Article | Open | Published:

# Thermodynamic potential and phase diagram for multiferroic bismuth ferrite (BiFeO 3 )

## Abstract

We construct a Landau–Ginzburg thermodynamic potential, and the corresponding phase diagram for pristine and slightly doped bismuth ferrite, a ferroelectric antiferromagnet at room temperature. The potential is developed based on new X-ray and neutron diffraction experiments complementing available data. We demonstrate that a strong biquadratic antiferrodistortive-type coupling is the key to a quantitative description of Bi1−x La x FeO3 multiferroic phase diagram including the temperature stability of the antiferromagnetic, ferroelectric, and antiferrodistortive phases, as well as for the prediction of novel intermediate structural phases. Furthermore, we show that “rotomagnetic” antiferrodistortive–antiferromagnetic coupling is very important to describe the ferroelectric polarization and antiferrodistortive tilt behavior in the R3c phase of BiFeO3. The Landau–Ginzburg thermodynamic potential is able to describe the sequence of serial and trigger-type phase transitions, the temperature-dependent behavior of the order parameters, and the corresponding susceptibilities to external stimuli. It can also be employed to predict the corresponding ferroelectric and antiferrodistortive properties of Bi1−x La x FeO3 thin films and nanoparticles by incorporating the gradient and surface energy terms that are strongly dependent on the shape, size, and preparation method.

## Introduction

### State-of-the art

Multiferroics, defined as ferroics with more than one long-range order, are ideal systems for fundamental studies of couplings among the ferroelectric (FE) polarization, structural antiferrodistortion, and antiferromagnetic (AFM) order parameters.1,2,3,4,5 BiFeO3 (BFO) is the one of the rare multiferroics with a strong FE polarization, antiferromagnetism at room temperature as well as conduction and magnetotransport at domain walls.6,7,8

Multiferroic properties have also been extensively demonstrated BiFeO3 thin films and heterostructures.9,10,11,12 In particular, the studies of thin epitaxial BiFeO3 films revealed a universal field induced phase transition, modulated phases and microstructure changes as a function of rare-earth (RE) elements (e.g., Dy, Sm, Ho) doping concentration.13,14,15,16,17 Further RE doping effect was studied systematically for thin BiFeO3 films, and it was shown experimentally and theoretically16,17,18 that the doping of BiFeO3 by Sm can lead to the enhancement of dielectric properties and tunability, as well as to the stabilization of the polar phase over a wide range of temperatures for the thin (Bi,Sm)FeO3 films and the short period superlattices BiFeO3–(Bi,Sm)FeO3.

Bulk BiFeO3 exhibits antiferrodistortive (AFD) order at temperatures below 1200 K; it is FE with a large spontaneous polarization below 1100 K and is AFM below Neel temperature T N ≈ 650 K.19, 20 The very high AFD transition temperature of multiferroic BiFeO3 offers the unique possibility to study the influence of AFD order on the FE and AFM phase transitions. Despite extensive experimental and theoretical studies of BiFeO3 physical properties,21,22,23,24,25,26,27 many important issues concerning the physical mechanisms responsible for the emergence and manifestation of its multiferroic and electrophysical properties remain unclear.4,5,6,7,8,9,10,11,12,13,14,15,16,17,18,19,20,21,22,23,24,25,26 For example, the possibility of rare “trigger-type” phase transitions,28 in which different order parameters appear simultaneously at the same transition temperature, is under debate in BiFeO3.29 Further, reliable experimental results and analysis4,5,6,7,8,9,10,11,12,13,14,15,16,17,18,19,20,21,22,23,24,25,26 indicate the importance of the AFD-type couplings in BiFeO3, such as biquadratic AFD–AFM and AFD–FE couplings, and different AFD order parameters regarded as “AFD–AFD” coupling. The antiferrodistortion comes from the static rotation of some atomic groups with respect to other parts of the crystal.30 In this work, the term AFD-symmetry means only the static rotational symmetry of the oxygen octahedra MO6 with respect to the cube A8 cell in AFD perovskites with the structural formula AMO3. Oxygen atoms are displaced with respect to the centers of the cube faces A8 in the AFD phase, and the angle or the value of the corresponding displacement is a structural order parameter (see for e.g., ref. 31). According to group theory, the aforementioned biquadratic coupling can exist in all AFD multiferroics.32

### Research motivation and impact

Our primary goal is to explain and describe quantitatively the experimental data obtained in pure BiFeO3 and ab initio calculations performed previously, and in the process, construct a thermodynamic potential of Landau–Ginzburg (LG) type, which describes FE and AFD properties in pure BiFeO3. Such a LG-potential is currently lacking that can be used to reconstruct the FE polarization and AFD tilts in the low temperature AFM phase as well as high temperature phases, which are known in addition to a new phase that is disclosed in this work. Further discussion testifies to the essential impact of the AFD order on the FE and AFM long-range order and provides theoretical background to the appearance of trigger-type phase transitions due to the strong biquadratic coupling.

Though the main subject of the investigations is pure bismuth ferrite, we have also included the case of slightly La-doping4 (5%), which does not significantly change the structural parameters of the compound as compared to the pristine BiFeO3 (which is necessary for theoretical fitting), but notably lowers the critical transition temperatures and thus increases the reliability of the structural measurements at elevated temperatures. Thus the slightly doped compound with virtually no difference in the multiferroic behavior and a phase diagram as compared with pristine BiFeO3 ideally suits our purposes as a reference material for the theoretical fitting. The compounds with larger content of La ions are characterized by the orthorhombic phases without remnant polarization at room temperature and thus beyond the scope of the current study.33,34,35

## Results

### Experimental results

Structural data obtained for the BiFeO3 compounds during the X-ray diffraction (XRD) and neutron powder diffraction (NPD) measurements confirmed their single-phase rhombohedral structure (R-phase), which is stable from room temperature up to approximately 810 °C for the pristine compound and ~780 °C for the doped one. The results of the diffraction measurements show a gradual expansion of the unit cell parameters and a volume increase with temperature increase. Chemical substitution of the bismuth ions by small amount of lanthanum ions (5%) only slightly modifies the structural parameters. We did not observe any notable structural anomaly near the magnetic transition temperature, implying a weak correlation between magnetic order and crystal structure in contrast to ref. 35.

Normalized lattice parameters shown in Fig. 1a, b displays tetragonal-like distortion of the reduced unit cell associated with the polar displacements of the cations directed along the c-parameter (in rhombohedral lattice with hexagonal settings). Evolution of the structural parameters estimated for the doped compound shows faster elongation of the a-parameter as compared to the c-parameter, resulting in a decrease in tetragonality. Temperature dependences of the unit cell volume and tetragonality parameter are shown in Fig. 2a, c.

It is known that doping with lanthanum as well as with other RE elements diminishes the covalency of the Bi(La)–O chemical bond36, 37 and thus reduces the polar displacements of the cations and the tetragonality of the structure. Reduction in the polar displacement of the lightly doped Bi1−x RE x FeO3 compounds has been confirmed experimentally by neutron diffraction data as well as piezoresponse force microscopy technique.38, 39 Taking into account the evolution of tetragonality observed for the compounds, one can estimate the transition temperature of the tetragonal structure to the cubic-like structure at about 1100 °C for the pristine BiFeO3 and about 1000 °C for the doped compound.

It should be noted that the tetragonality estimated for both compounds gradually increases with temperature up to about 500 °C and then quite rapidly reduces down to the value below the calculated one for the room temperature structure. The rhombohedral angle calculated for the pseudo-cubic metric shows the opposite trend with a decrease up to T ~ 500 °C followed by gradual increase (see Table S1 in the Supplementary Materials). The critical temperature about 500 °C is also noticed by tracing the evolution of the structural parameters discussed below.

