Letter | Published:

Femtosecond activation of magnetoelectricity

Nature Physicsvolume 14pages370374 (2018) | Download Citation

Abstract

In magnetoelectric and multiferroic materials, the magnetic degree of freedom can be controlled by electric field, and vice versa. A significant amount of research has been devoted to exploiting this effect for magnetoelectric data storage and manipulation devices driven by d.c. electric fields1,2,3,4. Aiming at ever-faster schemes of magnetoelectric manipulation, a promising alternative approach offers similar control on a femtosecond timescale, relying on laser pulses4,5,6 to control both the charge7,8 and the magnetic9,10 order of solids. Here we photo-induce magnetoelectricity and multiferroicity in CuB2O4 on a sub-picosecond timescale. This process is triggered by the resonant optical generation of the highest-energy magnetic excitations—magnons with wavevectors near the edges of the Brillouin zone. The most striking consequence of the photo-excitation is that the absorption of light becomes non-reciprocal, which means that the material exhibits a different transparency for two opposite directions of propagation of light. The photo-induced magnetoelectricity does not show any decay on the picosecond timescale. Our findings uncover a path for ultrafast manipulations of the intrinsic coupling between charges and spins in multiferroics4, which may reveal unexplored magnetic configurations and unravel new functionalities in terms of femtosecond optical control of magnetism.

Main

The tetragonal dielectric magnetic material CuB2O4 (space group I\(\bar{4}\)2d, point group \(\bar{4}2m\))11 has a rich phase diagram (see Fig. 1a). If the temperature is higher than 21 K, CuB2O4 is paramagnetic. A weak ferromagnetic phase (II) and a spiral antiferromagnetic phase (I) appear in the temperature ranges 9–21 K and below 9 K, respectively12, in the absence of an external magnetic field. The magnetic ground state is defined by two interactions, which can be expressed in a general way by means of the following Hamiltonian:13

$$H=J\sum _{i,j}{\hat{{\bf{S}}}}_{i}\cdot {\hat{{\bf{S}}}}_{j}+\sum _{i,j}{{\bf{D}}}_{ij}\cdot {\hat{{\bf{S}}}}_{i}\times {\hat{{\bf{S}}}}_{j}$$
(1)
Fig. 1: Phase diagram and experimental configurations.
Fig. 1

a, Phase diagram of CuB2O4. This figure shows the qualitative evolution of the critical temperature (T*) of the transition from incommensurate spiral antiferromagnetic (AF) phase (I) to commensurate weak ferromagnet (II) as a function of an external magnetic field applied along the a(b)-axis. The quantitative phase diagram can be found elsewhere22; here we report only the estimate of the critical field for the temperature relevant for our experiment (5 K). The Néel temperature (TN) corresponding to the transition to the paramagnetic state is also shown. b, Schematic representation of the experimental apparatus. The central photon energies of the pump and probe are 1.55 eV and 3.1 eV, respectively. Although the polarization of the probe was never changed (electric field || a(b)-axis), different pump polarizations were used, as explained in the main text. The delay time Δt between pump and probe pulses was continuously tuned to reconstruct the dynamical response to the photo-excitation. An external magnetic field was applied along one tetragonal axis; applying a magnetic field along the c-axis results in a different phase diagram22.

where J is the Heisenberg exchange interaction, \({\hat{{\bf{S}}}}_{i,j}\) are spin operators at sites i,j and D ij is the Dzyaloshinskii–Moriya (DM) vector. The competition between the Heisenberg exchange and DM interaction determines the phase diagram of CuB2O4. This material is magnetoelectric, and the origin of the magnetoelectric coupling is the hybridization between the d orbitals of copper and the p orbitals of oxygen14. The magnetoelectricity is limited to phase II, owing to the lack of time-reversal symmetry breaking in phase I (ref.14).

