Ferroelectric materials are heavily used in electro-mechanics and electronics. Inside the ferroelectric, domain walls separate regions in which the spontaneous polarization is differently oriented. Properties of ferroelectric domain walls can differ from those of the domains themselves, leading to new exploitable phenomena. Even more exciting is that a non-ferroelectric material may have domain boundaries that are ferroelectric. Many materials possess translational antiphase boundaries. Such boundaries could be interesting entities to carry information if they were ferroelectric. Here we show first that antiphase boundaries in antiferroelectrics may possess ferroelectricity. We then identify these boundaries in the classical antiferroelectric lead zirconate and evidence their polarity by electron microscopy using negative spherical-aberration imaging technique. Ab initio modelling confirms the polar bi-stable nature of the walls. Ferroelectric antiphase boundaries could make high-density non-volatile memory; in comparison with the magnetic domain wall memory, they do not require current for operation and are an order of magnitude thinner.
Domain boundaries make an intriguing and challenging research subject because of their peculiar properties and promising perspective in designing nanoelectronic devices. One typical paradigm is the discovery of electronic conductivity at ferroelectric domain walls in multiferroic oxides such as BiFeO3 (refs 1, 2, 3) and ErMnO3 (ref. 4). Charged domain walls in the ubiquitous ferroelectric BaTiO3 showed electron-gas-like conductivity while the individual domains remained excellent insulators5. Large photovoltages were generated by domain walls, attractive for photovoltaic devices6. These properties are particularly attractive because domain walls can be created, annihilated, rewritten and displaced electrically inside the material, potentially leading to agile nanoelectronics.
Recently, the polarity of twin boundaries in centrosymmetric CaTiO3 was shown7. Possible polarity of domain boundaries in nonpolar materials and, to a greater extent, local ferroelectricity in such boundaries make these objects attractive for both fundamental science and possible practical future applications.
How to identify materials with ferroelectric boundaries? Here based on a Landau theory treatment, we argue that antiphase boundaries in antiferroelectrics are likely to be ferroelectric. Implementing this result, we perform an atomic-scale study of the prototypical antiferroelectric lead zirconate PbZrO3 (PZ), using negative spherical-aberration imaging (NCSI) technique8 in an aberration-corrected transmission electron microscope (TEM) and demonstrate that antiphase boundaries with a π phase shift of the order parameter exhibit polarity, which, in view of the symmetry of the system, implies the existence of local ferroelectricity.
Ferroelectricity in antiferroelectric domain walls
Antiferroelectrics constitute a large group of dielectric materials that can be experimentally recognized by a structural phase transition between two nonpolar phases with a strong dielectric anomaly at the high temperature side of the transition9,10,11. Antiferroelectricity is a result of the interruption of an imminent ferroelectric phase transition having Curie temperature of T0 by a structural phase transition12 at a slightly higher temperature TA. This interruption occurs because of repulsive interaction between polarization and a structural order parameter appearing at TA.
A simple two instabilities Landau-type theory12,13,14,15 rationalizes the antiferroelectric behaviour using the following free energy expansion in terms of polarization, P, and structural order parameter, ξ,
A>0, and T0 is the Curie-Weiss temperature of the dielectric anomaly (see Supplementary Note 1 for more details on the two-instability theory of antiferroelectricity). Here the coefficient η>0 controls the repulsive biquadratic coupling between polarization and structural order parameter. The transition at TA is described by the contribution to the free energy FA(ξ), implying softening of a lattice mode associated with the order parameter ξ. For the low-temperature phase where the order parameter of the transition, ξ, acquires a spontaneous value of ξ0, the susceptibility, defined as , takes the form
Equation (2) corresponds to antiferroelectric-type anomaly if increases on cooling. This is possible if the increase in ξ0 with lowering temperature dominates the behaviour of this term, which can be assured by large enough coupling constant η.
The above scenario suggests that domain boundaries provide favourable conditions for the development of local ferroelectricity. This can be elucidated considering the simplest type of ferroic domain boundary, the so-called Ising wall. In such wall, the order parameter ξ passes through zero in the middle of the boundary. Thus, in the middle of the boundary, the suppressing effect of the structural ordering (with respect to the ξ parameter) on the ferroelectric instability vanishes, creating favourable conditions for the development of local ferroelectricity at T<T0.