The structural data show that the chemical doping with lanthanum leads to an increase of the rhombohedral angle of the lattice, thus pointing to the reduction of the structural distortion,34, 40 wherein the tetragonality and the unit cell volume gradually decreases (e.g., for 16% of La compound, the unit cell volume is about 61.7 Å;3 rhombohedral angle alfa (R) ~ 89.68°). The structural parameters, such as the chemical bond angle Fe–O–Fe, gradually increase with an increase in temperature, while the bond lengths of Fe–O exhibit a different behavior for short and long bonds. The short bond length shows a progressive increase with temperature, while the long bond displays a restoring behavior similar to that observed for the tetragonality parameter and the rhombohedral angle (the inflection point is also about 500 °C). Similar evolution of the structural parameters has been observed for the La-doped compound and the pure compound, thus indicating that the same factors are causing the structural modification observed in both these compounds (Fig. 1b, d). The mentioned structural rearrangement is most probably associated with the oxygen octahedra tilts and rotations, which become more pronounced across the phase transition into the orthorhombic phase as discussed below.

In contrast to the evolution of tetragonality, the magnitude of polar ionic displacement shows a gradual decrease with increase in temperature for both compounds (Figs. 1 and 2). Because of the symmetry restrictions (viz. the presence of the 3-rotation axis in the rhombohedral lattice), the ionic shift is directed strictly along the c -axis of the lattice. The polar displacement calculated for the bismuth ions in the BiFeO3 is about 0.65 Å at room temperature, which leads to a polarization of ~67 µC/cm2 (assuming simple point charge model); the dipole moment attributed to the doped compound is about 4% smaller, thus resulting in proportionally lower polarization. The difference in the Fe–O bond lengths (the bond lengths for initial compound are 2.115 and 1.943 Å at room temperature) also contributes to the dipole moment of the compounds, accounting about 30% of overall polarization (Fig. S1 in Supplementary Materials). Temperature increase causes a modification of the ionic coordinates (Table S1 in Supplementary Materials) leading to a gradual decrease of the polar displacements of the Bi ions and nearly negligible changes for the Fe ions (Fig. S1 in Supplementary Materials). The reduction in the displacements of the Bi ions becomes more pronounced at high temperatures showing certain anomaly at ~500 °C for the initial compound.

Thermal evolution of the bond lengths Bi(La)–O observed for the pristine bismuth ferrite shows certain anomaly at ~500 °C, followed by faster decrease in the magnitude as compared to the dependence estimated for the doped compound. The difference in the behavior of the ionic displacement is associated with a modification of the character of the chemical bonds because of different covalent component in the Bi(La)–O lengths as confirmed by change density analysis ref. 36. More pronounced covalent component estimated for the initial compound makes it more stable at high temperatures as confirmed by the given structural data. The displacement estimated for the Fe ions shows only slight decrease with temperature increase for both compounds.

Significant displacement of the bismuth/lanthanum ions from their ideal perovskite positions is often associated with anomalous atomic displacement parameters.41 Refinement of the NPD patterns using anisotropic displacement parameters has considerably improved the reliability factors. The atomic displacement parameters calculated for the rhombohedral phase testify to an elongation of the thermal ellipsoids associated with bismuth/lanthanum ions along the polar axis [111]p.

The NPD patterns recorded for the compounds at high temperatures (~800 °C) have revealed drastic changes in the crystal structure associated with the rhombohedral-orthorhombic phase transition.42, 43 The diffraction data shows a narrow temperature range (about 20–30 °C) of the two-phase mixture state, thus confirming the high chemical homogeneity of the compounds. Further temperature increase leads to the formation of a single phase state with non-polar orthorhombic symmetry described by the space group Pnma (O-phase).

The RO structural transition for the initial compound is observed at ~840 °C; this transition is accompanied by an abrupt decrease in the reduced unit cell parameters, which becomes much closer in their magnitudes resulting in a pseudo-cubic symmetry. The unit cell volume calculated for the pristine compound BiFeO3 shows a drastic decrease (~1.6%); the doped compound also exhibits a comparable decrease in the unit cell volume (~1.8%) (Fig. 1), while the structural transition is shifted towards lower temperature and completes at about 780 °C. The changes of the unit cell parameters across the transition (Fig. 1) as well as the evolution of the polar ionic shifts imply a first-order displacive phase transition into the nonpolar orthorhombic state. Lower transition temperature observed for the doped compound has allowed us to perform reliable refinement of the structural parameters as the diffraction patterns are not deteriorated in quality because of decreased signal-to-noise and chemical decomposition started at T ~ 850 °С for the initial compound.

The diffraction results cannot provide reliable structural data necessary to reveal the origin of these phase transitions, because of uncertainty in the unit cell parameters calculated near the decomposition temperature. To clarify the structural evolution of the compounds at high temperatures, we have performed theoretical modeling of the phase stability of the different crystal structures as well as the estimated presence of the intermediate phases.

### Structural data veracity

It is known44,45,46 that a substitution of the bismuth ions by lanthanum ones lowers the temperatures of the structural transitions and increases structural stability of the compounds. The DTA/DSC measurements performed in the research have clarified the phase transition temperatures and an application of the obtained results has permitted us to accomplish a careful estimation of the structural parameters based on the neutron diffraction measurements. The phase purity of the compounds has been verified by the diffraction measurements and the obtained structural data are in accordance with the results declared in previous seminal works.13, 34, 44

It is known that the chemical decomposition of the pristine compound occurs at about 930 °C20, 35 while one can assume some release of the oxygen and bismuth ions at lower temperatures; the structural data used for theoretical calculations have been taken at a lower temperature range where any decomposition process is negligible. Moreover, the neutron diffraction process assumes that an interaction of the neutrons with matter occurs in a thick layer of the crystallites (about 100 nm) so that the diffraction data reflect the average structural parameters throughout the grains (not just their surface layers). Taking into account these arguments, one can have high confidence in the reliability of the provided structural results.

### Theoretical background

#### Extraction of the octahedral tilt and polarization

The temperature dependence of the oxygen octahedra tilt has been determined from the full set of oxygen positions, directly extracted from the structural data measured in R3c phase in this work. According to refs. 43, 47, for the R3c space group, the fractional coordinates of oxygen atoms in the one of 18 equivalent Wyckoff position have the form O: $$\left( {\frac{1}{2} + 2e - 2d,\quad - 4d,\quad 1 - s} \right)$$, where the temperature dependences e, d and s values will be determined from the experiment. Based on the coordinates, we determine the angle of oxygen octahedra tilt as $$\omega {\rm{ = }}\arctan \left( {\frac{{4\sqrt 3 e}}{{1 - 12d}}} \right)$$. In the same coordinate settings, Bi atom has the following fractional coordinates Bi: (0, 0, $${\frac{1}{4}}$$ + s). Components of the oxygen atom displacement Φ are equal to $${{\bf{\Phi }}_1} = {{\bf{\Phi }}_2} = {{\bf{\Phi }}_3} = \frac{a}{{\sqrt 8 }}\tan \frac{\omega }{{\sqrt 3 }} \approx \frac{a}{{\sqrt 2 }}\frac{{2e}}{{1 - 12d}}$$, where a is the lattice constant. Comparison with experiment gives the following values e ~ −0.03; d ~ −0.05; s ~ 0.05 and ω ~ 11°, which vary with temperature as anticipated. The calculated temperature dependence of the oxygen displacement Φ for the R3c phase is shown in Fig. 3a. Empty and filled diamonds correspond to pure BiFeO3 and BiFeO3 doped with 5% of La respectively.