Our choice of sample is motivated by two remarkable features of this material. First, extensive experimental evidence and theoretical analysis have demonstrated that the magnetoelectricity in CuB2O4 can be directly probed through its optical properties. The magnetoelectric phase exhibits an effect called ‘non-reciprocal directional dichroism’ (NDD): a different absorption coefficient for light propagating along two opposite directions through the material15,16. Second, the photoluminescence spectrum of CuB2O4 reveals that a light beam can generate high-energy magnons with wavevectors lying near the edges of the Brillouin zone, by means of radiative decay of an optically induced 3d-electronic transition of the copper atoms17. As a consequence, given the correspondence between the symmetries and conservation laws of photoluminescence and absorption18, the optical stimulus can simultaneously induce a 3d-electronic transition and high-energy magnons by absorption. This process has been widely studied and is known in the literature as ‘exciton–magnon’19,20,21. Because a magnon is in essence a perturbation of the magnetic system originating from a spin-flip event, the optical pumping of such elementary excitations causes a modification of the total spin of the medium, which affects both spin-dependent terms in the Hamiltonian in equation (1). In particular, magnons near the edges of the Brillouin zone have the highest frequency in the dispersion of CuB2O4 (ref. 13). A resonant optical generation of these spin excitations thus has the potential to modify the magnetic configuration and induce magnetoelectricity in CuB2O4 on the shortest timescale.

Our experiment relies on the pump–probe scheme, which allows one to detect only the effects induced by an intense pump beam (see Fig. 1b). In particular, we excite a zero-phonon d−d transition of copper atoms via the resonant pumping of phonon sidebands (see Fig. 2). By monitoring the modification of the optical transmissivity, we are able to ascertain whether, in the transient state, a photo-induced NDD (PI-NDD) is present. Therefore, our strategy consists in cooling the sample down to phase I, photoexciting it and verifying whether the magnetic phase transition to phase II is triggered. Because the pump–probe approach is exclusively sensitive to pump-induced effects, it can reveal whether the magnetoelectricity is photoinduced, whereas it is not sensitive to the magnetoelectricity if the material is already in the magnetoelectric phase before illumination by the pump beam. Earlier experiments proved that the NDD in CuB2O4 can be measured by reversing the externally applied magnetic field, and thus the magnetization of the medium, instead of the wavevector of light15. The reason lies in a change of sign of the magnetic dipole term in the light–matter interaction energy, which can be caused by reversing either the magnetization of CuB2O4 or the direction of propagation of light16. Hence we plan to measure the transient transmissivity by applying an external magnetic field along opposite directions. The experimental procedure and the data analysis used to disclose the PI-NDD are described in the Methods section.

Fig. 2: Spectrum of the pump beam and absorption of CuB2O4.
Fig. 2

The absorption spectrum of the sample was measured for different polarizations (see Methods for details). The relevant feature for our experiments is the zero-phonon line centred at 1.404 eV, which corresponds to the transition 3d x2 − y2 → 3d|+〉 and 3d|−〉 of the copper atoms, where |+〉 and |−〉 are two levels into which the excited state is split, and are given by the hybridization of the xy, yz and zx orbitals16. The phonon sidebands of the zero-phonon line are indicated in the figure. The spectrum of the pump beam overlaps with phonon sidebands31 corresponding to optical phonons29. Analysing both absorption spectra shown here, we find that if the pump beam is linearly polarized along the a(b)-axis, the penetration depth is comparable to the sample thickness (~100 μm). Consequently, photo-excitation induces considerable energy dissipation, so that the light–matter interaction cannot be described in terms of the non-dissipative approximation. On the other hand, if the pump beam is linearly polarized along the c-axis, the penetration depth is approximately 6 times the sample thickness; therefore the non-dissipative approximation can be invoked, and minor laser-heating can be expected. The zero-phonon line centred at 1.58 eV does not play an important role in our work.