Antiphase boundaries in PZ as candidates for ferroelectricity
The concept presented above can be applied to PZ. However, in PZ the situation is more complicated. At high temperatures, PZ has the ideal cubic perovskite structure shown in Fig. 1a. After cooling through a first-order phase transition at TA~500 K, the structure changes from cubic to orthorhombic mmm. The structural changes at the transition can be presented as a combination of displacements in two lattice modes16, one corresponding to the point (the wave vector ; ac is the lattice constant of the high-temperature cubic phase) in the Brillouin zone and the other corresponding to the R point (). The distortions associated with the point are mainly related to displacements of lead ions (Fig. 1b), while those associated with the R point derive from antiphase rotations of the oxygen octahedra (Fig. 1c) about the crystallographic axes of the cubic phase. Thus, the transition is governed by a mixed order parameter, containing -point and R-point-related components.
The possibility of local ferroelectricity in domain boundaries can be discussed referring to the -point-related component of the order parameter, corresponding to the so-called mode of the parent cubic structure, with lead displacements having the form12,17
where xc=n1ac, yc=n2ac (n1 and n2 are integers) are the coordinates in the cubic lattice frame and φ is the phase of the modulation.
The condensation of the order parameter linked to this mode is associated with a fourfold increase in the number of atoms per unit cell as schematically depicted in Fig. 1b. As a result, two types of domain states form: orientational and translational18. The orientational states (ferroelastic twins) differ by the orientation of the atomic displacements. The translational domain states that correspond to a given orientational state can be turned from one to another by shifting the lattice by ac, 2ac or 3ac, corresponding to a fraction of a lattice translation vector of the low-temperature phase. In view of the quadrupling of the unit cell, there are four translational domain states for each orientational state. In terms of Equation (3), lead displacements in these states correspond to φ=π/4, 3π/4, 5π/4 and 7π/4 (ref. 12). These states can be visualized in the plane of the complex order parameter ξ=ρeiφ, corresponding to the points marked with four circles (Fig. 2a), where φ is the phase of the order parameter and ρ is its modulus, proportional to the magnitude of lead displacements.
Three types of translational boundaries, corresponding to phase shifts of π/2, π and 3π/2 can separate the four translational states. The possible mappings of these translational boundaries are schematically shown in Fig. 2a with solid lines. Mapping ‘3’ is of a particular interest for the appearance of the local ferroelectricity. It corresponds to a π-wall (so-called antiphase boundary (APB))—that is, having a phase shift of π, at the middle of which the order parameter passes through the zero point hence the suppressing effect of the order parameter on the ferroelectric instability is reduced. Following this argument one might contemplate a π/2 translational domain boundary where the order parameter passes as well through zero (mapping ‘2’ in Fig. 2b) and wonder whether also in this case the ferroelectric instability is favoured. No theory of translational domain boundaries in PZ is available at present to quantitatively address this problem. However, such a problem has been addressed for an improper ferroelectric by Fouskova and Fousek19. These authors compared the energies of two variants of a domain wall in gadolinium molibdate (GMO), which have mapping on the plane of the two-component order parameter (q1, q2) marked with lines ‘1’ and ‘2’ in Fig. 2b. They demonstrated that the variant corresponding to mapping ‘2’, which passes through the origin is energetically unfavourable compared with the rotational variant, corresponding to mapping ‘1’. The problem in GMO is isomorphous to that in PZ to within the substitution (Re ξ, Im ξ) for (q1, q2). The results obtained for GMO enable us to speculate that passing through zero of the order parameter in a π/2 translational domain boundary in PZ is quite improbable. On the same lines, we argue that in orientational (twin) domain boundaries, which are also comparable to the walls treated by Fousek and Fouskova19, the order parameter is not expected to pass through zero in the wall neither. This implies that there is no special reason for the appearance of local ferroelectricity in twin boundaries, although such event cannot be excluded. It is therefore the π wall that is promising for the local ferroelectricity. We propose that APBs in PZ—that is, translational boundaries with phase shifts of π—are good candidates for the occurrence of local ferroelectricity.
The thickness of APBs in ferroics
The above discussion motivates experimental search for ferroelectricity in APBs in PZ. For such research, it seems appropriate to specify the notion APB in ferroics, which is not fully identical to that commonly used in non-ferroic materials.
