## Abstract

Consider observing two different waves with the same frequency and wavelength. When these waves are coupled, the amplitude alternates between the two waves periodically, a phenomenon called coherent beating oscillation. Such phenomena can be seen in familiar coupled pendulums and, on a cosmic scale, neutrino oscillations: the oscillation between different types of neutrinos. In solids, on the other hand, there are various wave excitations responsible for their thermal and electromagnetic properties. Here we report the observation of coherent beating between different excitation species in a solid: phonons and magnons. By using time-resolved magneto-optical microscopy, magnons generated in Lu_{2}Bi_{1}Fe_{3.4}Ga_{1.6}O_{12} gradually disappear by transforming to phonons, and after a while, they return to magnons. The period of the oscillation as a function of the field is consistent with the prediction of the magnon-phonon beating. The experimental results pave a way to coherent control of magnon-phonon systems in solids.

## Introduction

Phonons refer to vibration waves of a crystal lattice in solids (Fig. 1a). They are responsible for the elastic and thermal properties of solids. On the other hand, magnons, or spin waves, refer to the wavy motion of magnetization in magnets, responsible for the magnetic and thermal properties (Fig. 1a)^{1,2,3,4,5}. Phonons and magnons can interact in solids via the magneto-elastic and magnetostatic couplings^{6,7,8} (Fig. 1b).

The dynamics of phonons and magnons in each system is written in their dispersion curves, curves that show the relation between the wavenumber and frequency. Figure 1c shows dispersion curves of transverse acoustic (TA) phonons and magnons in a film of typical magnetic insulator, lutetium iron garnet (LuIG)^{9,10}. In the dispersion curves, the phonon dispersion and the magnon dispersion curves have an intersection, depicted as A in Fig. 1c, due to the magnetostatic gap in the magnon dispersion at *k* = 0. Around the intersection, a magnon-phonon hybridized state can be formed^{11,12,13,14}. This state, called a magnon polaron, was experimentally found to exhibit extremely long lifetime, much longer than pure magnons, attributed to the hybridization with phonons with long lifetime^{15,16}. In a lutetium iron garnet, the extended lifetime is confirmed by spin-heat conversion measurement even at room temperature^{17}. As a result, when magnons are excited and sufficient time has passed, the pure magnons are attenuated, leaving magnon polarons. In magnon polarons, theoretically, the hybridization can cause level splitting, giving rise to an anti-crossing gap at the intersection in the dispersion curves, as shown in Fig. 1d. When the two states across the gap are excited simultaneously in a coherent way, coherent superposition of these two states, corresponding to beating oscillation between phonons and magnons, may be created (Fig. 1b).

We report the observation of coherent beating between phonons and magnons in lutetium iron garnet. By using time-resolved magneto-optical (TRMO) microscopy, we measured spatio-temporal magnetization dynamics, which couples with phonons in a thin film of lutetium iron garnet, LuIG. We found the coherent beating lasts up to tens of nanoseconds, which experimentally confirms strong coupling between magnons and phonons in the bare film of LuIG.

