscale FM islands are nucleated in the AFM matrix38. In particular, as derived in Supplementary Note 4 and shown in Supplementary Fig. 7, the phase separated state in LMO should be present for doping levels e per u.c., giving rise to metallic FM islands of 4–20 nm diameter containing an excess charge density . The observed SPM state could thus be a direct manifestation of the electronic phase separation due to low level of bulk carrier doping.
Bulk doping mechanism
In LMO films, excess carriers in the bulk of the film can be introduced extrinsically either by chemical doping, like in the case of Sr-doped LMO where magnetization reaching 3.5 μB per Mn (close to the theoretical value) was measured in La0.7Sr0.3MnO3 films39, or by excess oxygen (cation deficiency) incorporated during the growth process22,25,26,28. Since all the samples were grown under the same conditions, one would expect the magnetization per Mn atom due to extrinsic bulk doping to remain independent of the LMO thickness N. Figure 4a shows the saturation magnetization per Mn atom versus N (green). For N=4 and 5 u.c. the magnetization is very small, but then increases sharply at N=6 to 0.9 μB per Mn, reaching a maximum of 2.2 μB per Mn at N=24, followed by a drop to 0.85 μB per Mn at N=200. Such a highly nonmonotonic behaviour combined with the vanishing magnetization for N≤Nc essentially rules out uniform doping.
Alternatively, in highly doped La0.7Sr0.3MnO3 films there is experimental evidence39 for spatial separation into two stacked sheets: a dead layer of few u.c. at the bottom with no magnetization and uniformly magnetized live layers on top. Taking into account a dead layer of Nc=5, Fig. 4b shows the measured magnetization per Mn in the remaining N−Nc live layers. In contrast to the expected constant magnetization (dotted), the experimental data (blue) show a sharp onset of magnetization at N=Nc+1 with 5.4 μB per Mn that decays to 0.85 μB per Mn for N=200 u.c., which renders this possibility unlikely. In addition, the magnetization of our thickest sample sets an upper bound for the extrinsic bulk saturation magnetization in our samples. Then, one would expect the average magnetization of thinner films in presence of a dead layer to be always below this value and grow asymptotically as demonstrated by the dotted line in Fig. 4a. In contrast, among all films with N>Nc the smallest magnetization is found in the thickest sample (200 u.c.). Moreover, compared with previous systematic studies25,26, a bulk magnetization of 0.85 μB per Mn indicates that our films are stoichiometric with very low extrinsic doping consistent with our Rutherford Backscattering Spectrometry and Particle Induced X-ray Emission PIXE measurements (Li and Ariando—private communication).
Charge reconstruction model
Even though more complicated thickness-dependent effects including strain, growth defects and surface segregation could possibly give rise to nontrivial thickness dependence of the magnetization due to extrinsic doping, we propose here a simple alternative model. In the closely related LAO/STO heterostructures, electronic reconstruction driven by the polar catastrophe is believed to be responsible for a sharp onset of interface conductivity4. Since the LMO on TiO2-terminated STO has the same polar structure as of LAO/STO, a similar electronic reconstruction should be expected to occur also in LMO/STO heterostructures. Based on this analogy, Wang et al.27 recently proposed that a FM state forms at the LMO/STO interface above a critical thickness Nc. We expand here this approach and show that electronic reconstruction should in fact lead to a SPM rather than FM state.
Since the bandgap of LMO is smaller than that of STO, charge reconstruction leads to electron transfer from the top surface to the Mn orbitals at the LMO side of the LMO/STO interface27. The number of transferred electrons grows with N>Nc until it asymptotically reaches areal density of 0.5 excess electrons per u.c. (Fig. 5e). The double-exchange mechanism in the presence of excess electrons at the interface is expected to induce a transition from an insulating AFM (Fig. 5a) to a metallic FM state (Fig. 5b). Our calculation reveals, however, that a new ground state with spontaneous phase separation emerges (Supplementary Note 4 and Supplementary Fig. 8). In this state segregated nanoscale FM metallic islands of excess electrons with ρ≅0.17 e per u.c. are formed at the interface within the undoped insulating AFM matrix (Fig. 5c). The competition between kinetic energy, Coulomb interactions and the core spin exchange interaction determines the separation and size of the islands. Self-consistent calculation of the electrostatic potential shows that the metallic FM islands are confined to the vicinity of the interface, spreading over a finite thickness Ne of a few u.c. (Fig. 5e and Supplementary Fig. 9). For N=12, the islands reach D=20 nm and m=1.6 × 104 μB (Fig. 5f), which is in good agreement with the typical size and magnetic moment found in the experiment (Fig. 3j). Importantly, our model predicts that the phase separation occurs for all thicknesses (N>Nc) of LMO and the areal fraction of the magnetic islands remains below 1 (Fig. 5g). Since the islands are of nanometer size and well separated from each other, the system always remains in an insulating SPM state. Intriguingly, if the excess electrons at the LMO/STO interface originate from Mn orbitals at the LMO surface rather than from oxygen vacancies40,41, a double-layer of hole-doped and electron-doped islands will form as depicted in Fig. 5d.