The typical time-dependence of the optical transmissivity can be observed in the pump–probe traces in Fig. 3a: a plateau is established at a 600 fs delay and does not decay in a time-window of 40 ps. Additional experiments reveal that the level of the plateau is constant up to 500 ps (see Supplementary Fig. 1). After cooling the sample to phase I, we performed measurements as a function of the excitation fluence by using a pump beam linearly polarized along the a(b)-axis. The time-traces in Fig. 3a show the effect of the orientation of the magnetic field on the dynamics of the optical transmissivity for a few selected values of the pump fluence. A field-dependent and fluence-dependent contribution is visible in the data. We average the normalized transient transmissivities in the delay range from 600 fs to 40 ps. To quantify the effect of the magnetic field, we consider the difference of the average values obtained for the same excitation fluence and opposite orientations of the field. This difference corresponds to the definition of NDD16 in the photo-excited state, PI-NDD. Possible photo-induced modifications of the magnitude of the magnetization would not invalidate this procedure: such a phenomenon would affect both the time-traces used to evaluate the PI-NDD dynamics in an equivalent way, being determined only by the pump parameters (fluence and polarization). The results, shown by the orange dots in Fig. 3b, display a non-vanishing value of the PI-NDD in the fluence range 4.5–9 mJ cm−2. The values obtained using lower and higher (10.5 mJ cm−2) pump fluence are below the sensitivity level shown in Fig. 3b (see discussion of the sensitivity in the Methods section).

Fig. 3: Normalized transient transmissivity as a function of the fluence.
Fig. 3

a, Selected pump–probe traces. Each pair of datasets shows the effect of the orientation of the external magnetic field (Hext = 0.5 T) and thus of the magnetization. Opposite orientations of the magnetic field are indicated as H+ and H. The field used is intense enough to saturate the magnetization in phase II (ref. 15). The transient transmissivity (ΔT) is normalized to the transmissivity of the sample prior to the photo-excitation (T). b, PI-NDD as a function of the fluence, showing the effect of the orientation of the magnetic field on the transient transmissivity, for different pump polarization states and initial temperature. Details of the data analysis and a discussion of the sensitivity are given in the Methods.

The non-trivial experimental trend is consistent with the idea of a photo-induced phase-transition to phase II, according to the following picture. If the fluence is too low, the magnetic system is not perturbed enough to undergo the phase transition and thus no PI-NDD can be detected. Once the pump beam is intense enough, the medium is driven into the magnetoelectric phase and the PI-NDD is observed. If the sample is heated even further, the transition to the paramagnetic phase occurs and once again no PI-NDD is measured. The time-traces of the PI-NDD (see Supplementary Fig. 2) confirm that the effect is established in 600 fs. Below, we will confirm the suggested picture with three additional and independent experiments represented by the other datasets in Fig. 3b and by Fig. 4.

Fig. 4: Normalized transient transmissivity as a function of the magnetic field.
Fig. 4

a, Selected pump–probe traces. These datasets show the effect of the orientation and magnitude of the magnetic field on the transient transmissivity. As the field becomes more intense, the difference between the data obtained with opposite orientations of the field vanishes. The pairs of datasets corresponding to different intensities of the field are vertically translated for presentation purposes. b, The experimental conditions used to obtain these data allowed observation of the PI-NDD, as reported in Fig. 3b. The sensitivity level here is identical to the value shown in Fig. 3b; the dashed line (guide to the eye) and the error bars are removed from the points below the sensitivity level (see discussion in the Methods).

Let us recall that the pump–probe experimental scheme is sensitive exclusively to effects triggered by the pump beam. Although we can detect the light-induced magnetoelectricity (via the PI-NDD) in the measurements just described, this should not be the case if a similar experiment was performed with the sample already in phase II before the photo-excitation. This argument is supported by the magenta data points in Fig. 3b, which show the results of experiments in which the temperature of the sample was set to 15 K (phase II). No PI-NDD is detected when CuB2O4 is in the magnetoelectric phase before the photo-excitation, supporting our interpretation of the results.