## Results

### Sample and measurement setup

To explore the beating oscillation in solids, we have developed TRMO microscopy. Figure 1e shows a schematic illustration of the experimental setup used in the present study. We used a thin film of Lu_{2}Bi_{1}Fe_{3.4}Ga_{1.6}O_{12} (LuIG) with the thickness of 1.8 *μ*m as a sample, exhibiting large magneto-optical effects^{18,19} and small magnetization damping (See Supplementary Note 1). To excite magnetization dynamics, we focused a pulsed laser light (pump pulse) with the wavelength of 800 nm onto the sample, where the wavelength corresponds to almost half the energy of the bandgap of LuIG (~2.3 eV)^{18,19}. The duration and the energy of the pulse is 100 fs and 1.0 *μ*J per pulse, respectively. The pump pulse excites spin waves, or magnons, via the photo-induced demagnetization and the photo-induced expansion effects^{20,21,22,23,24}. We shaped the focus into a vertical line to selectively excite magnons with the wavevector **k** perpendicular to the vertical line (*y* axis) by using the Huygens-Fresnel interference^{25}. Next, we shined another weak light pulse (probe pulse) with the wavelength of 630 nm (100 fs, 50 nJ per pulse) on the sample from the normal direction. We measured the spatial distribution of the magneto-optical Faraday rotation of the probe pulse transmitted through the sample by using a CCD camera (See Method for details)^{26}. The Faraday rotation at each position on the sample *θ*_{F}(**r**, *t*) reflects the local magnetization precession amplitude projected along the propagation direction of the probe pulse. By sweeping the time delay between the pump and probe pulses, we obtained temporal evolution of the spatial images of the magnetization dynamics excited by the pump pulse. We extended the maximum delay time to 35 ns by using optical fibers, so that the frequency resolution of the obtained images reaches 28 MHz, which is enough to resolve the magnon-phonon gap frequency in the sample^{7,8}. All the measurements were performed at room temperature.

### Observation of coherent oscillation between phonons and magnons

Figure 1f shows a spatial image of the polarization-rotation angle obtained at 3.5 ns after the pump-pulse irradiation. Vertical wave patterns appear in the vicinity of the focus of the pump pulse, demonstrating the magnon excitation by the pump pulse. By observing the sign change of the rotation caused by reversing the external magnetic field (See Supplementary Note 2), we confirmed that the polarization rotation is due mainly to the magneto-optical Faraday effect rather than the distortion-induced polarization rotation. Here, we define \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)=\int {\theta }_{{{{{{{{\rm{F}}}}}}}}}({{{{{{{\bf{r}}}}}}}},t){e}^{i{{{{{{{\bf{k}}}}}}}}{{{{{{{\bf{r}}}}}}}}}d{{{{{{{\bf{k}}}}}}}}\) as the Fourier transform of the spatial image of the Faraday rotation angle with respect to the spatial coordinate. Figure 1g shows the \(| {\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t){| }^{2}\) at *t* = 3.5 ns. In the *k*_{x} > 0 region [**k** = (*k*_{x}, *k*_{y})], a region corresponding to waves propagating right in Fig. 1f, we see clear peaks of \(| {\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t){| }^{2}\) at *k*_{x} = 2.93 × 10^{4 }rad ⋅ cm^{−1} ≡ *k*_{TA} (*k*_{x} = 1.38 × 10^{4 }rad ⋅ cm^{−1} ≡ *k*_{LA}) corresponding to the intersection point between magnons and TA (LA; longitudinal acoustic) phonons calculated from the parameters of LuIG. This shows that the magnon polarons are created at the intersections of the dispersion curves of magnons and phonons after the pump-pulse irradiation.

In Fig. 2a, we show the temporal evolution of the real part of \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) at ∣**k**∣ = *k*_{TA} and **k**//**B**. Importantly, the envelope of the \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) signal clearly oscillates; the envelope amplitude decreases from *t* = 15 ns to *t* = 20 ns, while it increases from *t* = 20 ns to *t* = 25 ns up to almost the same amplitude as at *t* = 15 ns. This oscillation is in contrast to the ordinary relaxation dynamics of magnons, which monotonically decreases, but rather implies oscillation of magnon density.

In Fig. 2b, we show the frequency power spectrum of \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\), *F*_{k}(*ω*) = ∫*θ*_{F}(**r**, *t*)*e*^{i(kr−ωt)}*d***k***d**t*, at ∣**k**∣ = *k*_{TA}, where **k**//**B**. The frequency spectrum exhibits two peaks, suggesting the level splitting at the intersection of the magnon and TA phonon dispersion curves. The splitting width 70 MHz coincides with the inverse of the period for the observed oscillation envelope shown in Fig. 2a (14 ns), implying that the splitting is related to the observed oscillation.