In thin samples (N≤Nc) the weak magnetization arises from canting in the AFM phase19,42. Correspondingly, the low Bz(x,y) shown in Fig. 1a,b apparently originates from AFM domains with different canting orientations42. The electronic reconstruction at N>5 induces a transition into the SPM phase at the interfaces which results in a sharp onset of magnetization. Moreover, the regions between the SPM islands as well as the central part of the films remain AFM and should, therefore, contribute about 0.2 μB per u.c. due to canting in the AFM phase19,42. This picture is further supported by the temperature dependence of H/M (Supplementary Fig. 10). The magnetic susceptibility obeys Curie–Weiss law with extrapolated Θ that is lower than the actual transition temperature, which apparently arises from bulk AFM response23 modified by the presence of the SPM islands. The saturation magnetization in Fig. 4a (red) was calculated taking into account the double-layer SPM islands and the bulk AFM contribution of 0.2 μB per u.c. Since charge transfer to the interface increases monotonously with N up to 0.5 e per u.c. (Fig. 5e), the overall saturation magnetization increases as well, as shown in Fig. 1g (black). However, the relative contribution of the interface SPM to the average magnetization per Mn atom peaks at intermediate thicknesses in good agreement with the experimental data (Fig. 4a).
The contribution of the electronic reconstruction mechanism is expected to diminish in the limit of thick samples. Consequently, the deviation between the calculated and the measured magnetization in the thicker samples in Fig. 4a indicates the presence of additional bulk contribution to the magnetization. Indeed, in the general case of low doping the magnetism due to electronic reconstruction should coexist with bulk magnetism, leading to SPM islands residing both in the bulk of the LMO films and on the surfaces. Interestingly, although microscopic phase separation in bulk manganites has been discussed in the literature18,19,38,43,44, its consequence of forming a SPM state has not been considered. Hence the finding of SPM has broad implications on our comprehension of magnetic and transport properties of LMO. In particular, our results imply that a macroscopic FM state should be attainable only at high doping, while SPM should prevail over a wide range of intermediate doping levels. Since the blocking temperature TB of the SPM islands is rather high, the magnetization is hysteretic over a wide range of temperatures below TB, making the distinction between FM and SPM difficult based on global measurements. Furthermore, since a FM state is expected to be metallic, the SPM state in which nanoscale FM islands reside in an AFM matrix may provide the explanation for the existence of a FM insulating state in LMO films.
To conclude, the intriguing interplay of AFM, FM, and SPM and the controllable nanoscale phase separation provide the basis for novel physics and new functionalities in LMO/STO heterostructures. Our calculations show that a relatively small increase in carrier concentration can transform the insulating SPM into a conducting FM state opening the route to electric gate control of magnetism and magnetoresistance, with potential applications in magnetic recording and spintronics. LMO is thus an important addition to the oxide family of heterostructure materials offering novel possibilities for engineering of multifunctional multi-layers.
The magnetic imaging was performed using Pb SOT devices34, a typical effective diameter of ∼100 nm and white noise of ∼200 nΦ0 Hz−1/2 (see Supplementary Note 5, Supplementary Fig. 11 and Supplementary Table 1). The SOT was mounted in a home-built scanning probe microscope using a series SQUID array amplifier45 for signal readout. Scanning was performed using Attocube integrated xyz scanner with xy range of 30 μm and z range of 15 μm. To bias the SOT to a sensitive point, an out-of-plane field H was applied (see Supplementary Table 1). No influence of H on the sample response was observed. All the measurements were performed at 4.2 K in He exchange gas at ∼1 mbar. The pixel size of all the SOT images shown in the main text is 5 × 5 nm2 and the acquisition time was about 5 min per image.