By definition, any two elementary unit cells in a perfect crystalline structure can be superimposed by translation with an elementary vector belonging to the set of the lattice translation vectors of the structure. Some crystals exhibit distinct neighbouring regions, where a unit cell in one can superimpose a unit cell in the other by the application of a vector differing from an allowed lattice translation vector by approximately half of an elementary lattice translation vector. In this case, the boundary separating the two regions is called APB. Hereafter, the aforementioned translation vector is called an APB vector. We term this primary definition of the APB definition-0.
Figure 3a shows a two-dimensional (2D) schematic of an APB. Here only one chain of atoms parallel to the Ox direction is shown and the whole 2D ‘crystal’ can be obtained by repeating the chain in the Oy direction with a period c. In this drawing, the APB vector differs from a lattice translation vector exactly by a/2—that is, by a half of the elementary translation vector. In a more realistic model, the separation between the neighbouring ‘atoms’ in the Ox directions should be a/2 only inside regions of ‘domain I’ and ‘domain II’ of the structure, while at the APB it should evidently be slightly different from this value.
For the model depicted in Fig. 3b, another definition of the APB (termed hereafter definition-1) can be introduced based on definition-0 given above. Specifically, it is seen that the regions ‘I’ and ‘II’ can be characterized by the alternation of the signs of the atomic displacements along the Oy direction, which are either b or −b. As is clear from Fig. 3a, one can identify the presence of the APB by a shift of the phase of this alienation and ascribe the position of the APB to the place where this phase shift takes place. For the model depicted in Fig. 3a, the APB can be viewed as a layer that is a/2 thick in the Ox direction. In terms of definition-0, by removing away this layer, the periodicity throughout the whole system, which was violated by the presence of the APB, is restored. In terms of definition-1, at this layer, the regular alternation of the atomic displacements in the Ox direction is violated. On the basis of any of the two definitions, we can attribute to the APB the width of a and speak about its location with the accuracy of the interatomic distance. Definition-1 is more convenient in practical work compared with definition-0.
The model depicted in Fig. 3a corresponds to the situation in non-ferroic crystals. Meanwhile, for ferroics, that situation is, in general, different and requires a special treatment. The new features are as follows: (i) definition-1 is not consistent any more with the primary definition-0, and (ii) a thickness equal to the correlation length rather than the interatomic distance should be ascribed to the APB. This situation is discussed next.
In ferroics, APBs occur once a structural phase transition is accompanied with a unit cell multiplication. Figure 3b shows the evolution of the structure at such a phase transition in a ferroic ‘material’ where the unit cell volume is doubled at the transition and the period in the Ox direction changes from a/2 to a. Specifically, the structural evolution shown in this figure corresponds to the case, where, in the ordered phase, the structure is in a single domain state. It is seen that such single domain structure is equivalent to that inside regions ‘I’ and ‘II’ of the non-ferroic 2D crystal shown in Fig. 3a.
In such a ferroic 2D crystal, APBs may readily occur, separating between so-called translational domains. Specifically, for a ferroic having a second-order phase transition or of a first order close to the second-order transition (the typical situation that enables the Landau theory treatment), in an APB, the structure evolves gradually between the two translational domains on a spatial scale of about the correlation length ζ. The primary statement of the Landau theory is that ζ is much larger than the lattice constant of the material. In practice, because of an interplay of numerical factors such difference may not be very large; however, conceptually, ζ should be larger than the lattice constant. A ferroic ‘material’ exhibiting two translational domains marked with ‘I’ and ‘II’, which are separated by an APB, is schematically depicted in Fig. 3c.
We now pose the question of the thickness and position of a ferroic APB. Using definition-0, one treats the APB as the area different from the translational invariant domains ‘I’ and ‘II’. Note that the translational invariance requires not only the periodicity in the Ox direction but also the identity of the atomic displacements in the Oy direction. Thus, we consider the APB as an object having the thickness w3≅ζ. The APB is the whole region, with the thickness of about ζ, where the lattice periodicity is violated. Once the APB contains many distorted unit cells, one can say that, in an APB, the modulus of the order parameter deviates from its bulk value.
