Ultrafast optically induced ferromagnetic/antiferromagnetic phase transition in GdTiO from first principles
pacs:
I Abstract
Epitaxial strain and chemical substitution have been the workhorses of functional materials design. These static techniques have shown immense success in controlling properties in complex oxides through the tuning of subtle structural distortions. Recently, an approach based on the excitation of an infrared active phonon with intense midinfrared light has created an opportunity for dynamical control of structure through special nonlinear coupling to Raman phonons. We use firstprinciples techniques to show that this approach can dynamically induce a magnetic phase transition from the ferromagnetic ground state to a hidden antiferromagnetic phase in the rare earth titanate GdTiO for realistic experimental parameters. We show that a combination of a JahnTeller distortion, Gd displacement, and infrared phonon motion dominate this phase transition with little effect from the octahedral rotations, contrary to conventional wisdom.
Ii Introduction
The properties of ABO perovskites arise not only from the crystal structure generally, they also depend sensitively on small structural distortions, in contrast with most other inorganic materials families. For example, the magnetoresistive properties of perovskite manganites,^{1} and metalinsulator transitions in the perovskite nickelate^{2; 3; 4} and titanate families^{5; 6} are strongly linked with socalled ‘rotations’ of the BO octahedra, which are associated with zoneboundary phonons of the cubic perovskite structure. Researchers have learned how to successfully tune this dependence using a variety of techniques, such as epitaxial strain^{7; 8} and stabilization,^{9} pressure,^{10} and doping.^{1} Dynamical control of the properties of perovskites has been far more challenging, and has so far been largely based on lightinduced electronic excitation or temperature changes.^{11; 12; 13}
Recent experiments have demonstrated the potential for modifying the properties of materials using ultrafast optical pulses to selectively and coherently excite particular phonon modes. One such mechanism involves optical excitation of an IRactive phonon , which produces a displacement of a Ramanactive mode due to a particular anharmonic coupling between the modes of the form (although the relevant coupling term is not always clear in experimental studies, most theoretical works so far have focused on couplings of the form ). This nonlinear phononic effect, and the subtle structural changes it induces, has been invoked to interpret observations of a fiveordersofmagnitude decrease in resistivity in PrCaMnO,^{14; 15} a material that is insulating at equilibrium at all measured temperatures.^{16; 17} Additionally, the charge and orbitallyordered phase of LaSrMnO can be destabilized well below the orbital ordering temperature by selective vibrational excitation of an MnO stretching mode.^{18} In a particularly notable example, the observation of transient superconductivity above the transition temperature in vibrationally excited YBaCuO was also attributed to a nonlinear phononic effect.^{19} Experiments that exploit this mechanism have, together with firstprinciples calculations,^{15; 20; 21; 22} produced profound new insights into the structural dynamics of materials out of equilibrium.
Here, we use the family of orthorhombic perovskite titanates to develop a generalized theory of nonlinear phononics, which we use in combination with density functional theory calculations to reveal the existence of a hidden magnetic phase in GdTiO accessible under experimentally realistic conditions. It is generally understood that rotations of the TiO octahedra strongly affect the coupling between neighboring Ti orbitals and therefore control the bandwidth and magnetic superexchange interactions. In the equilibrium phase diagram, the rotation amplitudes increase as the size of the rare earth cation decreases. This change in rotation amplitudes is accompanied by a change in the magnetic ground state, with GAFM SmTiO and FM GdTiO straddling the boundary between the AFM and FM parts of the phase diagram. Interestingly, an Atype AFM phase has been speculated to exist between SmTiO and GdTiO, however no stoichiometric system exists between these materials. Although it may seem that the AAFM phase could be obtained by judiciously tuning octahedral rotation angles, Mochizuki and Imada^{5} point out that the JahnTeller mode plays a critical role in stabilizing the AAFM phase (Pavarini and coworkers had a similar insight^{23}). In particular, the AAFM phase requires the combination of a “strong” JahnTeller distortion (as in GdTiO) and “moderate” octahedral rotation distortion (as in SmTiO). However, the JahnTeller distortion is coupled to the rotations and weakens rapidly as the rotations decrease. There is no known way to independently control the relative magnitudes of these distortions. Indeed, as far as we are aware, neither bulk chemical techniques (solid solutions) nor strain engineering have been able to experimentally stabilize the AAFM phase in any perovskite titanate.