When we measure pure magnons directly with the TRMO technique, we should see the periodically oscillating signal as a function of time with the frequency of magnons. Since we measure magneto-optical Faraday rotation, the signal disappears when magnons are transformed into phonons. Therefore, the observed oscillation of the signal envelope shown in Fig. 2a implies the periodic coherent beating oscillation between magnon and phonon in the time domain.

To confirm that the observed envelope oscillation is magnon-phonon beating oscillation, we examine field-angular dependence; if the observed oscillation is the beating, it should disappear for LA phonons since the magnon-phonon coupling coefficient takes minimum for LA phonons when **k**//**B**. The effective magnetic field **b** = (*b*_{y}, *b*_{z}) acting on local magnetization due to the magnon-phonon coupling can be written as^{27},

where *b*_{1} and *b*_{2} are the magneto-elastic coupling constants, and *θ*_{k} is the relative angle between the wavevector of magnons and the saturation magnetization. *ϵ*_{xx} and *ϵ*_{xz} are the elastic strain tensor components induced by phonons. *ϵ*_{xx} (*ϵ*_{xz}) becomes nonzero for LA (TA) phonons. When *θ*_{k} = 0(**k**//**B**), LA phonons induce minimal effective fields, while TA phonons induce maximum effective fields. On the other hand, both LA and TA phonons induce minimal effective fields when *θ*_{k} = 90^{∘}(**k**⊥**B**). Therefore, the coherent oscillation should disappear when *k*_{x} = *k*_{LA}(**k**//**B**), *k*_{x} = *k*_{LA}(**k**⊥**B**), and *k*_{x} = *k*_{TA}(**k**⊥**B**). We show the temporal evolution of the real part of the experimentally obtained \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) at *k*_{x} = *k*_{LA}(**k**//**B**) in Fig. 2d. When **k**//**B**, the envelope amplitude of the \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) does not oscillate but monotonically decreases. The frequency spectrum of the \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) exhibits a single peak at *k*_{x} = *k*_{LA}(**k**//**B**), as shown in Fig. 2e, consistent with the *θ*_{k} dependence of the effective field representing the magnon-phonon coupling [Fig. 2f]. Figure 2g and h show the temporal evolution of \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}\) at *k*_{x} = *k*_{LA}(**k**⊥**B**) and *k*_{x} = *k*_{TA}(**k**⊥**B**), respectively. The envelope of \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) does not oscillate in both cases, consistent with the prediction that the effective field is minimized under these conditions. We also performed measurement at *θ*_{k} = 45°, where the magneto-elastic coupling is maximized for LA phonon, however, we could not see clear oscillation due to large damping of magnons (See Supplementary Note 3).

To demonstrate how coherent beating oscillation is observed in real space, we show the temporal change in the wave pattern excited by the pump pulse in Fig. 2i. At *t* = 15 ns, we see clear wave pattern with the characteristic wavelength of *λ*_{TA} = 2*π*/*k*_{TA} = 2.1 *μ*m, while at *t* = 20 ns, the period of the strong wave pattern changes to *λ*_{LA} = 2*π*/*k*_{LA} = 4.6 *μ*m. This is because the magnon amplitude \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) at *k* = *k*_{TA} decreases owing to coherent beating oscillation, while the \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) at *k* = *k*_{LA} remains finite. After another 10 ns, the wave pattern of *k*_{TA} mode recovers its intensity, which are all consistent with the result shown in Fig. 2a and d.