The temperature dependence of FE polarization was calculated using the following relation $$P{\rm{ = }}\frac{{6{q_e}\left( {{q_{{\rm{Bi}}}}{\rm{\delta }}{z_{{\rm{Bi}}}} + {q_{{\rm{Fe}}}}\delta {z_{{\rm{Fe}}}}} \right)}}{{{V_{{\rm{u}}{\rm{.c}}{\rm{.}}}}}}$$, where q e is the elementary charge of electron, q Bi = 4.38 and q Fe = 3.61 are corresponding Born effective charges taken from,48 where δz Bi and δz Fe are displacements of Bi and Fe atoms from their centro-symmetric positions, c is the lattice constant along polar axis, and V u.c. is the unit cell volume, $${V_{{\rm{u}}{\rm{.c}}{\rm{.}}}}{\rm{ = }}\left( {\sqrt 3 {\rm{/2}}} \right){a^2}c$$. The factor of “6” takes into account the presence of six formula units inside the unit cell. The temperature dependence of the recalculated spontaneous polarization P in R3c phase is shown in Fig. 3b. Empty and filled diamonds correspond to experimental results for pure BiFeO3 and doped with 5% of La, respectively measured in this work.

#### Thermodynamic potential

Our primary goal is not only to explain and describe quantitatively the experimental data, but also to construct a thermodynamic potential of LG type, that describes AFM, FE and AFD properties for pure BiFeO3 and BiFeO3 slightly doped with La, including the FE-AFD R3c phase, different structural AFD phases (orthorhombic Pbnm, tetragonal I4/mcm) and cubic Pm3m phase. For this purpose, we include the AFD, FE and AFM contributions and the biquadratic coupling among them:

$${\rm{\Delta }}G{\rm{ = \Delta }}{G_{{\rm{AFD}}}}{\rm{ + \Delta }}{G_{{\rm{FE}}}}{\rm{ + \Delta }}{G_{{\rm{AFM}}}}{\rm{ + \Delta }}{G_{{\rm{BQC}}}}$$
(1)

The AFD energy is a six-order expansion on the two tilt vectors (Φ i and Ψ i ):

$$\begin{array}{ccccc}& \\ {\rm{\Delta }}{G_{\rm AFD}} {\rm{ = }}a_i^{({\rm{\Phi }})}{\bf{\Phi }}_i^2{\rm{ + }}a_{ij}^{({\rm{\Phi }})}{\bf{\Phi }}_i^2{\bf{\Phi }}_j^2{\rm{ + }}a_{ijk}^{({\rm{\Phi }})}{\bf{\Phi }}_i^2{\bf{\Phi }}_j^2{\bf{\Phi }}_k^2{\rm{ + }}a_i^{({\rm{\Psi }})}{\bf{\Psi }}_i^2\\ \\ {\rm{ + }}a_{ij}^{({\rm{\Psi }})}{\bf{\Psi }}_i^2{\bf{\Psi }}_j^2{\rm{ + }}a_{ijk}^{({\rm{\Psi }})}{\bf{\Psi }}_i^2{\bf{\Psi }}_j^2{\bf{\Psi }}_k^2.\\ \end{array}$$
(2a)

Here Φ i and Ψ i are components of pseudovectors, determining out-of-phase and in-phase static rotations of oxygen octahedral groups (eigenvectors of AFD modes of lattice vibrations), and Einstein summation convention is employed. These vectors correspond to Glazer tilt systems a b c and a + b + c +, respectively and have different transformation properties. AFD order parameters Φ i and Ψ i could be measured as either tilt angles of oxygen octahedra or oxygen atoms displacement from the symmetric position in an ideal cubic perovskite structure.

FE energy ΔG FE is a sixth-order expansion on the polarization vector P i .

$${\rm{\Delta }}{G_{\rm FE}}{\rm{ = }}a_i^{(P)}P_i^2{\rm{ + }}a_{ij}^{(P)}P_i^2P_j^2{\rm{ + }}a_{ijk}^{(P)}P_i^2P_j^2P_k^2.$$
(2b)

Sixth-order expansion on the tilts Φ i (Eq. 2a) is necessary to describe the first-order transition from the cubic Pm3m to tetragonal I4/mcm phases, and we find that a sixth-order expansions for Ψ i and P i are necessary to quantitatively describe the temperature dependence of different order parameters. AFM energy ΔG AFM is a fourth-order expansion in terms of the AFM order parameter vector L i because this phase transition in BiFeO3 is known to be the second order one.

$${\rm{\Delta }}{G_{{\rm{AFM}}}}{\rm{ = }}a_i^{({\rm{L}})}L_i^2 + a_{ij}^{({\rm{L}})}L_i^2L_j^2.$$
(2c)

In accordance with the classical LG theory, we assume that the coefficients $$a_i^{(\Phi )}$$, $$a_j^{(\Psi )}$$ and $$a_k^{({\rm{P}})}$$ are temperature dependent according to Barrett law,49 $$a_i^{(\Phi )}{\rm{ = }}a_T^{(\Phi )}{T_{q\Phi }}\left( {\coth \left( {{T_{q\Phi }}{\rm{/}}T} \right) - \left( {{T_{q\Phi }}{\rm{/}}{T_\Phi }} \right)} \right)$$, $$a_j^{(\Psi )}{\rm{ = }}a_{\rm{T}}^{(\Psi )}{T_{{\rm{q}}\Psi }}\left( {\coth \left( {{T_{{\rm{q\Psi }}}}{\rm{/T}}} \right) - \coth \left( {{T_{q\Psi }}{\rm{/}}{{\rm{T}}_\Psi }} \right)} \right)$$ and $$a_k^{(P)}{\rm{ = }}a_T^{(P)}\left( {{T_{qP}}\coth \left( {T_{qP}/T} \right) - {T_{\rm{C}}}} \right)$$, where T Φ, T Ψ and T C are corresponding virtual Curie temperatures, T qΦ, T qΨ and T qP are characteristic temperatures.50

As it was shown recently,51 similar Barrett-type expressions can be used for AFM coefficient $$a_i^{\rm{L}}(T)$$ of pure bismuth ferrite $$a_i^{\rm{L}}(T) = {\alpha _{{\rm{LT}}}}{T_{\rm{L}}}\left( {\coth \left( {{T_{\rm{L}}}/T} \right) - \coth \left( {{T_{\rm{L}}}/{T_{\rm{N}}}} \right)} \right)$$ with the Neel temperature T N = 645 K and characteristic temperature T L = 550 K. The expression $$L\sim\sqrt {a_1^{\rm{L}}\left( T \right){\rm{/}}{{\rm{a}}_{11}}}$$, valid in the isotropic approximation, describes quantitatively both the temperature dependence of the AFM order parameter measured experimentally in BiFeO3 by neutron scattering by Fischer et al.19 and anomalous AFM contribution to the specific heat behavior near the Neel temperature measured experimentally by Kallaev et al.52. The Neel temperature is a bit higher (T N = 650 K) for Bi0.95La0.05FeO3 53 (see the first column in Table 1, where all observed transition temperatures in BiFeO3 and Bi0.95La0.05FeO3 are listed).