We demonstrate that the nonlinear phononics mechanism can be used to essentially “switch off” the net magnetization in GdTiO by inducing an AAFM phase. Although we find that the AAFM phase can be realized dynamically in bulk GdTiO, the required peak electric fields are quite high. However, we show that a modest amount of epitaxial strain can position GdTiO closer to the phase boundary, such that the AAFM phase is induced at low peak electric fields of the optical pulse. We also elucidate the origin of the magnetic transition in terms of the structural distortions that accompany the optical excitation. Surprisingly, although the octahedral rotation distortions are affected by optical excitation, their amplitudes change very little from their equilibrium values and their effect on the magnetic configuration energy is negligible. Instead, we find that it is primarily the JahnTeller mode that plays the key role in switching off the net magnetization in GdTiO, and dynamically inducing the AAFM phase. These are precisely the conditions under which Mochizuki and Imada speculated that the AAFM phase could be realized. Our results demonstrate that the nonlinear phononics mechanism can be leveraged to modulate the complex interplay between structural distortions in perovskites, and their electronic and magnetic properties. We also shed light on the structural dynamics of perovskites out of equilibrium, a regime in which these materials have been little explored.
Iii Results
iii.1 Theory
TwoMode Model.– An expansion of the lattice energy clarifies the nonlinear phononics process for a centrosymmetric crystal in which the IR and Raman modes have different symmetry. For simplicity we first consider a model involving only a single IR mode and a single Raman mode (this model is similar to that presented in Refs. 24 and 15). The lattice energy is defined by
(1) 
where and are, respectively, the frequency and amplitude of the IR (Raman) phonon and is a coupling coefficient. The last term contains the polarization change in the crystal, defined as , where , known as the mode effective charge,^{25} describes the strength of the coupling between the excited IR phonon and the electric field of the light pulse () (we ignore the effects of the oscillating IR mode on the polarization). Note that since is invariant under all symmetry operations of the crystal, in order for to be nonzero, must also be invariant under all symmetry operations of the crystal. By convention, we label this totally symmetric mode . (Nonlinear coupling of the form , linear in the IR mode displacement and quadratic in Raman mode displacement, are not allowed because of inversion symmetry (taking ). In noncentrosymmetric crystals, some IR phonons are fully symmetric. In this case, these terms are allowed.)
We desire a large, static displacement of the Raman mode that is longlived on the timescale of the IR mode. Taking derivatives of Eqn. 1 with respect to the IR and Raman amplitudes for a fixed electric field direction,
(2)  
(3) 
reveals that this depends on three materialsspecific criteria: 1) Strong coupling between the excited IR mode and the incoming light pulse (large ^{26}), 2) Strong coupling between the excited IR mode and the Raman mode (large ) and; 3) The frequency of the IR phonon should be higher than that of the Raman mode, such that the Raman mode does not oscillate within the period of the IR mode. Eqn. 3 also shows that as long as the IR phonon is ringing, there will be a unidirectional force on the Raman mode.
Eqns. 1 – 3 provide useful insight into the basic physical process exploited in the nonlinear phononics mechanism, however real materials contain many IR and Raman phonons. In general, when an IR mode is optically excited, all symmetryallowed modes will contribute to the dynamical response. The twomode model ignores the dynamic coupling between Raman modes and will provide a poor description of the structural dynamics when the coupling between these modes is strong. Additional complications arise when more than one IR mode is excited by the incoming light pulse, as shown in Figure 2. As the oscillator strength of the second mode increases, the structural dynamics becomes increasingly complicated, and the twomode model will again fail to provide a correct description. Ultimately, without knowing the relevant nonlinear coupling coefficients explicitly, it is not possible to predict a priori which modes will be strongly coupled or have a large contribution to the dynamical response. Hence, all IR and Raman phonons should be treated on equal footing. We present a model below that does just that.
ManyMode Model.– In order to make the problem concrete and tractable, here we focus on the case where light is polarized along the principal crystallographic axes and parallel with the particular IR phonon we wish to excite. Additionally, we use the perovskite crystal structure as a starting point, without loss of generality, because it is the most stable crystal structure for more than half of all perovskites, including GdTiO (extension of this model to arbitrary crystal systems – with or without inversion symmetry – is straightforward, but cumbersome).