The LMO films on TiO2-terminated single crystal STO (001) substrates were deposited by pulsed laser deposition from a polycrystalline LMO target in an oxygen partial pressure of 102 mbar at 750 °C by using 1.8 J cm−2 pulses at 248 nm with a repetition rate of 2 Hz. The STO substrates (CrysTec GmbH, Berlin) of 5 × 5 mm2 and 0.5 mm thickness were double side polished and chemically treated in buffered hydrofluoric acid and annealed at 950 °C in oxygen, resulting in singly terminated STO surface with atomically flat terraces of single STO unit-cell height and terrace width of ∼300 nm. The layer-by-layer growth of the films was monitored in situ using reflection high-energy electron diffraction and the samples were cooled to room temperature in oxygen at the deposition pressure. See Supplementary Fig. 12 for representative atomic force microscopy images of N=12 and 24 u.c. LMO films showing atomic-step terraces are preserved, demonstrating the layer-by-layer growth of the LMO thin films.
Global magnetization measurements of the samples were done using a Quantum Design magnetic properties measurement system vibrating sample magnetometer with temperature range of 2–300 K. The M–H loops of LMO films were obtained after subtraction of the STO diamagnetic background signal.
Simulations of Bz field distribution
To simulate the local field distribution Bz(x,y) in the SPM state, we use a random distribution of non-overlapping magnetic islands using the experimentally attained distribution of sizes and moments m in the 8 u.c. sample shown in Fig. 3j. Figure 3e shows the ZFC state in which the in-plane moment orientation was taken to be random along the x and y easy axes, as discussed in Supplementary Note 3. The shown Bz(x,y) was calculated using the experimental values of SOT diameter of 114 nm and scan height of 105 nm. The result of Fig. 3e compares well with the experimental data in Fig. 3a both in the size of characteristic features and in the span of Bz(x,y). Figure 3f shows Bz(x,y) of the same sample as in Fig. 3e but with all the moments oriented randomly either in the −x or −y directions to simulate the fully magnetized case at H>Hc applied at 225° with respect to the +x axis. In contrast to the FM case, in which a uniform field is attained at full magnetization, the resulting Bz(x,y) remains highly inhomogeneous because the SPM islands are well separated. Figure 3f shows that a fully magnetized SPM state displays Bz(x,y) that is similar to the ZFC state with a moderate reduction in the field span consistent with the experimental data in Fig. 3a–d. An SPM state fully magnetized in the +x and +y directions (Fig. 3g) results in Bz(x,y) that is identical to Fig. 3f but of opposite polarity, as observed experimentally in Fig. 3b,c. Similar result is attained by polarizing all the islands in the +x direction (Fig. 3h) albeit with slightly reduced field span since all the SPM island are oriented in a unique direction (+x) which is not case for Fig. 3f,g.
For each sample, a sequence of Bz(x,y) images was acquired, increasing in steps of 1 mT from 0 to 250 mT after sweeping the field from−250 mT. After numerically detecting and correcting the relative drifts in the xy plane, each pair of images was subtracted to obtain ΔBz(x,y) (Fig. 2c). Each dipole-like feature in ΔBz(x,y) is assumed to originate from a SPM island that reversed its in-plane magnetic moment oriented at an angle θ from−m to +m. The value of m is determined by the diameter D and thickness Ne (taken from theory in Fig. 5e) of the island using magnetization of 4 μB per Mn with lattice parameter of 0.39 nm. Fitting is then performed with D, θ and h as free parameters including a convolution with the SOT size (keeping the same Ne and SOT height h for all islands). Figure 2d shows an example of the fit result. Since D is smaller than h and the SOT diameter, the resulting ΔBz(x,y) is essentially described by a point-like in-plane magnetic moment m almost independent of its size D. Therefore, the choice of Ne (taken from theory) affects the derived D but has little effect on the derived value of m.
All relevant data are available on request, which should be addressed to Y.A., Ariando or E.Z.