The AFD–FE–AFM coupling energy ΔG BQC is a biquadratic form of the order parameters L i , P i , Φ i and Ψ i . The detailed forms of these contributions, which account for the parent phase symmetry Pm3m of BiFeO3 and different transformation properties of the out-of-phase tilt Φ i and in-phase tilt Ψ i , are listed in the Appendix B, Supplementary Materials. The short form of ΔG BQC is

$$\begin{array}{ccccc}\\ {\rm{\Delta }}{G_{{\rm{BQC}}}} & {\rm{ = }}{\xi _{ij}}{\bf{\Phi }}_i^2{\bf{\Psi }}_j^2{\rm{ + }}{\zeta _{ijkl}}{{\bf{\Phi }}_i}{{\bf{\Phi }}_j}{P_k}{P_l}{\rm{ + }}{\eta _{ij}}{\bf{\Psi }}_i^2P_j^2\\ \\ & {\rm{ + }}{\kappa _{ij}}{\bf{\Phi }}_i^2L_j^2{\rm{ + }}{\lambda _{ij}}P_i^2L_j^2,\\ \end{array}$$
(2d)

For a given symmetry, the coupling energy in Eq. 2d includes nine unknown tensorial coefficients in Voight notation for the AFD–AFD (ξ11, ξ12) and AFD–FE (ζ44, ζ11, ζ12, η 11 η 12) biquadratic couplings. Due to the lack of experimental data, FE–AFM and AFD–AFM constants λ ij and κ ij 32 are assumed to be isotropic, $${\lambda _{ij}}{\rm{ = }}\lambda {\delta _{ij}}$$ and $${\kappa _{ij}}{\rm{ = }}\kappa {\delta _{ij}}$$.

Note, that DM interaction was not included in the potential (1), because we have focused on the influence of the simplest and omnipresent biquadratic couplings between the tilt, polarization, and (anti)ferromagnetism. Also we see no serious grounds to include more complex DM-related coupling like L × M × P × Φ in the bulk functional, which can be allowed by the symmetry. Also we have neglected all gradient and flexo-type coupling terms, because we restricted ourselves to the consideration of homogeneous bulk BiFeO3.

#### LG potential coefficients

LG potential coefficients have been determined from experiments using the fitting procedure. The procedure started from the high temperature structural phases (cubic, tetragonal I4/mcm and orthorhombic Pbnm) and then goes down to the low temperature FE-rhombohedral R3c phase. Expansion coefficients of the LG potential for pure BiFeO3 and BiFeO3 doped with 5% of La extracted from the fitting of measured the AFD and FE order parameters in rhombohedral R3c, orthorhombic Pbnm and tetragonal I4/mcm phases are listed in the Table 2.

Note, that for the complex sequence of the first-order phase transitions, the virtual Curie temperatures T C, T Φ and T Ψ, listed in the Table 2, can be different from the corresponding transition temperatures from R3c to Pbnm phase, from Pbnm to I4/mcm phase and from I4/mcm to Pm3m phase measured experimentally and listed in the Table 1. At the first glance, virtual Curie temperatures, T C = (1300–1380) K, and T Φ = (1440–1470) K listed in the Table 2, seem noticeably higher than the corresponding transition temperatures T FE = 1100 K and T S2 = (1350–1400) K observed experimentally. The temperature T Ψ = 1200 K is lower than the transition one, T S1 = 1250 K. Actually, the Curie temperatures should coincide with the transition temperatures only for the single second-order transition between e.g. non-structural cubic paraelectric phase with P i  = 0 and pure FE phase with P j  ≠ 0. For the complex sequence of the first-order structural-phase transitions and-polar phase transitions, observed for the BiFeO3 (R3c with nonzero P 1 = P 2 = P 3 ≠ 0 and Φ 1 = Φ 2 = Φ 3 ≠ 0 Pbnm phase with nonzero Φ 1 = Φ 2 ≠ 0 and Ψ 3 ≠ 0 I4/mcm phase with the only nonzero Φ 1 ≠ 0 Pm3m phase without any long-range order), the virtual Curie temperatures T C, T Φ and T Ψ can be different from corresponding transition temperatures T FE, T S1 and T S2 due to the 6th-order nonlinear terms of the order parameter, like $$a_{ijk}^{({\rm{P}})}P_i^2P_j^2P_k^2$$ or $$a_{ijk}^{(\Phi )}{\bf{\Phi }}_i^2{\bf{\Phi }}_j^2{\bf{\Phi }}_k^2$$, as well as due to the transition temperature shifts by the biquadratic (or even bilinear) coupling terms in Eq. 2d.32, 51 Furthermore, at the transition temperatures from R3c and Pnma, and from Pnma to I4/mcm, the two involved phases have the same free energy, and thus usually the transition temperatures are lower than the corresponding Curie temperatures. It appears that the shift caused by the 6th-order nonlinearity is typically small in pure and slightly doped BiFeO3, not more than (10–50) K, but the shift caused by the biquadratic coupling $${\rm{\zeta }}_{ijkl}^{}{\bf{\Phi }}_i^{}{\bf{\Phi }}_j^{}P_k^{}P_l^{}$$ decreases the virtual Curie temperature T C by more than 150 K towards experimentally observed value T FE. The difference of about (50–100) K between the observed AFD transition temperatures and corresponding Curie temperatures are mostly related to the coupling between the different structural order parameters described by the term $${\rm{\xi }}_{ij}^{}{\bf{\Phi }}_i^2{\bf{\Psi }}_j^2$$ in Eq. 2d. Moreover, the coefficients of the nonlinear terms should exhibit temperature dependence in order to have better agreement between the theory and the experiments.

Let us emphasize that an intermediate metastable monoclinic phase with Φ 1 = Φ 2 ≠ Φ 3 and P 1 = P 2 ≠ P 3 can appear between the rhombohedral and orthorhombic phases (e.g., around (1100–1200 K) in addition to the observed phases. The energy of the monoclinic phase decreases with changing coefficients ζ44 and ζ12, (at that ζ12 becomes larger with ζ44 decrease at the fixed value of ζ11 +2 ζ12 + ζ44). The phase may become stable in BiFeO3 slightly doped with Ca or Mn.54, 55

The fitting results, which illustrate how the considered functional fit the experimentally measured temperature dependence of the AFD order parameter and FE polarization in the FE-AFD R3c phase of the pure BiFeO3 and BiFeO3 with 5% of La, are shown in the Fig. 3a, b. Note that the temperature dependence of the dielectric permittivity measured by Kamba et al.56, as well data obtained Lobo et al.57, was taken into account (Fig. S2c, Supplementary Material), when we chose the optimal fitting parameters for polarization temperature dependence in R3c phase. Dashed curves for BiFeO3 are calculated without biquadratic AFD–AFM and FE–AFM couplings terms $$\left( {\kappa {\bf{\Phi }}_{}^2 + \lambda P_{}^2} \right)L_{}^2$$. Thus AFD–AFM and FE–AFM couplings are sufficient to cause the small fractures of AFD and FE order parameters at Neel temperature, and to increase their saturation rate in the AFM phase, as shown in Fig. 3a, b. However AFD-AFM and FE-AFM couplings are relatively weak to shift the lowest AFM transition temperature by 645 K towards R3c-Pbnm transition at 1100 K. The corresponding temperature dependence of BiFeO3 AFM order parameter (theoretical fitting and the neutron scattering by Fischer et al.19) is shown in Fig. S2a, Supplementary Material.