The orthorhombic Pbnm structure has 20 atoms per primitive cell and therefore 60 zonecentered phonons. There are 25 IRactive phonons: 9 polarized along each of the a and baxes ([100] and [010]), and 7 polarized along the caxis ([001]). Additionally, there are 7 Ramanactive phonons of symmetry that are accessible through the nonlinear phononics process. Expanded to third order, Eqn. 1 becomes,
(4)  
We use Latin indices for IRactive phonons and Greek indices for Ramanactive phonons. Again, leads to a unidirectional displacement of mode but now multiple Raman modes may be displaced by selective excitation of IR mode . The terms allow for coupling between two different IR modes and a Raman mode. Juraschek and coworkers explored this coupling term theoretically for the case of two IR phonons polarized along different directions, where a coupling to non Raman phonons is induced.^{22} Nova et al. have explored this term experimentally by simultaneously exciting two IR phonons with different polarizations in ErFeO.^{27} This term also couples two IR phonons with parallel polarization, again displacing an Raman mode. The term couples three displaced Raman modes. Since multiple IR modes are now included the change in the polarization must also be expanded as .
Taking derivatives of Eqn. 4 gives the equations of motion for the nonlinear phononics process to third order:
(5)  
(6)  
We describe below how we integrate the manymode model with density functional theory calculations to obtain a firstprinciples description of the structural dynamical response of a given material to optical excitation.
Integrating the ManyMode Model with FirstPrinciples Calculations.– Figure 3 shows the workflow we have implemented for obtaining the required inputs to the manymode model, and for exploring the dynamical response of materials induced through the nonlinear phononics mechanism. A number of different steps are involved:

Relax the crystal structure of interest The atomic positions and lattice parameters of the given material are fully relaxed using density functional theory. Forces must be tightly converged to ensure phonon properties are accurate.

Compute phonon properties and Born charges Phonon frequencies, eigenvectors and Born effective charges are calculated using density functional perturbation theory. The eigenvectors and Born charges are required for calculation of the mode effective charges, which appear in Eqns. 5 and 6, along with the phonon frequencies.

Model lattice contribution to the dielectric function The phonon properties and Born charges are also used to model the lattice dielectric function. This is not strictly required for simulating the dynamical response, however it is helpful for connecting our model with experimental information, such as the reflectivity and zerofrequency dielectric response.

Compute thirdorder coupling terms The thirdorder nonlinear coupling coefficients , and are calculated with density functional theory using finite differences. Details are provided in the Methods section.

Explore consequences for functional properties The manymode model outputs a set of IR and Raman amplitudes, which are added back to the relaxed crystal structure to give a snapshot of the dynamical response of the material to optical excitation. The consequences for the band gap, magnetic configurations, and other properties can then be explored using density functional theory.
iii.2 Magnetic phase transition in GdTiO
GdTiO adopts the distorted crystal structure with a ferromagnetic alignment of the Ti 3d spins below 30 K. As mentioned above, GdTiO contains a number of IRactive modes and we found it was possible to position the system both closer to and further away from the FM – AAFM phase boundary, depending on which mode we chose to excite. We compared the magnetic configuration energy of the AAFM, GAFM and CAFM states with the FM state for excitation of various IR modes and identified a 72.4 meV phonon polarized along the crystallographic axis ([001] direction) as being most likely to induce the desired magnetic phase transition. For all the results presented below, we checked that the material remains insulating. Figure 4 shows the difference in the magnetic configuration energy between the FM and AAFM states as a function of peak electric field (we also checked the energy difference between the FM phase and the other AFM orders but the AAFM phase remains closest in energy to FM over the entire peak electric field range). The optically induced change in magnetic energy results from both the oscillating IR phonons (due to a biquadratic spinphonon coupling) and the unidirectionally displaced Raman phonons. This is most clearly understood by expanding the outofplane (axis) Heisenberg exchange constant, , in both the oscillating excited mode and the total unidirectionally displaced Raman mode amplitudes . By symmetry alone, , where and are negative coefficients in this case. The interpretation is that the oscillating IR phonon induces a change in the effective exchange constants because it appears as . That is, although the time average of is zero – the average amplitude does not change – the time average of is not zero. This is essentially the same physics that produces the unidirectional displacement of the Raman phonons, since the IR mode also appears as in the relevant coupling term in Equations 1 and 4. This effect of the IR phonon on magnetism has not been addressed previously in the nonlinear phononics literature, however our results suggest that coupling between the spins and IR phonons cannot be ignored.