The optical properties of CuB2O4 along the a(b)-axis are different from the properties along the c-axis, consistent with the tetragonal structure of the sample. Figure 2 shows that if the electric field of the pump beam is parallel to the a(b)-axis, optical absorption is stronger than for light linearly polarized along the c-axis. Thus we investigate the fluence-dependence of the transient transmissivity by using a pump beam linearly polarized along the c-axis, which should not heat the material intensively. More specifically, a light beam linearly polarized along the c-axis does not induce the exciton-magnon process (no sharp peak at 1.4 eV in Fig. 2), whereas this transition is photo-activated if the linear polarization of light is along the a(b)-axis. The results of this experiment (green dots in Fig. 3b) are consistent with our expectation and further corroborate our interpretation: no PI-NDD is observed in this data set, as the light–matter interaction takes place in a non-dissipative regime and the exciton-magnon transition is not induced.

Seeking further substantiation, we conceived an additional experiment. The phase diagram in Fig. 1a shows that the magnetic phase transition can be triggered by an external field with critical value of the order of Hc ≈ 2 T, if the sample temperature is 5 K (ref. 22). Consequently, measuring the transient transmissivity as a function of the external magnetic field should disclose a non-vanishing PI-NDD as long as Hext < Hc. Increasing the field above the critical value is expected to suppress the PI-NDD signal, because the transition to phase II is induced by the field before the interaction with the pump pulses. Using a pump fluence and polarization that allowed a successful observation of the PI-NDD in Fig. 3b, we studied the field dependence of the effect. The results confirm our physical interpretation (see Fig. 4). Measurements performed by applying an external field of intensity lower than 2 T show PI-NDD and are in quantitative agreement with the data in Fig. 3b (within the error bars). If the external field is more intense, the PI-NDD is suppressed.

Our extensive experimental investigation demonstrates overall a non-vanishing PI-NDD, implying a contribution to the optical transient transmissivity that is dependent on the orientation of the magnetic field and, consequently, linearly dependent on Hext. This observation demonstrates that magnetoelectricity is photo-induced. In fact, the optical transmissivity is defined by the symmetric components of the dielectric tensor: symmetry considerations show that, in a non-magnetoelectric material, these terms depend quadratically (at the lowest order) on an externally applied magnetic field23. On the other hand, it is experimentally assessed that the optical transmissivity of CuB2O4 in the magnetoelectric phase exhibits a contribution linearly dependent on an external magnetic field15,16. Our data in Fig. 4b reveal a contribution dependent on the sign of the field (that is, linear), although a linear increase of the PI-NDD as a function of the field is not visible, because this effect is in competition with the proximity of the phase-transition induced by Hext, which quenches the signal.

Having provided robust experimental evidence of the photo-induced magnetic phase transition, we must address a fundamental question: how does light couple to spins in CuB2O4 on a 600 fs timescale? It is known that laser pulses can increase the effective spin temperature in dielectrics24,25 and even trigger magnetic phase transitions26. These phenomena have been observed on the 10–100 ps timescale, consistent with the characteristic timescale of the magnetic excitations photo-induced in those experiments, which are typically magnons with wavevectors near the centre of the Brillouin zone26. In our case, the magnetic phase transition in CuB2O4 occurs in 600 fs, pointing to the involvement of magnons with wavevectors near the edges of the Brillouin zone. Because of the femtosecond period and nanometre wavelength of these elementary excitations, they are known as femto-nanomagnons27. The characteristic timescales of femto-nanomagnons are typically shorter than those of zone-centre magnetic excitations10,28, and this holds for CuB2O4 as well13. Although non-resonant impulsive stimulated Raman scattering of the femto-nanomagnons has been demonstrated, this process is not relevant in our experiment: no coherent oscillations at the magnonic frequency have been observed27.