Figure 4 illustrates the temperature dependence of oxygen displacement components (Φ i and Ψ i ) for different phases of BiFeO3. Experimental data of Arnold et al.58 and ab initio calculation results of Kornev and Bellaiche59 are compared with our fitting (solid curves). Figure 4 shows a pronounced set of the first-order phase transitions. By analyzing the tilt absolute value, we can conclude that the out-of-phase tilt vector Φ first appears at the boundary between cubic Pm3m and tetragonal I4/mcm phases in accordance with the first-order phase transition scenario, and then it mostly rotates at the borders between different structural phases (Fig. S3b, Supplementary Material). Meanwhile another in-phase tilt vector Ψ exists in the Pbnm phase only, and disappears at its boundaries in accordance with the first-order phase transition scenario. The temperature behavior of the out-of-phase and in-phase tilts is similar to that in CaTiO3.

The temperature dependences of the free energies for different phases (tetragonal I4/mcm, orthorhombic Pbnm and rhombohedral R3c, and non-observable “intermediate” Imbm) are shown in the Fig. 5a. As one can see from the figure, the predicted “intermediate” Imbm phase with Φ 1 = Φ 2 ≠ 0 has the lowest energy in a narrow temperature range between 1305 and 1322 K. However, its energy is almost the same as the energy of the predicted by DFT I4/mcm phase. Hence the phase can be indeed (meta) stable in the narrow temperature interval of 17 K width, and we believe that this prediction could be up for debate, similar to the discussion of the intermediate phases separating R3c and Pnma phases in Ca-doped BiFeO3 46 and pure CaTiO3.60 Note that this phase (without changing the sequence of other phases) can be eliminated by simultaneously changing the coefficients $$a_{12}^{(\Phi )}$$ and $$a_{112}^{(\Phi )}$$ by about 25%, but the changes lead to the visible disagreement between the theoretical curves and measured experimental data, namely in the shift of the phase transition temperature between R3c and Pbnm phases to 1150 K. In this case, although the Imbm phase is thermodynamically stable in the narrow temperature region, it has not been experimentally observed due to the high kinetic energy barriers of the first-order transition from I4/mcm to Imbm phases.

Hence, we can achieve a quantitative agreement with experimental results for a definite set of values for the expansion coefficients in Eqs. 2a,b,c,d, which satisfy the definite inequalities for the coefficients listed in the Table 2. All the information we extracted about the biquadratic coupling coefficients are listed in the table. Unexpectedly, the temperature dependence of the coupling coefficients $${\rm{\xi }}_{12}^{}$$ appears noticeable for pure and lightly doped BiFeO3.

The biquadratic coupling strength is estimated in different phases in Appendix B, Supplementary Materials.

The ΨΦ-coupling between in-phase and out-of phase tilts can be regarded strong enough if the following inequality is valid $$\left( {2a_{11}^{(\Phi )} + a_{12}^{(\Phi )}} \right)a_{11}^{(\Psi )} \le {\left( {{\rm{\xi }}_{12}^{(\Phi \Psi )}} \right)^2}$$. The coupling is weak for the opposite sign >> in the inequality. The positive ΨP-coupling is very strong everywhere to prevent the polarization appearance in Pbnm phase, because $$4\left( {a_{11}^{({\rm{P}})}{\rm{ + }}a_{12}^{({\rm{P}})}} \right)\left( {a_{11}^{(\Psi )}{\rm{ + }}a_{12}^{(\Psi )}} \right){\rm{ < < }}{\left( {\eta _{11}^{(\Psi {\rm{P}})}{\rm{ + }}2\eta _{12}^{(\Psi {\rm{P}})}} \right)^2}$$ under the required condition $$\eta _{ij}^{(\Psi {\rm{P}})}$$≥10.30 Appeared that the ΨΦ-coupling is weak only in the vicinity of the Pbnm-I4 mcm phase transition and becomes relatively noticeable outside it, and strong in R3c phase (see blue area in Fig. 5b). The coupling between the FE polarization and out-of-phase tilts can be regarded as strong if the following inequality is valid: $$4\left( {a_{11}^{(P)} + a_{12}^{({\rm{P}})}} \right)\left( {a_{11}^{(\Phi )} + a_{12}^{(\Phi )}} \right) \le {\left( {{\rm{\zeta }}_{11}^{(\Phi P)} + 2{\rm{\zeta }}_{12}^{(\Phi P)} + {\rm{\zeta }}_{44}^{(\Phi P)}} \right)^2}$$. Conversely, this coupling can be regarded as weak for the opposite sign “>>” of the inequality. It appears that the PΦ-coupling is very strong for the entire R3c phase (see Fig. 5c).

Note that a trigger-type phase transition is possible only for the sufficiently large negative value of the coupling coefficient.28 Since the best fitting corresponds to an unexpectedly strong ΨΦ and PΦ-biquadratic couplings, and some of the coupling coefficients are negative (ζ11 < 0, ζ44 < 0 and ξ12 < 0), this result is a strong indication for the trigger-type28 phase transition between R3c and Pbnm phases, where three components of polarization (P 1 = P 2 = P 3) and one out-of-phase tilt component (Φ 3) disappear and in-phase tilt (Ψ) appear simultaneously. However, the transition between Pbnm and I4/mcm phases, where Ψ and Φ 2 disappear, is successive rather than the trigger-type due to the small coupling value in the temperature range and possible existence of intermediate Imbm phase within a super narrow temperature range. The transition from I4/mcm to Pm3m phase may be of a trigger-type, if the transition were of the second order. However the suggestion contradicts to Kornev et al. results for tetragonal phase.59

#### Substitution of La doping by other dopants

Chemical doping with RE elements leads to the decrease of the phase transitions temperatures and increases the structural stability of these compounds. The obtained results testify close Landau-Ginzburg-Devonshire (LGD) coefficients for both initial and slightly La-doped BFO compounds [see Table 2]. The result allows us to expand our theoretical approach to the case of other dopants. It is assumed that addition of the small amount “x” (less than 5%) of RE doping affects the potential expansion coefficients of BFO and LGD in a linear way, $$a_i^{({\rm{P}},\Phi ,\Psi )}\left( {x,T} \right){\rm{ = }}a_i^{({\rm{P}},\Phi ,\Psi )}\left( {0,T} \right){\rm{ + }}x\delta a_i^{({\rm{P}},\Phi ,\Psi )}$$, due to the joint action of electrostriction and rotostriction couplings, and Vegard strains (other name is chemical pressure)20 produced by the dopants and/or vacancies inclusion.16,17,18, 61 The Vegard strains δu ij can be written as the product of Vegard tensor coefficients W ij and the instant dopant concentration x(r), δu ij (r) = W ij x(r). Allowing for electrostriction and rotostriction couplings, the coefficients $$\delta a_i^{({\rm{P}},\Phi ,\Psi )}$$ are proportional to the convolution of the electrostriction (Q ijkl ) and rotostriction (R ijkl ) tensor coefficients with the Vegard strains, namely that the corresponding terms are $$x\delta a_i^{({\rm{P}})}{\rm{ = }}{Q_{iikl}}\delta {u_{kl}}({\bf{r}}) \cong {Q_{iikl}}{W_{kl}}x({\bf{r}})$$, $$x\delta a_i^{(\Phi )}{\rm{ = }}R_{iikl}^{(\Phi )}\delta {u_{kl}}({\bf{r}}) \cong R_{iikl}^{(\Phi )}{W_{kl}}x({\bf{r}})$$ and $$x\delta a_i^{(\Psi )}{\rm{ = }}R_{iikl}^{(\Psi )}\delta {u_{kl}}({\bf{r}}) \cong R_{iikl}^{(\Psi )}{W_{kl}}x({\bf{r}})$$. Our approach reconstructs the coefficients $$a_i^{({\rm{P}},\Phi ,\Psi )}\left( {0,T} \right)$$, while the coefficients $$\delta a_i^{({\rm{P}},\Phi ,\Psi )}$$ can be calculated (for a definite doping) in a straightforward way if the tensors W ij , Q ijkl and R ijkl are known from microscopic calculations or experiments, where not only the amount of RE dopant, but also the degree of non-stoichiometry (e.g., the vacancies concentration) is controlled with high accuracy. The non-stoichiometry control is especially important because it can affect the free energy coefficients via electrostriction and rotostriction coupling with the Vegard strains produced by the vacancies similarly to the doping effect.