Figure 4 shows that although the system approaches the AAFM state with increasing peak electric field, the FM state remains stable over the entire electric field range. The magnetic transition could be induced by simply increasing the peak electric field, however it is desirable to keep the peak electric field as low as possible, in order to minimize sample damage and heating. We therefore need some way to position GdTiO closer to the FM – AAFM phase boundary.
Recent work has shown how strain engineering can tune LaCaMnO into a chargeordered insulating phase with extreme photosusceptibility.^{13} Ultrafast optical excitation of the strained material induces a transition to a longlived, hidden metallic phase. Likewise, we calculated the energy difference between the AAFM, GAFM, CAFM and FM states as a function of both tensile and compressive biaxial strain (the strain was applied in the plane perpendicular to the axis). Figure 5a shows that both tensile and compressive strain decrease the energy of all of the AFM phases relative to the FM state, however the AAFM phase again remains closest in energy to the FM state. In fact, epitaxial strain by itself can induce the AAFM phase in GdTiO. However, the strains required (tensile strains greater than 2% and compressive strains greater than 2.5%) are quite large and likely unrealizable in real GdTiO thinfilms. Nonetheless, calculation of the relevant exchange coefficients and magnetic does show how strain moves GdTiO closer to the FM – AAFM phase boundary. The difference between the FM and AAFM phases corresponds to a change from FM to AFM ordering along the axis of the crystal. The outofplane exchange coefficient () tracks this energy difference well, as Figure 5b shows. As the inplane lattice constants increase, the inplane (plane) exchange coefficients () decrease. This leads to a steady decrease in the critical for tensile strain (Figure 5c). Because of the sharp decrease in the outofplane exchange coefficient () with tensile strain we look for optically induced magnetic switching at tensile strain, where the critical temperature is still large and is still greater than zero. (+1.5% tensile strain corresponds approximately to growth on GdScO.)^{7; 28} Previous theoretical work has also explored strain as a possible strategy for stabilizing the AAFM phase in rareearth titanates (and specifically GdTiO) although much larger values of strain were typically required.^{29; 30; 31; 32}
Figure 6(a) now shows that excitation of the same IRactive phonon (now at 70.8 meV in the strained material) pushes GdTiO across the phase boundary, stabilizing the AAFM phase at lower peak electric fields than in the unstrained system. We find that the combined peak IR and Raman response stabilizes the AAFM phase for MV/cm. The average unidirectional Raman response alone requires MV/cm to induce this change, a still modest peak electric field value. These results suggest that a previously unidentified magnetic phase of the rare earth titanates may be reached dynamically by the nonlinear phononics process.
What is the structural origin of the switch from the FM to the AAFM phase? To answer this question, we use the symmetryadapted modes of the parent cubic phase as a basis to decompose the nonequilibrium structural changes into contributions from different distortions.(See Supplementary Information) Because the Raman displacement is quasistatic, we focus on this aspect of the structural changes. We group the components of the Raman modes into three categories, which have been highlighted in the titanate literature because of their effect on electronic and magnetic properties in the equilibrium phase diagram: two octahedral rotation distortions (transforming like the irreducible representations , for the rotation in Glazer notation, and for the inphase rotation), three distortions that change TiO bond lengths (:O , :O, and :O represent distortions of the octahedral oxygen environment) and modes involving displacements of the Gd cations (:Gd and :Gd). Each phonon is a linear combination of all three kinds of structural distortion, although some modes may be dominated by a particular type of distortion.