As previously mentioned, the photo-excitation in our experiment induces optical phonons (sidebands), a dd transition and magnons near the edges of the Brillouin zone. Although the phonon non-radiative relaxation heats the lattice18 on an estimated timescale below our time resolution (see Fig. 5), this process alone cannot drive the phase transition, as no structural modification takes place when CuB2O4 evolves from phase I to II. We observe that the ground and excited states shown in Fig. 5 have different spin16, making an electric dipole contribution to this transition spin-forbidden. The parity-forbiddance of the dd transition is weakly removed by the hybridization of the excited state with different d orbitals16,17. However, the simultaneous generation of excited 3d electrons and femto-nanomagnons can result in a pair-excitation transition within an electric dipole framework, restoring the conservation of spin: this is the canonical interpretation of the exciton-magnon process19,20,21. The resonant generation of high-energy magnons strongly perturbs the magnetic system, not solely because of the difference in spin between the ground and the excited states. In fact, the femto-nanomagnons in CuB2O4 exhibit a strong magnon–magnon interaction leading to an estimated characteristic lifetime of about 670 fs. This number is derived from the bandwidth of the two-magnon mode detected in the Raman spectrum of this compound29. A pronounced magnon–magnon interaction entails considerable energy dissipations in the spin system and short lifetime of the magnons, inducing ultrafast heating of spins. In the present case, the photogeneration of electrons and lattice provides two additional scattering channels for the high-energy magnons, shortening the lifetime of the magnetic quasiparticles below the 670 fs estimation. We ascribe the cause of the magnetic phase-transition to the excitation and subsequent dissipations of high-energy magnons. Although femto-nanomagnons are induced also via the radiative relaxation of the 3d electrons17, this process is not relevant on the sub-picosecond timescale. In fact, our measurements of time-resolved photoluminescence (see Supplementary Fig. 3) demonstrate a characteristic relaxation time in the microsecond regime, consistent with the constant value of the plateau observed in the transient transmissivity up to a 500 ps delay (see Supplementary Fig. 1).

Fig. 5: Schematic representation of the relaxation dynamics.
Fig. 5

The potential energy curves of the ground state (GS) and of the excited state (ES) are represented. The sphere indicates the dynamics of the system, and its colour is a pictorial illustration of the excitation state of the medium. The curved arrows with continuous lines represent non-radiative relaxation processes, while the wavy arrow indicates the radiative decay channel resulting in the emission of photoluminescence (PL). The phonon relaxation is estimated to occur in less than 300 fs (our time-resolution), considering the width of the sidebands in Fig. 2. Note that the pump pulses induce both lattice and spin excitation (see main text); for this reason, the x-axis of the figure represents both spin (Qs) and phonon (Qp) degrees of freedom. The dashed red arrows indicate the flow of energy and heat, which induces an increase in the effective spin and lattice temperature, T. The zero-phonon (ZP) transition is illustrated by a yellow double arrow.

We note that also a non-radiative decay channel of the photo-excitation involving phonon–magnon scattering may result in the generation of magnons near the edges of the Brillouin zone. Recent experiments show that an energy transfer from the lattice to the spin excitations can occur if the phononic and magnonic dispersion relations are close30. This situation occurs in CuB2O4 near the edges of the Brillouin zone in the case of magnons13 and optical phonons, here photo-excited and generated during the non-radiative lattice relaxation18.

Our findings have implications not only in terms of ultrafast optical manipulation of magnetoelectric and multiferroic materials4, but also for the development of new concepts for photonic technologies, given the femtosecond photo-activation of a nanosecond-long directional transparency demonstrated here.

Methods

Sample preparation and optical characterization

A single crystal of CuB2O4 was grown by the flux method. The orientation of the single crystal was determined by X-ray diffraction. The sample was cut into thin plates with wide faces orthogonal to the (b)a-axis. Each wide face was polished to obtain a flat surface. The thickness of the sample was approximately 100 μm. A halogen lamp was used for the optical absorption measurements. A monochromatic light beam was obtained by using a grating-type monochromator. The intensity of the transmitted beam was detected by a photodiode. The optical absorption spectrum was calculated from the intensity spectrum of the transmitted light. Note that CuB2O4 has a transparency window in correspondence of the probe photon energy31. The onset of the charge-transfer transition, which is the bandgap, arises at 3.7 eV (ref. 31).