## Discussion

To resume the theoretical results, we can state that using the experimental temperature dependences obtained in this work, together with other independently available experimental data and ab initio calculations, we develop a LG type thermodynamic potential of pristine and slightly doped bismuth ferrite that describes quantitatively their multiferroic phase diagrams with the AFM (below 645 K) and FE-AFD R3c (below 1100 K) phases, different structural AFD phases (orthorhombic Pbnm at 1100 K < T < 1250 K, tetragonal I4/mcm 1250 K < T < 1350 K) and cubic parent Pm3m phase at T > (1350–1400 K).

By the fitting to experiment and ab initio data for the temperature behavior of the sub-lattice magnetization L, FE polarization P, out-of-phase and in-phase octahedral tilts Φ and Ψ, we determined the full set of 4-6-6-LG thermodynamic expansion coefficients, some of which reveal a rather strong temperature dependence. As anticipated, the Barrett-type temperature dependences appear to be valid for all generalized stiffness α i (T) determining the “isotropic” quadratic terms like αL(T)L 2, αP(T)P 2, αΦ(T)Φ 2 and α Ψ(T)Ψ 2. Unexpectedly, some of the tensorial expansion coefficients of 4th and 6th order structural terms $$a_{ij}^{(\Phi )}{\bf{\Phi }}_i^2{\bf{\Phi }}_j^2$$, $$a_{ijk}^{(\Phi )}{\bf{\Phi }}_i^2{\bf{\Phi }}_j^2{\bf{\Phi }}_k^2$$, $$a_{ij}^{(\Psi )}{\bf{\Psi }}_i^2{\bf{\Psi }}_j^2$$, and $$a_{ijk}^{(\Psi )}{\bf{\Psi }}_i^2{\bf{\Psi }}_j^2{\bf{\Psi }}_k^2$$ the coupling coefficients $${\rm{\xi }}_{ij}^{}{\bf{\Phi }}_i^2{\bf{\Psi }}_j^2$$ should have specific (e.g., linear or saturating) temperature dependences. Therefore, a conventional LG-theory first developed for primary ferroics with the second-order phase transitions, that postulated the temperature-dependent coefficient only for the 2nd order coefficients αL(T), αP(T), and αΦ(T), is insufficient for multiferroics with the strong interactions between different order parameters.

Hence we conclude that the AFD part of BiFeO3 thermodynamic potential is much more complex than the one in CaTiO3 50 that is a primary ferroic. Moreover, the strong biquadratic AFD-type coupling between the AFD, polar and AFM sub-systems is critical to the quantitative description of the available experimental data for both pristine and slightly doped with La bismuth ferrite. Keeping in mind that the trigger-type phase transitions originate from the same ion contributions, the strong interaction between different order parameters can be expected. Since the best fitting for BiFeO3 corresponds to the unexpectedly strong ΨΦ and PΦ-biquadratic couplings and some of the coupling coefficients are negative (ζ11 < 0, ζ44 < 0 and ξ12 < 0), this result is the independent and rather strong support for a trigger-type28 phase transition between R3c and Pbnm phases.

X-Ray and NPD measurements determine a full set of the unit cell parameters, bond angles, and lengths, as well as the ionic displacements in pristine and slightly doped with 5% La bismuth ferrite. The structural parameters, FE polarization and AFD octahedral tilt have been extracted from the measured data in the temperature range 300–1150 K. The experimental data and the results of the theoretical modeling are integrated to determine the evolution of the FE and AFD long-range order parameters, thermodynamic potentials and coefficients across the temperature-driven phase transition into the nonpolar structural phase. The obtained data have detailed the structural phase diagram, focusing on high temperature phases, which could not be observed experimentally because of the decomposition process. In particular, a new structural phase described by space group Imbm has been predicted.

Using the experimental results obtained in this work, together with other independent available experimental data and ab initio calculations, we have developed a LG type thermodynamic potential of pristine and slightly doped bismuth ferrite that describes quantitatively their multiferroic phase diagrams with the AFM and FE-AFD R3c phases, different structural AFD phases and cubic parent phase. We have proved a trigger-type transition between R3c and Pbnm phases. We are confident that this transition happens without any “virtual” intermediate phase appearance. The well-pronounced and temperature-separated trigger-type transitions are surprisingly uncommon for ferroic AFD FEs. Complementary to the trigger-type transition, which are surprisingly uncommon for ferroic AFD FEs, we have predicted new intermediate phase described by Imbm phase between Pbnm and I4/mcm phases. The impossibility of avoiding this phase proves that the transition between Pbnm and I4/mcm cannot be of a trigger-type, as regarded previously.

Based on the obtained experimental data, we have extracted the spontaneous polarization of BiFeO3 in R3c phase and estimated AFD parameters including AFD-type biquadratic couplings across the phase transition into the orthorhombic phase for the first time. Furthermore, we have proved that “rotomagnetic” AFD-AFM coupling is very important to describe the FE polarization and AFD tilt behavior in the R3c phase of BiFeO3. The coupling was neither considered for BiFeO3, nor probed experimentally for other perovskites, while it was predicted for EuTiO3.32

The benefit of the LG-type thermodynamic potential is not only in its capability to describe the observed sequence of the phase transitions along with the temperature behavior of the order parameters, corresponding susceptibilities to external stimuli in the one of the most promising multiferroic, but also it opens the way to model theoretically polar and antiferrodistoritive properties in thin films and nanoparticles of pristine and slightly doped with RE ions bismuth ferrite by incorporating the effect of the interfacial energy and electrostrictive interaction.12

## Methods

Ceramic samples of La-doped BiFeO3 with dopant concentrations x = 0, 0.05 were prepared by the two-stage solid-state reaction using high purity oxides (Alfa Aesar) as described in refs 40, 62. The oxides Bi2O3, La2O3, and Fe2O3 taken in stoichiometric ratio were thoroughly mixed using a planetary ball mill (Retsch PM 200). Pure BiFeO3 was synthesized at 870 °C for 10 min. La-Doped compound was prepared at 950 °C for 15 h. The XRD patterns were collected at room temperature using a Rigaku D/MAX-B diffractometer (Cu-K α radiation) equipped with an Anton Paar heating stage. NPD measurements were performed with the high-resolution neutron powder diffractometer FIREPOD (λ = 1.7982 Å, E9 instrument, HZB). Diffraction data were analyzed by the Rietveld method using the FullProf software package.63 Thermal analysis was carried out using differential scanning calorimeter Mettler Toledo 822e in argon atmosphere.

## References

1. 1.

Fiebig, M. Revival of the magnetoelectric effect. J. Phys. D Appl. Phys 38, R123–R152 (2005).

2. 2.

Spaldin, N. A. & Fiebig, M. The renaissance of magnetoelectric multiferroics. Science 309, 391–392 (2005).

3. 3.

Rondinelli, J. M. & Spaldin, N. A. Structure and properties of functional oxide thin films: insights from electronic structure calculations. Adv. Mater. 23, 3363–3381 (2011).

4. 4.

Pyatakov, A. P. & Zvezdin, A. K. Magnetoelectric and multiferroic media. Phys. Usp. 55, 557–581 (2012).