The two most commonly discussed structural distortions in the perovskite literature are the outofphase :O and inphase :O octahedral rotations. As the schematic phase diagrams in Figure 7 show, the amplitudes of these distortions increase in moving from La to Y in the rareearth titanate series ATiO (A=La,Nd,Sm,Gd,Y); there is a concomitant change in magnetic order from GAFM in LaTiO to FM in YTiO. This change in magnetic order is usually understood as a response to changes in the TiOTi bond angles (which are directly affected by the rotation amplitudes) and subsequent changes in the magnetic superexchange interactions. However, if we try to interpret our results in terms of this picture, we find something unexpected. First, let us consider our strain results and focus on small strains 1% around the bulk value, the region that is most likely to be applicable to thinfilm experiments. Figure 5a shows that small tensile strains favor the AAFM phase, whereas small compressive strains further stabilize the FM ground state. Now, how does this compare with the correlation between rotation angles and magnetism in bulk? The schematic phase diagrams in Figure 7 show that increasing the and rotation angles favors the FM phase, whereas decreasing them favors the AFM phase. However, Figure 7 also shows that compressive strain changes the and rotation angles such that the system is pushed towards the AFMFM phase boundary, whereas small tensile strains push the system further into the FM region (red shaded region). This is the opposite behavior to what we would expect based on the results in Figure 5. Quite astonishingly, if we now consider the dynamical response (blue shaded region), we see that as the peak electric field increases, the angle changes in such a way that the system moves away from the AFMFM phase boundary. Moreover, the change in rotation angle across the whole range of strains and peak electric fields is very small, barely more than 1. Similar results hold for the rotation (Figure 7b), where the change in rotation angle is even smaller. Clearly, considering only changes in rotation angles cannot explain the transition to AAFM order under optical excitation in GdTiO. (The strain results are essentially a volume effect but we defer further discussions to a forthcoming publication so we can focus here on the dynamical response.)
If changes in rotation angles do not induce a change in magnetic order in GdTiO through the nonlinear phononics mechanism, then which structural distortion is responsible? Figure 8a shows the percentage change in the symmetryadapted mode distortion amplitudes as a result of optical excitation (the same plot showing absolute changes can be found in the Supplementary Information). Positive changes indicate that the distortion increases in magnitude relative to the equilibrium structure, whereas negative changes indicate that the distortion decreases in magnitude. The JahnTeller mode undergoes the largest change by far, increasing in magnitude with respect to the equilibrium structure (this corresponds to a 158% change in the JahnTeller amplitude at for a peak electric field of 7 MV/cm). The mode, which changes the O and Gd environments, also increases in magnitude. In contrast, the two octahedral rotation modes, and , change very little. Contrary to conventional wisdom, our results suggest that judicious tuning of octahedral rotation angles is unlikely to produce the desired AAFM phase under experimentally realizable conditions. Instead, the JahnTeller mode is playing the key role in the magnetic switching process. To test this insight, we recalculated the energy difference between the FM and AAFM phases while selectively returning specific sets of distortions to their equilibrium values. Figure 8(b) shows that when all modes are returned to their equilibrium values except for the two rotation modes, the FM phase is stable over the entire range of peak electric fields we consider. When all modes are returned to their equilibrium values except the rotations and those involving displacements of the Gd ions, there is a crossover from the FM to the AAFM phase at high peak electric fields. Inclusion of the JahnTeller mode pushes the crossover to lower peak electric fields.
Iv Discussion
Our results demonstrate that the nonlinear phononics mechanism can be exploited to dynamically stabilize the AAFM phase of GdTiO in the manner suggested by Mochizuki and Imada – by modulating the amplitude of the JahnTeller mode while changing the rotations very little, a combination of conditions that is extremely difficult to realize in either bulk or thinfilm GdTiO. The “indirectness” of the nonlinear phononics process – light is used to excite a particular phonon mode, which then produces a displacement of another set of modes through anharmonic coupling – is sometimes seen as a disadvantage of the mechanism, since ions are only displaced from their equilibrium values by very small amounts. In this case however, the indirect nature of the mechanism is probably precisely what allows the stabilization of the AAFM phase. Octahedral rotations are very lowenergy distortions, in that they lower the energy of the cubic perovskite phase by a significant amount (over 1 eV in some cases) and have very large amplitudes in the distorted structure. Large amounts of energy, supplied through epitaxial strain, for example, are therefore required to change their amplitudes. In contrast, the amplitude of the JahnTeller mode is typically orders of magnitude smaller. We speculate that the nonlinear phononics mechanism supplies just enough energy to induce changes in the JahnTeller mode in GdTiO, but not enough to significantly affect the octahedral rotations. Of course, the dynamical response of other perovskites may be different; the structures of perovskites out of equilibrium are only beginning to be explored in detail, and so much more work is needed in this area.