Can one apply definition-1 to an APB in ferroics? In definition-1, we considered the APB to be atomically thin (in Fig. 3c it is w2) and specified its location to within the interatomic distance. However, in ferroics this definition loses its essential feature. Specifically, in non-ferroics definition-1 is equivalent to the primary definition-0. On the contrary, in ferroics, definition-1 is in conflict with the primary definition-0. In a ferroic material, two unit cells separated just by the APB of definition-1 cannot be superimposed by any translational vector at all; thus, it is impossible to speak about a phase shift at it. Thus, strictly speaking, when applied to ferroics, definition-1 of the APB does not correspond to the term ‘APB’ itself.
To summarize, APBs in ferroics are objects of a finite volume, not just a stepwise break of the periodicity.
Following the above analysis, we investigated PZ to search for local polarity in its domain boundaries. Employing the NCSI technique8 in an aberration-corrected TEM combined with quantum mechanical and optical simulation, we imaged and measured the atomic positions, including those of oxygen.
Figure 4a is a dark-field image of a PZ crystal, showing translational domains separated by domain walls (dark line contrast). These translational domains correspond to a single orientational domain. The topological nature of the domain walls allows reactions between them, provided the conservation of the total phase shift (topological charge) is kept. Encircled and marked ‘1’, ‘2’ and ‘3’ are annihilation of two APBs, annihilation of one APB and two π/2 walls and split of an APB into two π/2 walls, respectively.
A high-resolution TEM image of an APB is shown in Fig. 4b. It was recorded under NCSI condition with the electron beam along the crystallographic  direction. One readily checks that the two highlighted unit cells exhibit a π shift in the phase of the order parameter. The identity of these two unit cells can be checked with lead displacements. Passing a pair of rows in the  direction, the sign of lead displacements alternates as shown with the blue/pink arrows in Fig. 4b, following the law of the alienation dictated by Equation (3). The number of lead-containing rows between the two highlighted unit cells is 10 (and not a multiple of 4), evidencing the π phase shift and the existence of the APB region. On the basis of image simulation, the atomic positions corresponding to the experimental image are obtained from the model structure.
A violation of the correlation in the antipolar in-plane Pb displacements is clearly seen in the APB area (Fig. 4c). Owing to the depolarizing effect, polarity is expected only in the boundary plane—that is, along the  orthorhombic axis. Scrutinizing the x-atomic displacements shown in Fig. 4d, we find a systematic unipolar displacements of Zr in 7 elementary cubes (pseudocubic unit cells) with an average value of about 8 pm. This hints to a dipole moment inside the wall, having a dipole moment density of about 11 μC cm−2, obtained taking ac=0.413 nm and six electron charges for the Zr Born charge (see Supplementary Note 2). Details about oxygen displacements are provided in Methods. Re-arrangement of the oxygen atomic positions at the APB area clearly reveals breaking of the antiphase-correlated rotation of the octahedra. Within the accuracy of the experiments, width of the APB can be evaluated as one to two orthorhombic unit cells along the  direction.
To evaluate the polarity of the APB we used the following approach: we calculated the dipole moments based on the displacements of all the ions from their positions in the cubic phase associated with their Born charges. Then, we averaged these moments over the projection of the orthorhombic unit cell on the ab plane using a ‘sliding’ unit cell (see Methods). Figure 4e shows the dipole moment density obtained this way, as a function of the centre of the sliding unit cells. Note that this figure shows a deviation from zero polarity in the centrosymmetric domain bulk. This deviation indicates the measurement errors (s.d. σ<5 μC cm−2) of the polarization calculated this way. This relatively low accuracy is not surprizing when calculating the dipole moments of a 40-atom unit cell of the orthorhombic PZ. Importantly, one can ascribe in-plane polarity to the APB area, corresponding to some 14 μC cm−2, definitely exceeding the ‘noise’ level. The contribution of B-site to the polarity in the wall can be taken as an indication that the B-site atoms contribute to the ferroelectric soft mode of the material. From Fig. 4e, it is also clear that no polarity normal to the boundary can be ascribed to APB, which is consistent with the expected manifestation of the depolarizing effect.
The presence of local polarity in the APB in PZ was also investigated by first principles calculations (Supplementary Note 2). The results confirmed the observed polarity and agreed qualitatively with the experimental results. The corresponding atom displacements and polarity are shown in Fig. 5. Using ab initio results we have estimated the surface formation energy of the considered here π-wall as 190 mJ m−2. Our simulations also demonstate the bi-stability of the polar state of APBs in PZ.