5. 5.

Scott, J. F. Data storage: multiferroic memories. Nat. Mater. 6, 256–257 (2007).

6. 6.

Seidel, J. et al. Domain wall conductivity in La-doped BiFeO3. Phys. Rev. Lett. 105, 197603–197605 (2010).

7. 7.

He, Q. et al. Magnetotransport at domain walls in BiFeO3. Phys. Rev. Lett. 108, 067203–067206 (2012).

8. 8.

Catalan, G., Seidel, J., Ramesh, R. & Scott, J. F. Domain wall nanoelectronics. Rev. Mod. Phys. 84, 119–156 (2012).

9. 9.

Wang, J. B. N. J. et al. Epitaxial BiFeO3 multiferroic thin film heterostructures. Science 299, 1719–1722 (2003).

10. 10.

Maksymovych, P. et al. Ultrathin limit and dead-layer effects in local polarization switching of BiFeO3. Phys. Rev. B Condens. Matter 85, 014119–014116 (2012).

11. 11.

Beekman, C. et al. Ferroelectric self -poling, switching, and monoclinic domain configuration in BiFeO3 thin films. Adv. Funct. Mater. 26, 5166–517 (2016).

12. 12.

Xue, F., Li, Y., Gu, Y., Zhang, J. & Chen, L.-Q. Strain phase separation: formation of ferroelastic domain structures. Phys. Rev. B Condens. Matter 94, 220101(R) (2016).

13. 13.

Kan, D. et al. Universal behavior and electric-field-induced structural transition in rare-earth-substituted BiFeO3. Adv. Funct. Mater. 20, 1108–1115 (2010).

14. 14.

Minh, N. V. & Quan, N. G. Structural, optical and electromagnetic properties of Bi1-xHoxFeO3 multiferroic materials. J. Alloys Compd. 509, 2663–2666 (2011).

15. 15.

Borisevich, A. Y. et al. Atomic-scale evolution of modulated phases at the ferroelectric–antiferroelectric morphotropic phase boundary controlled by flexoelectric interaction. Nat. Commun. 3, 775 (2012).

16. 16.

Sankara, P. S. et al. Misfit strain driven cation inter-diffusion across an epitaxial multiferroic thin film interface. J. Appl. Phys. 115, 054103 (2014).

17. 17.

Maran, R. et al. Interface control of a morphotropic phase boundary in epitaxial samarium-modified bismuth ferrite superlattices. Phys. Rev. B Condens. Matter 90, 245131 (2014).

18. 18.

Maran, R. et al. Enhancement of dielectric properties in epitaxial bismuth ferrite–bismuth samarium ferrite superlattices. Adv. Electron. Mater. 2, 1600170 (2016).

19. 19.

Fischer, P., Polomska, M., Sosnowska, I. & Szymanski, M. Temperature dependence of the crystal and magnetic structures of BiFeO3. J. Phys. C Solid State Phys. 13, 1931–1940 (1980).

20. 20.

Catalan, G. & Scott, J. F. Physics and applications of bismuth ferrite. Adv. Mater. 21, 2463–2485 (2009).

21. 21.

Smolenskiĭ, G. A. & Chupis, I. E. Ferroelectromagnets. Sov. Phys. Usp. 25, 475 (1982).

22. 22.

Balke, N. et al. Enhanced electric conductivity at ferroelectric vortex cores in BiFeO3. Nat. Phys 8, 81–88 (2012).

23. 23.

Morozovska, A. N., Vasudevan, R. K., Maksymovych, P., Kalinin, S. V. & Eliseev, E. A. Anisotropic conductivity of uncharged domain walls in BiFeO3. Phys. Rev. B Condens. Matter 86, 085315–085313 (2012).

24. 24.

Kim, Y. M. et al. Interplay of octahedral tilts and polar order in BiFeO3 films. Adv. Mater. 25, 2497–2504 (2013).

25. 25.

Vasudevan, R. K. et al. Domain wall conduction and polarization-mediated transport in ferroelectrics. Adv. Funct. Mater. 23, 2592–2616 (2013).

26. 26.

Kim, Y. M. et al. Direct observation of ferroelectric field effect and vacancy-controlled screening at the BiFeO3/LaxSr1-xMnO3 interface. Nat. Mater. 13, 1019–1025 (2014).

27. 27.

Winchester, B. et al. Electroelastic fields in artificially created vortex cores in epitaxial BiFeO3 thin films. Appl. Phys. Lett. 107, 052903 (2015).

28. 28.

Holakovský, J. A new type of the ferroelectric phase transition. Phys. Status Solidi B 56, 615–619 (1973).

29. 29.

Scott, J. F. Iso-structural phase transitions in BiFeO3. Adv. Mater. 22, 2106–2107 (2010).

30. 30.

Gopalan, V. & Litvin, D. B. Rotation-reversal symmetries in crystals and handed structures. Nat. Mater. 10, 376–381 (2011).

31. 31.

Uwe, H. & Sakudo, T. Stress-induced ferroelectricity and soft phonon modes in SrTiO3. Phys. Rev. B Condens. Matter 13, 271–286 (1976).

32. 32.

Eliseev, E. A., Glinchuk, M. D., Gopalan, V. & Morozovska, A. N. Rotomagnetic couplings influence on the magnetic properties of antiferrodistortive antiferromagnets. J. Appl. Phys. 118, 144101 (2015).

33. 33.

Suresh, P. & Srinath, S. Effect of La substitution on structure and magnetic properties of sol-gel prepared BiFeO3. J. Appl. Phys. 113, 17D920 (2013).

34. 34.

Rusakov, D. A. et al. Structural evolution of the BiFeO3−LaFeO3 system. Chem. Mater. 23, 285–292 (2010).

35. 35.

Selbach, S. M., Tybell, T., Einarsrud, M. A. & Grande, T. The ferroic phase transitions of BiFeO3. Adv. Mater. 20, 3692–3696 (2008).

36. 36.

Fujii, K. et al. Experimental visualization of the Bi–O covalency in ferroelectric bismuth ferrite BiFeO3 by synchrotron X-ray powder diffraction analysis. Phys. Chem. Chem. Phys. 15, 6779–6782 (2013).

37. 37.

Karpinsky, D. V. et al. Evolution of electromechanical properties of Bi1-xPrxFeO3 solid solutions across the rhombohedral–orthorhombic phase boundary: Role of covalency. J. Alloys Compd. 638, 429–434 (2015).

38. 38.

Levin, I. et al. Displacive phase transitions and magnetic structures in Nd-substituted BiFeO3. Chem. Mater. 23, 2166–2175 (2011).

39. 39.

Karpinsky, D. V. et al. Temperature and composition-induced structural transitions in Bi1-xLa(Pr)xFeO3 ceramics. J. Am. Ceram. Soc. 97, 2631–2638 (2014).

40. 40.

Karpinsky, D. V. et al. Evolution of crystal structure and ferroic properties of La-doped BiFeO3 ceramics near the rhombohedral-orthorhombic phase boundary. J. Alloys Compd. 555, 101–107 (2013).

41. 41.

Shoemaker, D. P., Seshadri, R., Tachibana, M. & Hector, A. L. Incoherent Bi off-centering in Bi2Ti2O6O′ and Bi2Ru2O6O′: Insulator versus metal. Phys. Rev. B Condens. Matter 84, 064117 (2011).

42. 42.

Arnold, D. C., Knight, K. S., Catalan, G., Redfern, S. A. & Scott, J. F. The β-to-γ Transition in BiFeO3: A powder neutron diffraction study. Adv. Funct. Mater. 20, 2116–2123 (2010).