There is some experimental support for our findings. Zhang and coworkers^{33} grew very thinfilms of GdTiO, such that the octahedral rotations are suppressed. However, they found that ferromagnetism persisted, even in the absence of rotation distortions, and posit that the magnetism is controlled by “the narrow bandwidth, exchange and orbital ordering”. Regardless of the mechanism, clearly octahedral rotations are not as essential to the magnetic properties of GdTiO as has perhaps been assumed. Experimental confirmation of the dynamical magnetic response can in principle be achieved by timeresolved Faraday or Kerr probes^{34} referenced to the infrared lattice excitation, while corresponding birefringence measurements can detect changes in the JahnTeller mode amplitude.
We conclude by emphasizing that we are emphatically not claiming that octahedral rotations are never important in giving rise to the electronic and magnetic properties of perovskites. There is a large and wellestablished theoretical and experimental literature unambiguously showing the various ways in which these distortions affect the properties of perovskites. However, in the case of the rare earth titanates at least, it appears that octahedral rotations merely “set the stage” for the magnetic properties, while much smaller structural distortions (such as the JahnTeller mode) work together to induce the actual magnetic ground state.
V Methods
Firstprinciples calculations. Firstprinciples calculations were performed using projector augmented wave potentials and the PBEsol + U exchangecorrelation functional, as implemented in VASP. Onsite Coulomb and exchange parameters of = 5 eV, and = 0.64 eV were used^{35} (we found no qualitative change in our results for reasonable variations of ). We use a 600 eV plane wave cutoff and a MonkhorstPack grid. These choices produced good agreement with available experimental structural data for ATiO (A=La,Nd,Sm,Gd,Y). ^{36}(See Supplemenatary Figure 3 for detailed comparison of GdTiO.) For GdTiO we find the lattice constants Å, Å, Å, in good agreement with available hightemperature experimental values Å, Å, Å. Phonons and Born charges were calculated using density functional perturbation theory within VASP and used to calculate dynamical mode effective charges () and to model the frequencydependent dielectric response. ^{37}
Magnetic exchange and critical temperature. Magnetic exchange constants were calculated by fitting the A, C, GAFM, and FM configuration energies to a Heisenberg model , where labels nearest neighbors for inplane () and outofplane () spins. We note that including both Raman and IR phonons in the Heisenberg model results in an effective exchange coupling , with both and reaching negative values, inducing the FM to AAFM phase transition. Here is the excited IR phonon and is the total induced Raman distortion  see Fig. 8a.) The critical temperature is evaluated from the spin molecular field theory result with total exchange field of per spin.
Strain response of GdTiO. Strain was considered for both common growth modes of Pbnm perovskites. The first corresponds to growth along the axis and maintains the Pbnm space group (# 62). The second corresponds to growth perpendicular to the axis. This lowers the symmetry to (#11). We find that for tensile strain on orthorhombic substrates, the Pbnm phase is generally preferred. In the specific case addressed in the main text, +1.5% strain corresponds approximatly to growth on GdScO.
Calculation of nonequilibrium force constants. To calculate the nonequilibrium force constants, we use a finitedifference approach where force constant matrices () are calculated for each phonon, displaced about equilibrium. The nonequilibrium force constant matrices are then used to calculate the nonlinear coupling coefficients between the and the IR phonons (, , ) by projecting the force constant matrices into the basis of the equilibrium structure. For example, the realspace coupling between Raman mode , and IR modes and is found by . Here, is the realspace eigendisplacement amplitude associated with phonon . In this approach requires 15 phonon calculations: 1 for the equilibrium structure, and two increments for each of the 7 modes. All thirdorder terms that couple to are found in this way. We therefore have all necessary thirdorder coupling terms for the nonlinear phononics process. This approach is significantly less computationally burdensome than finitedifference techniques that calculate all thirdorder terms, or frozenphonon techniques that require converged meshes in phonon amplitude. In the frozen phonon technique would require 175 twodimensional meshes to calculate , 651 threedimensional meshes to calculate , and 84 threedimensional meshes to calculate all . Regardless, we have tested our computational approach against the frozen phonon method for multiple randomly selected , , and and found good agreement. We note that this computational technique may also be used for coupling to non Raman modes. In that case labels the realspace eignedisplacement amplitude of the non mode of interest.