Thus, the electron microscopy results provide experimental evidence for the anticipated polarity in APBs in the centrosymmetric PZ and the ab initio calculations give a further support to the experimental observations. As the observed polarity is the result of spontaneous symmetry breaking, the phenomenon observed at the APB is a signature of local ferroelectricity. This is supported by first principle calculations that reveals the bi-stability of the polarity at the APB. Although the switchability of the polarity was not demonstrated experimentally, the moderate values of the spontaneous polarization found in the APB suggest moderate values of its thermodynamic coercive field, which behaves as the cube of spontaneous polarization18, promising that the polarity is not only bi-stable but also switchable.
It is worth pointing out the qualitative difference between the phenomenon reported here and a scenario for magnetism in a domain boundary in an antiferromagnet. Roughly speaking, the antiferromagnetic ordering is a result of negative exchange interaction between the spins of the system. In antiferromagnetic walls, the exchange interaction may change the sign leading to a local ferromagnetic ordering, the order made by the same spins that are interacting in an antiferromagnetic way in the domains themselves. In our case, the ‘antipolar’ displacements inside the domains are mainly associated with the A-site (Pb) ions, whereas the polarity in the wall is driven by all the atoms: the A-site (Pb), B-site (Zr) atom and oxygens. This is consistent with the two-mode scenario for antiferroelectricity and is different from the mechanisms controlling antiferromagnetism.
The polar antiphase domain boundaries reported above are expected to be bi-stable and mobile. The bi-stability of polar domain walls in a nonpolar material is readily expected in view of the symmetry arguments. Understanding the mobility of the APBs is less evident. Since translational domains are identical in terms of all materials tensors no macroscopic stimulus can lift the energy degeneracy of the domains. However, under electric field, E, the dipole moment density in the wall is associated with the energy density −PE. This implies force acting on the wall once the electric field is inhomogeneous,—for example, when electric field gradient is applied across the wall.
Ferroelectric antiphase domain boundaries in antiferroelectrics can be viewed as functional elements, 1–10 nm wide, which carry information. Unlike twin domain walls, the polar translational walls are non-ferroelastic, which makes them strain-free, and thus even more appealing for potential information-carrying elements. In comparison with the attractive magnetic domain wall memory20, they do not require current for operation and are an order of magnitude thinner, thus adding potentially a new element for future high-density information storage.
Lead–zirconate crystals were grown by flux method. The PbO–B2O3 mixture (soaking at 1,050 K) was used as a solvent. The temperature of the melt was reduced at a rate 2 K h−1 down to 850 K. The remaining melt decanted and attached to the crucible walls were cooled to room temperature at a rate of 10 K h−1. Then, the crystals were etched in dilute acetic acid to remove residues of the solidified flux.
The TEM specimens were prepared using focused ion beam system. To remove the contamination and the damaged layers, plasma cleaning and NanoMill Model 1040 system operated at 500 V were used to clean and mill the lamella samples. The lamella samples were heated above TA and then cooled at ≈9 K min−1 to recover the orthorhombic phase at the thin edges. The TEM investigation was performed on an FEI Titan 80–300 microscope with a Cs corrector for the objective lens. The available point resolution was better than 0.08 nm at an operating voltage of 300 kV. The experimental image was filtered to minimize the effect of contrast noise. Structure modelling and image simulation were carried out using the CrystalKit-MacTempas software package.
The experimental image filtered using a special method21 was quantified in the following way. First, a least-square fit was performed by 2D Gaussian profiles to each of the individual intensity maxima of image that corresponds to the positions of atomic columns. On the basis of this, a transverse averaging of the shifts of each column species with respect to the cubic structure was plotted as a function of the vertical distance of Fig. 6a; the mean error is <5.6 pm for heavy Pb and Zr/O1/O2 columns and <10.6 pm for light oxygen columns with a confidence level of 95%. Second, for picometer precision measurements, the residual objective-lens aberrations and unavoidable tilting of the crystallographic zone axis away from the incident electron beam were examined in the image simulation to remove the deviation of the positions of contrast maxima in the image from the real atomic positions. For this, a procedure of iterative comparison of the calculated images with the experimental image was carried out through adjusting the image parameters on the basis of a perfect domain region in the experimental image until the best fit between the calculated and the experimental images was obtained. The used imaging parameters for the calculated image with the best fit were thus determined as the parameters used in the experiment. Afterwards, a structural model containing the APB was constructed for the image simulations based on the determined imaging conditions. An additional procedure of iterative comparison of the calculated images with the experimental image was carried out through adjusting the interfacial widths and the atomic positions near the boundary until the experimental image was best fitted by the calculated one. The structure model leading to the calculated image with the best fit to the experimental one provides the real atom positions at the APB area. The filtered experimental image and the simulated image with excellent match are shown in Fig. 6a,b.