### Excitation spectra of magnons and coherent oscillation frequency

We now discuss the results in terms of the relation between magnon excitation spectra and coherent oscillation frequency. By using the effective field **b**, we calculate the coherent oscillation frequency as follows (See Method),

where \({\sigma }_{k}={b}_{2}k\sqrt{\frac{2\gamma }{\rho {M}_{{{{{{{{\rm{s}}}}}}}}}{\omega }_{t}}}\) is the magnon-phonon gap frequency, *γ* = 2*π* × 2.8 × 10^{10}Hz ⋅ T^{−1} is the gyromagnetic ratio, *ρ* = 7.39 × 10^{3} kg ⋅ m^{−3} is the density of the sample, *M*_{s} = 1.48 × 10^{4 }A ⋅ m^{−1} is the saturation magnetization, and *k* = ∣**k**∣ is the wavenumber. *ω*_{m}(*k*; **B**) and *ω*_{p}(*k*) are the angular frequency of magnons and phonons, respectively. *ω*_{t} is the angular frequency at the intersection between magnon and phonon dispersion curves. In Fig. 3a, we show a magnified view of ∣*F*_{k}(*ω*)∣^{2} near the intersection. The spectrum intensity is in good agreement with the theoretical calculation exhibiting anticrossing gap around the intersection of the dispersion curves. Figure 3b shows the oscillation frequency as a function of the wavenumber obtained from the time-domain analysis of the \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\). The obtained oscillation frequency exhibits a V-shaped curve which takes a minimum at the intersection point. The bottom frequency of the V-shaped curve remains finite within the error bar. The result demonstrates again the formation of the anti-crossing gap caused by the magnon-phonon coupling, which has yet to be observed in magnetic garnet films^{28,29,30}. When the external magnetic field is increased to 13.0 mT, the spectrum peak shifts towards higher wavenumbers (Fig. 3c). The magnetic field dependence confirms that the observed gap is not due to the phonons, which do not respond to external magnetic fields. The experimental result is well reproduced by Eq. (2), as shown in Fig. 3b and d, showing that the observed envelope oscillation of \({\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t)\) is attributed to the coherent oscillation between phonons and magnons.

## Discussion

We numerically calculated the temporal evolution of the magnon amplitude \({\tilde{a}}_{k}(t)\) by calculating the Fourier transform of the spectral magnon amplitude *a*_{k}(*ω*)^{31}. We considered only the coupled dynamics between TA phonons and magnons, relevant to the observed oscillation. By considering the magnon-phonon interaction to the lowest order, Gilbert damping, and phonon relaxation, *a*_{k}(*ω*) can be written as follows (See Methods),