Optical pulse characteristics. Phonon frequencies, dynamical mode effective charges, nonlinear coupling coefficients, and optical pulse characteristics are fed into Eqns. 5 and 6, which are numerically simulated to find the dynamical response. We include all IR phonons polarized parallel to the incident light as well as all phonons in our simulations. We fix the timescale (fullwidth at halfmaximum) of a Gaussian pulse to be 300 fs and vary the peakelectric field () from 1 MV/cm to 7 MV/cm for carrier frequencies on resonance with the desired IR phonon (for a Gaussian pulse the extrinsic quantity affects the Raman subspace; the electric field range has been chosen consistent with experimentally reported values.^{14; 38})
Vi Data Availability Statement
Data is available upon reasonable request from the corresponding author.
Vii Acknowledgments
This work was supported by the National Science Foundation. NAB was supported by DMR1550347. Initial work on this project by GK was supported by DMR1550347, and subsequently by the Cornell Center for Materials Research with funding from the National Science Foundation MRSEC program (DMR1719875). This work used the Extreme Science and Engineering Discovery Environment (XSEDE) (through allocation DMR160052), which is supported by National Science Foundation grant number ACI1548562. We thank Farhan Rana, Jeffrey Moses, Craig Fennie and Gregory Fuchs for helpful discussions.
Viii Competing Interests
The authors declare no competing financial interests.
Ix Author Contributions
The authors contributed equally to this work.
X Supplementary Information
Supplementary information is available at the npj Quantum Materials’ website.
Xi References
References
 (1) Hwang, H. Y., Cheong, S., Radaelli, P. G., Marezio, M., & Batlogg, B. Lattice effects on the magnetoresistance in doped LaMnO. Phys. Rev. Lett., 75, 914–917 (1995).
 (2) Medarde, M. L. Structural, magnetic and electronic properties of RNiO perovskites (R = rare earth). J. Phys.: Condens. Matter, 9, 1679–1707 (1997).
 (3) Zhou, J. & Goodenough, J. B. Chemical bonding and electronic structure of RNiO (R = rare earth). Phys. Rev. B, 69, 153105 (2004).
 (4) Catalan, G. Progress in perovskite nickelate research. Phase Transitions, 81, 729?749 (2008).
 (5) Mochizuki, M. & Imada, M. Orbital physics in the perovskite Ti oxides. New J. Phys., 6, 154 (2004).
 (6) Pavarini, E. et al. Mott transition and suppression of orbital fluctuations in orthorhombic 3d perovskites. Phys. Rev. Lett., 92, 176403 (2004).
 (7) Choi, K. J. et al. Enhancement of ferroelectricity in strained BaTiO thin films. Science, 306, 1005–1009 (2004).
 (8) Lee, J. H. et al. A strong ferroelectricferromagnet created by means of spinlattice coupling. Nature, 466, 954–958 (2010).
 (9) Kim, T. H. et al. Polar metals by geometric design. Nature, 533, 68–71 (2016).
 (10) Hiroi, Z., Takano, M., Azuma, M., & Takeda, Y. A new family of copper oxide superconductors SrCuO stabilized at high pressure. Nature, 364, 315–317 (1993).
 (11) Miyano, K., Tanaka, T., Tomioka, Y., & Tokura, Y. Photoinduced insulatortometal transition in a perovskite manganite. Phys. Rev. Lett., 78, 4257–4260 (1997).
 (12) Kiryukhin, V. et al. An xrayinduced insulatormetal transition in a magnetoresistive manganite. Nature, 386, 813–815 (1997).
 (13) Zhang, J. et al. Cooperative photoinduced metastable phase control in strained manganite films. Nature Mater., 15, 956–960 (2016).
 (14) Rini, M. et al. Control of the electronic phase of a manganite by modeselective vibrational excitation. Nature, 449, 72–74 (2007).
 (15) Subedi, A., Cavalleri, A., & Georges, A. Theory of nonlinear phononics for coherent light control of solids. Phys. Rev. B, 89, 220301(R) (2014).
 (16) Tomioka, Y., Asamitsu, A., Kuwahara, H., Moritomo, Y., & Tokura, Y. Magneticfieldinduced metalinsulator phenomena in PrCaMnO with controlled chargeordering instability. Phys. Rev. B, 53, R1689–R1692 (1996).
 (17) Tokura, Y. Critical features of colossal magnetoresistive manganites. Rep. Prog. Phys., 69, 797 (2006).