How to cite this article: Anahory, Y. et al. Emergent nanoscale superparamagnetism at oxide interfaces. Nat. Commun. 7:12566 doi: 10.1038/ncomms12566 (2016).
Ohtomo, A. & Hwang, H. Y. A high-mobility electron gas at the LaAlO3/SrTiO3 heterointerface. Nature 427, 423–426 (2004).
Reyren, N. et al. Superconducting interfaces between insulating oxides. Science 317, 1196–1199 (2007).
Mannhart, J. & Schlom, D. G. Oxide interfaces–an opportunity for electronics. Science 327, 1607–1611 (2010).
Hwang, H. Y. et al. Emergent phenomena at oxide interfaces. Nat. Mater. 11, 103–113 (2012).
Sulpizio, J. A., Ilani, S., Irvin, P. & Levy, J. Nanoscale phenomena in oxide heterostructures. Annu. Rev. Mater. Res. 44, 117–149 (2014).
Junquera, J. & Ghosez, P. Critical thickness for ferroelectricity in perovskite ultrathin films. Nature 422, 506–509 (2003).
Thiel, S., Hammerl, G., Schmehl, A., Schneider, C. W. & Mannhart, J. Tunable quasi-two-dimensional electron gases in oxide heterostructures. Science 313, 1942–1945 (2006).
Boris, A. V. et al. Dimensionality control of electronic phase transitions in nickel-oxide superlattices. Science 332, 937–940 (2011).
Okamoto, S. & Millis, A. J. Electronic reconstruction at an interface between a Mott insulator and a band insulator. Nature 428, 630–633 (2004).
Brinkman, A. et al. Magnetic effects at the interface between non-magnetic oxides. Nat. Mater. 6, 493–496 (2007).
Ariando, et al. Electronic phase separation at the LaAlO3/SrTiO3 interface. Nat. Commun. 2, 188 (2011).
Kalisky, B. et al. Critical thickness for ferromagnetism in LaAlO3/SrTiO3 heterostructures. Nat. Commun. 3, 922 (2012).
Bi, F. et al. Room-temperature electronically-controlled ferromagnetism at the LaAlO3/SrTiO3 interface. Nat. Commun. 5, 5019 (2014).
Bert, J. A. et al. Direct imaging of the coexistence of ferromagnetism and superconductivity at the LaAlO3/SrTiO3 interface. Nat. Phys. 7, 767–771 (2011).
Li, L., Richter, C., Mannhart, J. & Ashoori, R. C. Coexistence of magnetic order and two-dimensional superconductivity at LaAlO3/SrTiO3 interfaces. Nat. Phys. 7, 762–766 (2011).
Ben Shalom, M., Sachs, M., Rakhmilevitch, D., Palevski, A. & Dagan, Y. Tuning spin–orbit coupling and superconductivity at the SrTiO3/LaAlO3 interface: a magnetotransport study. Phys. Rev. Lett. 104, 126802 (2010).
Caviglia, A. D. et al. Electric field control of the LaAlO3/SrTiO3 interface ground state. Nature 456, 624–627 (2008).
Moreo, A., Yunoki, S. & Dagotto, E. The phases separation scenario for manganese oxides. Science 283, 2034–2040 (1999).
Salamon, M. B. & Jaime, M. The physics of manganites: structure and transport. Rev. Mod. Phys. 73, 583–628 (2001).
Coey, J. M. D., Viret, M. & von Molnár, S. Mixed-valence manganites. Adv. Phys. 48, 167–293 (1999).
Van Roosmalen, J. A. M., Cordfunke, E. H. P., Helmholdt, R. B. & Zandbergen, H. W. The defect chemistry of LaMnO3±δ: 2. Structural aspects of LaMnO3+δ . J. Solid State Chem. 110, 100–105 (1994).
Huang, Q. et al. Structure and magnetic order in undoped lanthanum manganite. Phys. Rev. B 55, 14987–14999 (1997).
Prado, F., Sánchez, R. D., Caneiro, A., Causa, M. T. & Tovar, M. Discontinuous evolution of the highly distorted orthorhombic structure and the magnetic order in LaMnO3±δ perovskite. J. Solid State Chem. 146, 418–427 (1999).