Pump–probe set-up

The light source used for our pump–probe experiments is a regeneratively amplified mode-locked Ti:sapphire laser, delivering 100 fs, 700 μJ pulses with central photon energy of 1.55 eV and 5 kHz repetition rate. The output of the laser system is split into two beams: the pump beam (1.55 eV) and the probe beam, which has central photon energy of 3.1 eV. The probe beam is obtained by second-harmonic generation of the fundamental wavelength of the laser system, by means of a β-barium borate crystal. The pulse durations for pump and probe pulses were 100 fs and 300 fs, respectively. The two beams impinged on the sample with a relative angle smaller than 10°. The pump and probe were focused on the sample down to spot diameters of approximately 480 μm and 50 μm, respectively. The delay between pump and probe pulses was continuously tuned by a mechanical delay line, able to access the 0–500 ps range. The intensity of the pump beam was modulated by a mechanical chopper operating at 2.5 kHz, synchronized with the train of pump pulses. The angle between the pump and the probe beam is wide enough to avoid the pump beam impinging on the detector, ruling out any possible contribution to the signal originating from a second harmonic generation process of the pump. The scattered pump radiation did not affect our detection, as we had placed a colour filter in front of the photodiode to block any scattered 1.55 eV radiation while letting the 3.1 eV probe beam propagate to the detector. The sample was placed in a magneto-optical cryostat, allowing us to change the temperature of the medium in the range 4 K to 300 K. A split-coil superconducting magnet is able to generate a magnetic field up to 5 T along the b(a) axis of the sample, as shown in Fig. 1b.


Data analysis

The normalized transient transmissivity represented by each pump–probe trace was averaged in the range 600 fs to 40 ps to evaluate the plateau. We do not consider the data at shorter delays, because coherent nonlinear optical effects (‘coherent artifacts’32) due to the overlap of the pump and probe beams obscure the real value of the transient transmissivity. The PI-NDD (dotted curves in Figs. 3b and 4) is then expressed by the absolute value of the difference between measurements performed by applying the external magnetic field in opposite orientations along the b(a)-axis (see Fig. 1b). The experimental uncertainty of each pump-probe measurement is defined by the standard deviation of the data points used to evaluate the average of ΔT/T. The errorbars of the PI-NDD are then obtained by the sum of squared errors of the two average values of ΔT/T, as the two measurements are independent. However, the error bars calculated in this way do not take into account all the experimental sources of errors, such as mechanical drift of the sample during the time interval between the two measurements involved in calculating the PI-NDD (typically 2–3 hours). We identify the sensitivity of our experimental apparatus in Fig. 3b with the data point obtained for 1.5 mJ cm−2 fluence and pump polarization parallel to the a(b)-axis. In fact, we calculated the laser-heating of the sample, using the experimentally determined12 specific heat of CuB2O4 at T = 5 K. The increase of temperature induced by a pump beam linearly polarized along the a(b)-axis and with a fluence of 1.5 mJ cm−2 is estimated to be 1.5 K. In this configuration, no PI-NDD is thus expected, motivating our choice for the sensitivity value. The data points obtained below this level are not ascribed to the PI-NDD. This choice is motivated and its validity is confirmed by the results obtained and shown in Figs. 3b and 4b. We stress that, in these two figures, measurements performed under the same conditions provide values of the PI-NDD that are in quantitative agreement (within error bars).


Data availability

The data that support the plots within this paper and other findings of this study are available from the corresponding author upon request.

Additional information

Publisher’s note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

References

  1. 1.

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

  2. 2.

    Kosub, T. et al. Purely antiferromagnetic magnetoelectric random access memory. Nat. Commun. 8, 13985–13992 (2017).

  3. 3.

    He, X. et al. Robust isothermal electric control of exchange bias at room temperature. Nat. Mater. 9, 579–585 (2010).

  4. 4.

    Fiebig, M., Lottermoser, T., Meier, D. & Trassin, M. The evolution of multiferroics. Nat. Rev. Mater. 16046–16060 (2016).

  5. 5.

    Sheu, Y. M. et al. Using ultrashort optical pulses to couple ferroelectric and ferromagnetic order in an oxide heterostructure. Nat. Commun. 5, 5832 (2014).