where *κ*_{m} and *κ*_{p} are the relaxation constants of magnons and phonons, respectively. *f*_{k} is the external driving force for phonons, and \({g}_{{{{{{{{\rm{p}}}}}}}}}^{{{{{{{{\rm{ex}}}}}}}}}\) is the coupling between phonons and *f*_{k} (See Method). *ω*_{m} and *ω*_{p} are the angular frequency of magnon and phonon at a wavenumber *k*, respectively. In Fig. 4a and b, we compared the experimentally obtained temporal evolution of \(| {\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t){| }^{2}\) as a function of the wavenumber with the calculated magnon amplitude \(| {\tilde{a}}_{k}(t){| }^{2}\). The \(| {\tilde{F}}_{{{{{{{{\bf{k}}}}}}}}}(t){| }^{2}\) and \(| {\tilde{a}}_{k}(t){| }^{2}\) exhibit similar wavenumber-dependent oscillation. We estimated the magnon-phonon gap frequency *σ*_{k} and the relaxation constants *κ*_{m} and *κ*_{p} by fitting the experimentally obtained magnon amplitude, as shown in Fig. 4c. Table 1 shows the estimated magnon-phonon coupling strength and the relaxation constants of magnons and phonons at three different wavenumbers. The magnon-phonon coupling constant \({b}_{2}=\frac{{\sigma }_{k}}{k}\sqrt{\frac{\rho {M}_{{{{{{{{\rm{s}}}}}}}}}{\omega }_{t}}{2\gamma }}\) is estimated to be (1.8 ± 0.1) × 10^{5 }J ⋅ m^{−3} for all the wavenumbers, which agrees with a previous magneto-striction study^{32}. At *k* = 2.98 × 10^{4 }rad ⋅ cm^{−1}, *σ*_{k} is as large as 53.0 rad ⋅ MHz, while the relaxation constants of magnons and phonons are *κ*_{m} = 2.10 rad ⋅ MHz and *κ*_{p} = 0.49 rad ⋅ MHz, corresponding to the values of lifetime *τ*_{m} = 2.99 *μ*s and *τ*_{p}= 12.8 *μ*s, respectively. For all wavenumbers, *σ*_{k} is greater than *κ*_{m} and *κ*_{p}. The result shows that the gap frequency *σ*_{k} is greater than the spectrum linewidth of both phonons and magnons in the vicinity of the anti-crossing, satisfying the condition of phonon-magnon strong coupling. We calculated the cooperativity \(C={\sigma }_{k}^{2}/{\kappa }_{{{{{{{{\rm{m}}}}}}}}}{\kappa }_{{{{{{{{\rm{p}}}}}}}}}\) of the magnon-phonon coupling to evaluate the strength of the coupling in LuIG, which gives *C* = 2720 ± 2700 for *k* = 2.98 × 10^{4 }rad ⋅ cm^{−1}, *C* = 125 ± 81 for *k* = 3.15 × 10^{4 }rad ⋅ cm^{−1}, and *C* = 127 ± 53 for *k* = 3.30 × 10^{4 }rad ⋅ cm^{−1}. The cooperativity value is much greater than previously reported magnon-phonon coupling in nanomagnet^{30}. The large cooperativity is attributed to the small intrinsic magnetic damping and high-quality factor of phonon in garnet crystals^{33}. Although the error of the cooperativity is still large owing to the limitation of pump-probe delay time, the result implies intrinsic magnon-phonon coupling in a plane film of LuIG can be comparable with strong coupling appears in magnon-photon coupling in a cavity^{31,34}. The magnon-phonon coupling in the film can be further enhanced by fabricating phononic or magnonic crystals out of the plane film^{3}, which may aid in the control of magnons in magnonic circuits and devices. In addition, our demonstration of the magnon-phonon coherent oscillation provides a means of studying the dynamics of coherent superposition of coupled systems, which may pave a way to coherent control of magnetic and elastic properties in various magnetic materials.

## Method

### Time-resolved magneto-optical microscopy

The time-resolved magneto-optical imaging method is realized by combining the time-resolved optical spectroscopy and conventional magneto-optical imaging method, which enables the observation of magnetization dynamics in samples with the spatial resolution of 750 nm and temporal resolution of 1 ps. We used a 100 fs-duration Ti; Sapphire pulse laser system with the central wavelength of 800 nm and 1 kHz repetition frequency (Coherent Inc. Astrella). Pump pulses were prepared by separating a part of the emitted laser. To prepare probe pulses, the central wavelength of a part of the emitted laser was converted to 630 nm by an optical parametric amplifier. The power of the pump and probe pulses was 1.0 *μ*J and 50 nJ per pulse, respectively, which was controlled by the variable ND filter. The pump and probe pulses were linearly polarized along the *y*-axis (Fig. 1e) by using Glan-Taylor prisms. The pump pulse was shaped into a 2.3-μm wide and ~100-μm long vertical line by using a metallic slit. An objective lens collected the transmitted probe pulse with a magnification of 20 and was then introduced to an imaging setup. The imaging setup is composed of a half-waveplate mounted on a rotation stage, an analyzer, and a charge-coupled device (CCD) camera with another objective lens of which the magnification is two. The polarization of the probe pulses was measured using the rotation analyzer method. The detailed optical configuration and analysis are shown in the Supplementary Note 2. We switch on and off the pump beam with a mechanical shutter to measure the magneto-optical images with and without the spin-wave excitation by the pump beam, and take the difference between the images. By sweeping the time delay between the pump and probe pulses, we obtained the propagation dynamics of magnons in the sample. We used an optical fiber to extend the temporal delay between the pump and probe pulses up to 35.4 ns, of which the Fourier frequency resolution (28 MHz) corresponds to the typical energy scale of the magneto-elastic coupling^{32}. We used Lu_{2}Bi_{1}Fe_{3.4}Ga_{1.6}O_{12}(LuIG) grown on a [001] plane of a gadolinium gallium garnet substrate by liquid phase epitaxy as a sample. LuIG is a substituted magnetic garnet with the same crystallographic structure as Y_{3}Fe_{5}O_{12}(YIG), which is known to exhibit small Gilbert damping. The detailed material characterization is described in Supplementary Note 1. LuIG exhibits a large magneto-optical effect (1.5 deg/μm at 630 nm) and small magnetization owing to the Ga substitution^{17}, leading to the small ferromagnetic resonance (FMR) frequency. Owing to the small FMR frequency, the wavenumber of the dispersion intersection between magnons and phonons is small enough to be observed with the present TRMO microscopy. An external magnetic field was applied using a quadrupole electromagnet during the measurement. We analyzed the region in the magneto-optical image which is 10-*μ*m away from the pump focus so as not to include the signal at the pump focus where strong nonlinear effect of phonon such as structural distortion may arise. Owing to the distance between pump focus and the analyzed region, the obtained time-resolved signal has a finite time delay depending on the group velocity of the magnon polaron.