Gupta, A. et al. Growth and giant magnetoresistance properties of La-deficient LaxMnO3−(0.67<x<1) films. Appl. Phys. Lett. 67, 3494 (1995).
Choi, W. S. et al. Effects of oxygen-reducing atmosphere annealing on LaMnO3 epitaxial thin films. J. Phys. D: Appl. Phys. 42, 165401 (2009).
Kim, H. S. & Christen, H. M. Controlling the magnetic properties of LaMnO3 thin films on SrTiO3(100) by deposition in a O2/Ar gas mixture. J. Phys. Condens. Matter 22, 146007 (2010).
Wang, X. R. et al. Imaging and control of ferromagnetism in LaMnO3/SrTiO3 heterostructures. Science 349, 716–719 (2015).
Marton, Z. A., Seo, S. S., Egami, T. & Lee, H. N. Growth control of stoichiometry in LaMnO3 epitaxial thin films by pulsed laser deposition. J. Cryst. Growth 312, 2923–2927 (2010).
Hou, Y. S., Xiang, H. J. & Gong, X. G. Intrinsic insulating ferromagnetism in manganese oxide thin films. Phys. Rev. B 89, 064415 (2014).
Zhai, X., Mohapatra, C. S., Shah, A. B., Zuo, J.-M. & Eckstein, J. N. Magnetic properties of the (LaMnO3)N/(SrTiO3)N atomic layer superlattices. J. Appl. Phys. 113, 173913 (2013).
Garcia-Barriocanal, J. et al. Spin and orbital Ti magnetism at LaMnO3/SrTiO3 interfaces. Nat. Commun. 1, 82 (2010).
Gibert, M., Zubko, P., Scherwitzl, R., Íñiguez, J. & Triscone, J.-M. Exchange bias in LaNiO3–LaMnO3 superlattices. Nat. Mater. 11, 195–198 (2012).
Salluzzo, M. et al. Origin of interface magnetism in BiMnO3/SrTiO3 and LaAlO3/SrTiO3 heterostructures. Phys. Rev. Lett. 111, 087204 (2013).
Vasyukov, D. et al. A scanning superconducting quantum interference device with single electron spin sensitivity. Nat. Nanotechnol. 8, 639–644 (2013).
Finkler, A. et al. Self-aligned nanoscale SQUID on a tip. Nano Lett. 10, 1046–1049 (2010).
Goya, G. F., Berquó, T. S., Fonseca, F. C. & Morales, M. P. Static and dynamic magnetic properties of spherical magnetite nanoparticles. J. Appl. Phys. 94, 3520–3528 (2003).
Binder, K. & Young, A. P. Spin glasses: experimental facts, theoretical concepts, and open questions. Rev. Mod. Phys. 58, 801–976 (1986).
Dagotto, E. Nanoscale Phase Separation and Colossal Magnetoresistance Springer (2003).
Huijben, M. et al. Critical thickness and orbital ordering in ultrathin La0.7Sr0.3MnO3 films. Phys. Rev. B 78, 094413 (2008).
Liu, Z. Q. et al. Origin of the two-dimensional electron gas at LaAlO3/SrTiO3 interfaces: the role of oxygen vacancies and electronic reconstruction. Phys. Rev. X 3, 021010 (2013).
Yu, L. & Zunger, A. A polarity-induced defect mechanism for conductivity and magnetism at polar–nonpolar oxide interfaces. Nat. Commun. 5, 5118 (2014).
Skumryev, V., Ott, F. & Coey, J. M. D. Weak ferromagnetism in LaMnO3 . Eur. Phys. J. B 406, 401–406 (1999).
Nagaev, E. L. New type of self-localization state of carriers in an antiferromagnetic semiconductor. Pis’ma Zh. Eksp. Teor. Fiz. 55, 646–648 (1992).
Kagan, M. Y. & Kugel, K. I. Inhomogeneous charge distributions and phase separation in manganites. Physics-Uspekhi 44, 553–570 (2001).
Huber, M. E. et al. DC SQUID series array amplifiers with 120 MHz bandwidth. IEEE Trans. Appl. Supercond. 11, 1251–1256 (2001).