In the orthorhombic unit cell of PZ, oxygen atoms have five different crystallographic sites and lead atoms have two (Fig. 6c). Since the Pb1 (yellow) and Pb2 (light-blue below the yellow) overlap along the viewing direction and so do the O1, Zr and O2 atoms, the indistinguishable Pb1/Pb2 and O1/Zr/O2 atomic columns are moved as rigid entities in our image simulation. For clarity sake, the atomic position difference between Pb1 and Pb2 is not mentioned in the main text, and Fig. 3c presents the average atomic shifts of Pb1 and Pb2 derived from the final structural model. The displacements of overlapped O1 and O2 are summed up and shown in Fig. 7a. Ideally, there are no displacements for O4 and O5 atoms in the perfect domain region. Considering the antiphase rotation of the corner-linked octahedra, the displacements of O3, O4 and O5 atoms, which are directly observed in the experimental image, are also summed up to show the rotation behaviour of the octahedral (Fig. 7b). Note that in Fig. 7a,b, the displacement sums along x/y direction (/) are enhanced/reduced because of the same/opposite displacement directions of (O1 and O2)/O3 atoms, as clearly seen in Fig. 6c. In addition to the displacement values, re-arrangement of the oxygen atomic positions near the APB area reveals breaking of the antiphase-correlated rotation of the octahedra. The spontaneous polarization was calculated using the following formula:
where V, δi and Zi are the volume of the orthorhombic unit cell, displacement of atom i along the x or y direction from atomic positions of the centrosymmetric cubic perovskite structure and the effective charge of atom i. According to first-principles density-functional calculations on orthorhombic PbZrO3, the effective charges used in our calculation are ZPb=3.9, ZZr=6.0, ZO1,O2=−2.5, ZO3,O4,O5=−3.7 (see Supplementary Note 2). The spontaneous polarity for a sliding orthorhombic cell was calculated by atom displacements with respect to the cubic phase multiplied by the Born charges. By the ‘sliding’ cell we mean the orthorhombic cell of 40 atoms shifted each time along the  axis by b/4 (Fig. 6d).
Modelling of local ferroelectricity in APBs in PZ
To perform first-principles calculations, we used Plane-Wave Self-Consistent Field programme, which is a part of the Quantum Espresso package22 performing zero Kelvin Density Functional Theory full relaxation calculations. The calculations were performed within the Generalized-Gradient Approximation with the Perdew–Burke–Ernzerhof exchange-correlation functional23 using ultrasoft pseudopotentials by Vanderbilt24. The kinetic energy cutoff for wavefunctions was 60 Ry (816 eV). The convergence threshold on forces for ionic minimization was chosen to be equal to 10−3 a.u. (21 meV A−1).
How to cite this article: Wei, X.-K. et al. Ferroelectric translational antiphase boundaries in nonpolar materials. Nat. Commun. 5:3031 doi: 10.1038/ncomms4031 (2014).
Seidel, J. et al. Conduction at domain walls in oxide multiferroics. Nat. Mater. 8, 229–234 (2009).
Farokhipoor, S. & Noheda, B. Conduction through 71 degrees domainwalls in BiFeO3 thin films. Phys. Rev. Lett. 107, 127601 (2011).
Maksymovych, P. et al. Tunable metallic conductance in ferroelectric nanodomains. Nano Lett. 12, 209–213 (2012).
Meier, D. et al. Anisotropic conductance at improper ferroelectric domain walls. Nat. Mater. 11, 284–288 (2012).
Sluka, T., Tagantsev, A. K., Bednyakov, P. & Setter, N. Free-electron gas at charged domain walls in insulating batio. Nat. Commun. 4, 1808 (2013).