### Calculation of dispersion relation of magnon polaron

In this note, we calculate the dispersion relation of magnon polaron by considering the total Hamiltonian, which involves the spin Hamiltonian, lattice Hamiltonian, and magneto-elastic coupling Hamiltonian as follows^{8},

where, the repetitive use of indices *i*, *j* indicates summation with *i* ≠ *j*, and *H*_{0} is the external magnetic field, *D* = 2*J**S**a*^{2}/*γ**ℏ* is the exchange stiffness, *γ* is the gyromagnetic ratio, *ℏ* is the Dirac constant, *S* is total spin, *J* is the exchange constant, *a* is the lattice constant, *ρ* is the density of the material, *α* = *c*_{12} + *c*_{44} and *β* = *c*_{44} are the elastic constant, *b*_{2} is the shear magneto-elastic constant, *M*_{i} is the *i* -th component of magnetization, *u*_{i} is the *i* -th component of displacement, *M*_{s} is the saturation magnetization, *ω*_{pμ}(*k*) = *v*_{μ}*k* is the dispersion relation of phonon with mode index *μ*, \({v}_{{{{{{{{\rm{L}}}}}}}}}=\sqrt{\alpha /\rho },{v}_{{{{{{{{\rm{T}}}}}}}}}=\sqrt{\beta /2\rho }\) is the velocity of phonon, where L and T represent TA phonon and LA phonon, respectively. *ω*_{m}(*k*) is the dispersion relation of magnons, derived as follows by using the long-wavelength limit of B. A. Kalinikos’s method^{9}. In the long-wavelength limit, the dispersion relation of magnons is written as follows,

where, \({\lambda }_{{{{{{{{\rm{ex}}}}}}}}}=2{A}_{{{{{{{{\rm{ex}}}}}}}}}/{\mu }_{0}{M}_{{{{{{{{\rm{s}}}}}}}}}^{2}\,\left[{{{{{{{{\rm{m}}}}}}}}}^{2}\right]\) is the exchange constant, *ω*_{M} = *γμ*_{0}*M*_{s}, \({g}_{k}=1-\left[1-\exp (-kd)\right]/(kd)\) with the sample thickness *d*. *ω*_{Hα} = *γ**μ*_{0}*H*_{α} and *ω*_{Hβ} = *γ**μ*_{0}*H*_{β} is the Larmor precession frequency defined by anisotropic effective field *H*_{α}, *H*_{β}. We ignore the term originating from compressive strain because it is zero when the relative angle between *θ*_{k} is either 0 or 90^{∘}. In this case, the total effective Hamiltonian is written as follows^{8},

where \({\hat{a}}_{k}({\hat{a}}_{k}^{{{{\dagger}}} })\) is the annihilation (creation) operator of a magnon with a wavenumber *k*, and \({b}_{k\mu }({b}_{k\mu }^{{{{\dagger}}} })\) is the annihilation (creation) operator of a phonon with a wavenumber *k* and mode index *μ* = T, L. *σ*_{kμ} is the coupling constant between magnon and phonon which is written as follows,