We thank E. Altman, J.M.D. Coey, X. Renshaw Wang and L.V. Weiming for fruitful discussions. This work was supported by the Minerva Foundation with funding from the Federal German Ministry of Education and Research, by the Israel Science Foundation (Grant No. 132/14), and by Rosa and Emilio Segré Research Award. E.Z. acknowledges support by US-Israel Binational Science Foundation (BSF), Jerusalem, Israel, and the US National Science Foundation (NSF) research Grant 2015653 NSF/DMR-BSF. The work at NUS was supported by the Singapore National Research Foundation (NRF) under the Competitive Research Programs (CRP Award Nos. NRF-CRP 8-2011-06, NRF-CRP10-2012-02, and NRF-CRP15-2015-01) and the NUS FRC (AcRF Tier 1 Grant Nos. R-144-000-346-112 and R-144-000-364-112). Y.A. acknowledges support by the Azrieli Foundation and by the Fonds Québécois de la Recherche sur la Nature et les Technologies.
The authors declare no competing financial interests.
Supplementary Figures 1-12, Supplementary Table 1, Supplementary Notes 1-5 and Supplementary References (PDF 2450 kb)
Supplementary Movie 1
Supplementary Movie 1 shows a sequence of 1.5 × 1.5 μm2 Bz(x,y) images in the N=8 u.c. sample acquired upon increasing μ0H‖set from 0 to 150 mT in steps of 1 mT applied at θ=52° relative to the x axis (and the  STO direction) after full magnetization of the sample at -250 mT. The first frames of the movie mainly show the instrumental x,y drift arising from application of H‖. With increasing μ0H‖set subtle changes in Bz(x,y) at random locations begin to be visible. These changes grow significantly on approaching Hc ≈ 95 mT followed by reduction in the changes at higher fields. Note that the Bz(x,y) images at the beginning and at the end of the movie are practically inverted, indicating that all the SPM islands have fully reversed their moments. (MOV 4564 kb)
Supplementary Movie 2
Supplementary Movie 2 shows a similar process in the N=12 u.c. sample upon increasing μ0H‖set from 0 to 250 mT at θ=7°. After the initial drift, random small changes become visible. Our maximal in-plane field of 250 mT is, however, insufficient to reach a full inversion of all the SPM islands. (MOV 3072 kb)
Supplementary Movie 3
The corresponding ΔBz(x,y) images in the N=12 u.c. sample are shown in Supplementary Movie 3 for μ0H‖set from 125 to 250 mT obtained by subtraction of consecutive images in Supplementary Movie 2 (note an order of magnitude smaller colour bar span). Randomly-appearing dipole-like features show the magnetization reversal process of SPM islands. Most of the dipole-like features are oriented close to the x direction along the easy magnetization axis of  STO. (MOV 2161 kb)
Supplementary Movie 4
Supplementary Movie 4 shows the x,y coordinates of the SPM island reversal events (after drift correction) in the N = 8 u.c. sample as H‖set is increased. The events show random uncorrelated behaviour consistent with the SPM state. The compilation of all the locations is presented in Fig. 3i. (MOV 1808 kb)
Supplementary Movie 5
The thermally activated process of the magnetic reversal of the SPM islands is presented in Supplementary Movies 5 and 6 of N = 6 u.c. sample. The in-plane field was rapidly ramped to 80 mT and a sequence of Bz(x,y) images (Supplementary Movie 5) was acquired at a constant μ0H‖ = 80 mT for about 1.5 h. The acquisition time of each image was 360 sec with 20 sec interval between the images. (MOV 1108 kb)
Supplementary Movie 6
The sequence of ΔBz(x,y) images (Supplementary Movie 6) is attained by subtraction of consecutive Bz(x,y) images. The dipole-like features in Supplementary Movie 6 show that following the rapid increase in μ0H‖ the islands continue to reverse their moments predominantly in the direction of μ0H‖ for an extended period of time through a thermally activated process. The number of the reversal events decays with time as seen in Supplementary Movie 6. The relaxation rate of the total in-plane magnetic moment dM/dt in the scanned area presented in Fig. 2g is obtained by vectorial summation of the reversing moments m along H‖ direction for each frame of Supplementary Movie 6. (MOV 673 kb)
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Anahory, Y., Embon, L., Li, C. et al. Emergent nanoscale superparamagnetism at oxide interfaces. Nat Commun 7, 12566 (2016). https://doi.org/10.1038/ncomms12566
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