 (18) Tobey, R. I., Prabhakaran, D., Boothroyd, A. T., & Cavalleri, A. Ultrafast electronic phase transition in LaSrMnO by coherent vibrational excitation: evidence for nonthermal melting of orbital order. Phys. Rev. Lett., 101, 197404 (2008).
 (19) Mankowsky, R. et al. Nonlinear lattice dynamics as a basis for enhanced superconductivity in YBaCuO. Nature, 516, 71–73 (2014).
 (20) Subedi, A. Proposal for ultrafast switching of ferroelectrics using midinfrared pulses. Phys. Rev. B, 92, 214303 (2015).
 (21) Fechner, M. & Spaldin, N. A. Effects of intense optical phonon pumping on the structure and electronic properties of yttrium barium copper oxide. Phys. Rev. B, 94, 134307 (2016).
 (22) Juraschek, D., Fechner, M., & Spaldin, N. A. Ultrafast structure switching through nonlinear phononics. Phys. Rev. Lett., 118, 054101 (2017).
 (23) Pavarini, E., Yamasaki, A., Nuss, J., & Andersen, O. K. How chemistry control electron localization in 3d perovskites: a Wannier function study. New J. Phys., 7, 188 (2005).
 (24) Först, M. et al. Nonlinear phononics as an ultrafast route to lattice control. Nature Physics, 7, 854–856 (2011).
 (25) Zhao, X. & Vanderbilt, D. Phonons and lattice dielectric properties of zirconia. Phys. Rev. B, 65, 075105 (2002).
 (26) Gonze, X. & Lee, C. Dynamical matrices, born effective charges, dielectric permittivity tensors, and interatomic force constants from densityfunctional perturbation theory. Phys. Rev. B, 55, 10355–10368 (1997).
 (27) Nova, T. F. et al. An effective magnetic field from optically driven phonons. Nature Physics, 13, 132 (2017).
 (28) Uecker, R. et al. Spiral formation during Czochralski growth of rareearth scandates. Journal of Crystal Growth, 295, 84–91 (2006).
 (29) Huang, X., Tang, Y., & Dong, S. Strainengineered Atype antiferromagnetic order in YTiO: A firstprinciples calculation. Journal of Applied Physics, 113, 17E108 (2013).
 (30) Weng, Y., Huang, X., Tang, Y., & Dong, S. Magnetic orders of LaTiO under epitaxial strain: A firstprinciples study. Journal of Applied Physics, 115, 17E108 (2014).
 (31) Yang, L.J., Weng, Y.K., Zhang, H.M., & Dong, S. Strain driven sequential magnetic transitions in strained GdTiO on compressive substrates: a firstprinciples study. J. Phys.: Condens. Matter, 26, 476001 (2014).
 (32) Huang, X., Xu, Q., & Dong, S. Orientationdependent magnetism and orbital structure of strained YTiO films on LaAlO substrates. Journal of Applied Physics, 117, 17C703 (2015).
 (33) Zhang, J. Y., Jackson, C. A., Raghavan, S., Hwang, J., & Stemmer, S. Magnetism and local structure in lowdimensional Mott insulating GdTiO. Phys. Rev. B, 88, 121104(R) (2013).
 (34) Kampfrath, T. et al. Coherent terahertz control of antiferromagnetic spin waves. Nature Photonics, 5 (2010).
 (35) Okamoto, S., Millis, A. J., & Spaldin, N. A. Lattice Relaxation in Oxide Heterostructures: LaTiO/SrTiO Superlattices. Phys. Rev. Lett., 97, 056802 (2006).
 (36) MacLean, D. A., Ng, H.N., & Greedan, J. E. Crystal structures and crystal chemistry of the RETiO perovskites: RE = La, Nd, Sm, Gd, Y. J. Solid State Chem., 30, 35–44 (1979).
 (37) Gonze, X. & Lee, C. Dynamical matrices, Born effective charges, dielectric permittivity tensors, and interatomic force constants from densityfunctional perturbation theory. Phys. Rev. B, 55, 10355–10368 (1997).
 (38) Mankowsky, R., von Hoegen, A., Först, M., & Cavalleri, A. Ultrafast Reversal of the Ferroelectric Polarization. Phys. Rev. Lett., 118, 197601 (2017).