  6. 6.

    Johnson, S. L. et al. Femtosecond dynamics of the collinear-to-spiral antiferromagnetic phase transition in CuO. Phys. Rev. Lett. 108, 037203–037208 (2012).

  7. 7.

    Rini, M. et al. Control of the electronic phase of a manganite by mode-selective vibrational excitation. Nature 449, 72–74 (2007).

  8. 8.

    Fausti, D. et al. Light-induced superconductivity in a stripe-ordered cuprate. Science 331, 189–191 (2011).

  9. 9.

    Stupakiewicz, A., Szerenos, K., Afanasiev, D., Kirilyuk, A. & Kimel, A. V. Ultrafast nonthermal photo-magnetic recording in a transparent medium. Nature 542, 71–74 (2017).

  10. 10.

    Bossini, D., Belotelov, V. I., Zvezdin, A. K., Kalish, A. N. & Kimel, A. V. Magnetoplasmonics and femtosecond optomagnetism at the nanoscale. ACS Photon 3, 1385–1400 (2016).

  11. 11.

    Martinez-Ripoll, M., Martnez-Carrera, S. & Garca-Blanco, S. The crystal structure of copper metaborate, CuB2O4. Acta Crystallogr. B 27, 677–681 (1971).

  12. 12.

    Petrakovskii, G. et al. Weak ferromagnetism in CuB2O4 copper metaborate. J. Magn. Magn. Mater. 205, 105–109 (1999).

  13. 13.

    Martynov, S., Petrakovskii, G., Boehm, M., Roessli, B. & Kulda, J. Spin-wave spectrum of copper metaborate in the incommensurate phase. J. Magn. Magn. Mater. 299, 75–81 (2006).

  14. 14.

    Khanh, N. D. et al. Magnetic control of electric polarization in the noncentrosymmetric compound (Cu,Ni)B2O4. Phys. Rev. B 87, 184416–184421 (2013).

  15. 15.

    Saito, M., Arima, T., Ishikawa, K. & Taniguchi, K. Magnetic control of crystal chirality and the existence of a large magneto-optical dichroism effect in CuB2O4. Phys. Rev. Lett. 101, 117402 (2008).

  16. 16.

    Toyoda, S. et al. One-way transparency of light in multiferroic CuB2O4. Phys. Rev. Lett. 115, 267207 (2015).

  17. 17.

    Toyoda, S., Abe, N. & Arima, T. Gigantic directional asymmetry of luminescence in multiferroic CuB2O4. Phys. Rev. B 93, 201109 (2016).

  18. 18.

    Peyghambarian, N., Koch, S. W. & Mysyrowicz, A. Introduction to Semiconductor Optics. (Prentice Hall, Englewood Cliffs, NJ/London, 1993).

  19. 19.

    TanabeY.. & Aoyagi, A. K. Excitons in Magnetic Insulators. (North-Holland, 1982).

  20. 20.

    Macfarlane, R. M. & Allen, J. W. Exciton bands in antiferromagnetic Cr2O3. Phys. Rev. B 4, 3054–3067 (1971).

  21. 21.

    Moriya, T., Tanabe, Y. & Sugano, S. Magnon-induced electric dipole transition moment. Phys. Rev. Lett. 15, 1023–1025 (1965).

  22. 22.

    Fiebig, M., Sänger, I. & Pisarev, R. V. Magnetic phase diagram of CuB2O4. J. Appl. Phys. 93, 6960–6963 (2003).

  23. 23.

    LandauL. D.. & Lifshitz, E. Electrodynamics of Continuous Media. 2nd edn, (Elsevier, 1984).

  24. 24.

    Kimel, A. V., Pisarev, R. V., Hohlfeld, J. & Rasing, T. ultrafast quenching of the antiferromagnetic order in FeBO3: direct optical probing of the phonon–magnon coupling. Phys. Rev. Lett. 89, 287401–287405 (2002).

  25. 25.