43. 43.

Palewicz, A., Przeniosło, R., Sosnowska, I. & Hewat, A. W. Atomic displacements in BiFeO3 as a function of temperature: neutron diffraction study. Acta Crystallogr. B Struct. Sci. 63, 537–544 (2007).

44. 44.

Karimi, S., Reaney, I. M., Han, Y., Pokorny, J. & Sterianou, I. Crystal chemistry and domain structure of rare-earth doped BiFeO3 ceramics. J. Mater. Sci. 44, 5102 (2009).

45. 45.

Arnold, D. C. Composition-driven structural phase transitions in rare-earth-doped BiFeO3 ceramics: a review”. IEEE Trans. Ultrason. Ferroelectr. Freq. Control 62, 62–82 (2015).

46. 46.

Khomchenko, V. A., Troyanchuk, I. O., Többens, D. M., Sikolenko, V. & Paixão, J. A. Composition-and temperature-driven structural transitions in Bi1-xCaxFeO3 multiferroics: a neutron diffraction study. J. Phys. Condens. Matter 25, 135902 (2013).

47. 47.

Megaw, H. D. & Darlington, C. N. W. Geometrical and structural relations in the rhombohedral perovskites. Acta Crystallogr. A 31, 161–173 (1975).

48. 48.

Okuno, Y. & Sakashita, Y. Born effective charges and piezoelectric coefficients of BiXO3. Jpn. J. Appl. Phys. 48, 09KF04 (2009).

49. 49.

Barrett, J. H. Dielectric constant in perovskite type crystals. Phys. Rev. 86, 118–120 (1952).

50. 50.

Gu, Y., Rabe, K., Bousquet, E., Gopalan, V. & Chen, L. Q. Phenomenological thermodynamic potential for CaTiO3 single crystals. Phys. Rev. B Condens. Matter 85, 064117 (2012).

51. 51.

Morozovska, A. N., Khist, V. V., Glinchuk, M. D., Gopalan, V. & Eliseev, E. A. Linear antiferrodistortive-antiferromagnetic effect in multiferroics: physical manifestations. Phys. Rev. B Condens. Matter 92, 054421 (2015).

52. 52.

Kallaev, S. N. et al. Heat capacity and dielectric properties of multiferroics Bi1-xGdxFeO3 (x=0–0.20). Phys. Solid State 56, 1412–1415 (2014).

53. 53.

Amirov, A. A. et al. Specific features of the thermal, magnetic, and dielectric properties of multiferroics BiFeO3 and Bi0.95La0.05FeO3. Phys. Solid State 51, 1189–1192 (2009).

54. 54.

Karpinsky, D. V. et al. Structural and magnetic phase transitions in Bi1-xCaxFe1-xMnxO3 multiferroics. J. Alloys Compd. 692, 955–960 (2017).

55. 55.

Karpinsky, D. V. et al. Crystal structure and magnetic properties of Bi1-xCaxFe1-xMn(Ti)xO3 ceramics across the phase boundary. J. Mater. Sci. 51, 10506–10514 (2016).

56. 56.

Kamba, S. et al. Infrared and terahertz studies of polar phonons and magnetodielectric effect in multiferroic BiFeO3 ceramics. Phys. Rev. B Condens. Matter 75, 024403 (2007).

57. 57.

Lobo, R. P. S. M., Moreira, R. L., Lebeugle, D. & Colson, D. Infrared phonon dynamics of a multiferroic BiFeO3 single crystal. Phys. Rev. B Condens. Matter 76, 172105 (2007).

58. 58.

Arnold, D. C., Knight, K. S., Morrison, F. D. & Lightfoot, P. Ferroelectric-paraelectric transition in BiFeO3: crystal structure of the orthorhombic β phase. Phys. Rev. Lett. 102, 027602 (2009).

59. 59.

Kornev, I. A. & Bellaiche, L. Nature of the ferroelectric phase transition in multiferroic BiFeO3 from first principles. Phys. Rev. B Condens. Matter 79, 100105 (2009).

60. 60.

Kennedy, B. J., Howard, C. J. & Chakoumakos, B. C. Phase transitions in perovskite at elevated temperatures - a powder neutron diffraction study. J. Phys. Condens. Matter 11, 1479 (1999).

61. 61.

Morozovska, A. N. et al. Defect thermodynamics and kinetics in thin strained ferroelectric films: the interplay of possible mechanisms. Phys. Rev. B Condens. Matter 89, 054102 (2014).

62. 62.

Troyanchuk, I. O. et al. Phase transitions, magnetic and piezoelectric properties of rare-earth-substituted BiFeO3 ceramics. J. Am. Ceram. Soc. 94, 4502–4506 (2011).

63. 63.

Rodríguez-Carvajal, J. Recent advances in magnetic structure determination by neutron powder diffraction. Phys. B 192, 55–69 (1993).

## Acknowledgements

The work of D.V.K., M.V.S., S.A.G. and I.O.T. was supported by the Russian Science Foundation (project # 15-19-20038). Neutron diffraction experiments have been supported by the European Commission under the 7th Framework Programme through the ‘Research Infrastructure’ action of the ‘Capacities’ Programme, NMI3-II Grant number 283883’. The work at Penn State is supported by the U.S. Department of Energy, Office of Basic Energy Sciences, Division of Materials Sciences and Engineering under Award FG02-07ER46417 (FX and LQC) and by the NSF MRSEC under Grant No. DMR-1420620 (F.X. and V.G.). A.N.M. and E.A.E. acknowledge the Center for Nanophase Materials Sciences, which is a DOE Office of Science User Facility, CNMS2016-061.

## Author information

D.V.K., I.O.T., A.F. and M.V.S. conducted structural measurements and wrote the experimental part of the paper. E.A.E. and F.X. performed theoretical calculations, supervised by M.D.G., V.G. and L.Q.C., I.O.T. and S.A.G. prepared the samples. A.N.M. proposed theoretical research ideas and formulated the problem, wrote the introductive, theoretical and discussion parts of the paper. All co-authors densely worked on the results analyses and text improvements.

### Competing interests

The authors declare no competing financial interests.

Correspondence to Dmitry V. Karpinsky.

## Rights and permissions

Reprints and Permissions

• #### DOI

https://doi.org/10.1038/s41524-017-0021-3

• ### Advances in magnetoelectric multiferroics

• N. A. Spaldin
•  & R. Ramesh

Nature Materials (2019)

• ### Crystallization, non-isothermal kinetics and structural analysis of nanocrystalline multiferroic bismuth ferrite (BiFeO3) synthesized by combustion method

• M. Manonmani
• , V. Jaikumar
• , S. Gokul Raj
•  & G. Ramesh Kumar

Journal of Thermal Analysis and Calorimetry (2019)

• ### Configurable topological textures in strain graded ferroelectric nanoplates

• Kwang-Eun Kim
• , Seuri Jeong
• , Kanghyun Chu
• , Jin Hong Lee
• , Gi-Yeop Kim
• , Fei Xue
• , Tae Yeong Koo
• , Long-Qing Chen
• , Si-Young Choi
• , Ramamoorthy Ramesh
•  & Chan-Ho Yang

Nature Communications (2018)

• ### A thermodynamic potential for barium zirconate titanate solid solutions

• Jinlin Peng
• , Dongliang Shan
• , Yunya Liu
• , Kai Pan
• , Chihou Lei
• , Ningbo He
• , Zhenyu Zhang
•  & Qiong Yang

npj Computational Materials (2018)