Yang, S. Y. et al. Above-bandgap voltages from ferroelectric photovoltaic devices. Nat. Nanotechnol. 5, 143–147 (2010).
Van Aert, S. et al. Direct observation of ferrielectricity at ferroelastic domain boundaries in CaTiO3 by electron microscopy. Adv. Mater. 24, 523 (2012).
Jia, C. L., Lentzen, M. & Urban, K. Atomic-resolution imaging of oxygen in perovskite ceramics. Science 299, 870–873 (2003).
Shirane, G., Sawaguchi, E. & Takagi, Y. Dielectric properties of lead zirconate. Phys. Rev. 84, 476–481 (1951).
Isupov, V. A. Ferroelectric and antiferroelectric perovskites PbB’0.5B”0.5O3 . Ferroelectrics 289, 131–195 (2003).
Tan, X., Ma, C., Frederick, J., Beckman, S. & Webber, K. G. The antiferroelectric ↔ ferroelectric phase transition in lead-containing and lead-free perovskite ceramics. J. Am. Ceram. Soc. 94, 4091–4107 (2011).
Tagantsev, A. K. et al. The origin of antiferroelectricity in PbZrO3 . Nat. Commun. 4, 2229 (2013).
Cross, L. E. A thermodynamic treatment of ferroelectricity and antiferroelectricity in pseudo-cubic dielectrics. Philos. Mag. 1, 76–92 (1956).
Okada, K. Phenomenological theory of antiferroelectric transition. i. second-order transition. J. Phys. Soc. Jpn 27, 420 (1969).
Balashova, E. V. & Tagantsev, A. K. Polarization response of crystals with structural and ferroelectric instabilities. Phys. Rev. B 48, 9979–9986 (1993).
Ostapchuk, T. et al. Polar phonons and central mode in antiferroelectric PbZrO3 ceramics. J. Phy. Condens. Matter. 13, 2677–2689 (2001).
Cowley, R. A. Lattice dynamics and phase transitions of strontium titanate. Phys. Rev. 134, A981 (1964).
Tagantsev, A. K. & Cross, L. E. and Fousek. Domains in Ferroic Crystals and Thin Films Springer (2010).
Fouskova, A. & Fousek, K. Continuun theory of domain walls Gd2(MoO4)3 . Phys. Stat. Sol. (a) 32, 213 (1975).
Parkin, S. S. P., Hayashi, M. & Thomas, L. Magnetic domain-wall racetrack memory. Science 320, 190–194 (2008).
Jia, C.-L. et al. Atomic-scale study of electric dipoles near charged and uncharged domain walls in ferroelectric films. Nat. Mater. 7, 57–61 (2008).
Giannozzi, P. et al. Quantum espresso: a modular and open-source software project for quantum simulations of materials. J. Phys. Condens. Matter. 21, 395502 (2009).
Perdew, J. P., Burke, K. & Ernzerhof, M. Generalized gradient approximation made simple. Phys. Rev. Lett. 77, 3865–3868 (1996).
Vanderbilt, D. Soft self-consistent pseudopotentials in a generalized eigenvalue formalism. Phys. Rev. B 41, 7892–7895 (1990).
The research leading to these results has received funding from the EU 7th Framework Programme under Grant Agreement 312483—ESTEEM2 (Integrated Infrastructure InitiativeI3) and from the European Research Council under the EU 7th Framework Programme (FP7/2007-2013)/ERC grant agreement no (268058) Mobile-W. The Swiss National Science Foundation is acknowledged for additional financial support (Grant number 3 200020_140539/1 and 200020_144463/1). The research was also supported by the National Centre for Science in Poland, grant number 1955-B-H03-2011-40. We thank Z. Ujma for supplying the PZO crystal, H.C. Du for continuous support in using the software package for image mapping, D. Meertens for sample preparation using focused ion beam and J. Barthel for training on the CS-corrected electron microscope. We thank Professor N. Marzari for valuable help with the first principles calculations.
The authors declare no competing financial interests.
About this article
Cite this article
Wei, XK., Tagantsev, A., Kvasov, A. et al. Ferroelectric translational antiphase boundaries in nonpolar materials. Nat Commun 5, 3031 (2014). https://doi.org/10.1038/ncomms4031