    Bossini, D., Kalashnikova, A. M., Pisarev, R. V., Rasing, T. & Kimel, A. V. Controlling coherent and incoherent spin dynamics by steering the photo-induced energy flow. Phys. Rev. B 89, 060405 (2014).

  26. 26.

    Afanasiev, D. et al. Control of the ultrafast photoinduced magnetization across the Morin transition in DyFeO3. Phys. Rev. Lett. 116, 097401 (2016).

  27. 27.

    Bossini, D. et al. Macrospin dynamics in antiferromagnets triggered by sub-20 femtosecond injection of nanomagnons. Nat. Commun. 7, 10645–10653 (2016).

  28. 28.

    Bossini, D. & Rasing, T. Femtosecond optomagnetism in dielectric antiferromagnets. Phys. Scr. 92, 024002 (2017).

  29. 29.

    Ivanov, V. G. et al. Phonon and magnon Raman scattering in CuB2O4. Phys. Rev. B 88, 094301 (2013).

  30. 30.

    Hashimoto, Y. et al. All-optical observation and reconstruction of spin wave dispersion. Nat. Commun. 8, 15859–15865 (2017).

  31. 31.

    Pisarev, R. V., Kalashnikova, A. M., Schöps, O. & Bezmaternykh, L. N. Electronic transitions and genuine crystal-field parameters in copper metaborate CuB2O4. Phys. Rev. B 84, 075160 (2011).

  32. 32.

    Brito Cruz, C. H., Gordon, J. P., Becker, P. C., Fork, R. L. & Shank, C. V. Dynamics of spectral hole burning. IEEE J. Quantum Electron. 24, 261–269 (1988).

Download references

Acknowledgements

We thank J. Omachi for the time-resolved photoluminescence measurements and N. Nemoto, Y. Arashida and H. Sakurai for technical support. This work was supported by JSPS KAKENHI grant no. 26247049 and the Photon Frontier Network Program funded by the Ministry of Education, Culture, Sports, Science, and Technology (MEXT), Japan. D.B was supported by the Japanese Society for Promotion of Science (JSPS) ‘Postdoctoral Fellowship for Overseas Researcher’ no. P16326. S.T was also supported by JSPS through the Program for Leading Graduate Schools (MERIT) and a Grant-in-Aid for JSPS Fellows (14J06840).

Author information

Author notes

    • D. Bossini

    Present address: Experimentelle Physik VI, TU-Dortmund, Dortmund, Germany

Affiliations

  1. Institute for Photon Science and Technology, Graduate School of Science, The University of Tokyo, Tokyo, Japan

    • D. Bossini
    • , K. Konishi
    • , J. Yumoto
    •  & M. Kuwata-Gonokami
  2. Department of Advanced Materials Science, The University of Tokyo, Kashiwa, Japan

    • S. Toyoda
    •  & T. Arima
  3. RIKEN Center for Emergent Matter Science (CEMS), Wako, Japan

    • S. Toyoda
  4. Department of Physics, Graduate School of Science, The University of Tokyo, Tokyo, Japan

    • J. Yumoto
    •  & M. Kuwata-Gonokami
  5. Photon Science Center, Graduate School of Engineering, The University of Tokyo , Tokyo, Japan

    • M. Kuwata-Gonokami

Authors

  1. Search for D. Bossini in:

  2. Search for K. Konishi in:

  3. Search for S. Toyoda in:

  4. Search for T. Arima in:

  5. Search for J. Yumoto in:

  6. Search for M. Kuwata-Gonokami in:

Contributions

D.B. conceived the project with contributions from K.K., T.A. and M.K-G. The sample was grown and characterized by S.T. D.B. performed the time-resolved experiments and analysed the data. All the authors took part in regular discussions and contributed to the writing of the manuscript.

Competing interests

The authors declare no competing financial interests.

Corresponding author

Correspondence to D. Bossini.

Supplementary information

  1. Supplementary Notes

    Supplementary Notes 1–3, Supplementary References.

About this article

Publication history

Received

Accepted

Published

DOI

https://doi.org/10.1038/s41567-017-0036-1