By diagonalizing the Hamiltonian, we obtain the following condition for the frequency of the magnon polaron *ω*^{8},

We used *λ*_{ex} = 4.2 × 10^{−13} [m^{2}], *v*_{L} = 6.51[km ⋅ s^{−1}], *v*_{T} = 3.06 [km ⋅ s^{−1}], *b*_{2} = 1.8 × 10^{5} [J ⋅ m^{−3}], *ρ* = 7.39 × 10^{3} [kg ⋅ m^{−3}].

### Derivation of coherent oscillation frequency

In this note, we derive the coherent oscillation frequency from the total effective Hamiltonian defined in the last note. We consider the parallel magnetic field configuration where wavevector **k** and **M** are parallel. In this configuration, only the TA phonon couples with the magnons, thus we set mode index *μ* = T Here, we start from the effective total Hamiltonian as follows,

The effective Hamiltonian can be diagonalized using Bogoliubov transformation defined as follows,

where,

and

The Bogoliubov transformation leads to the diagonalized Hamiltonian as follows,

where *ω*_{c}(*k*) = (*ω*_{pT} + *ω*_{m})/2 + *ω*_{s}, *ω*_{c}(*k*) = (*ω*_{pT} + *ω*_{m})/2 − *ω*_{s}. Here, we define the coherent state of the hybridized wave as follows,

where *γ*_{k} = *u*_{k}*α*_{k} − i*v*_{k}*β*_{kT} (*δ*_{k} = *u*_{k}*β*_{kT} − i*v*_{k}*α*_{k}) is the amplitude of upper (lower) branch of the magnon polaron, *α*_{k} (*β*_{kT}) is the amplitude of magnon (phonon), which are the eigenvalues of the coherent state \(\left|{\gamma }_{k}\right\rangle ,\left|{\delta }_{k}\right\rangle ,\left|{\alpha }_{k}\right\rangle ,\left|{\beta }_{k{{{{{{{\rm{T}}}}}}}}}\right\rangle\). By using time-resolved magneto-optical microscopy, we can measure the amplitude of the magnon, which is proportional to the magnon number. The magnon number at an arbitrary time *t* is calculated by using the coherent state of magnon polaron, as follows,

where, \(\tan \phi ={{{{{{{\rm{Im}}}}}}}}({\delta_k }^{* }{\gamma }_{k})/{{{{{{{\rm{Re}}}}}}}}({\delta_k }^{* }{\gamma }_{k})\). For an initial state, we suppose *α*_{k} = 0, *β*_{kT} ≠ 0 as we excite phonon predominantly by the pump pulse. Then *γ*_{k} = − *i**v*_{k}*β*_{kT}, *δ*_{k} = *u*_{k}*β*_{kT} and *ϕ* = *π*/2 holds, leading to the temporal evolution of magnon number as follows,

Since the frequency difference between upper and lower branch of magnon polaron is expressed by Δ*f* = *ω*_{c} − *ω*_{d} = 2*ω*_{s}, this derivation leads to the expression in Eq. (2). We plotted the Δ*f* in Fig. 3b and d in the main part of our paper.

### Numerical calculation of coherent oscillation

In this note, we derive the coherent oscillation amplitude as a function of wavenumber *k* and time *t*. We consider non-Hermitian Hamiltonian including loss of magnons and phonons, and external field under parallel configuration as follows,

where *κ*_{m}(*κ*_{pT}) is the damping constant of magnon (TA phonon), *κ*^{ex} is the coupling constant between phonon and external excitation force *F*_{k}(*ω*). The equation of motion of the operators leads to the following form.

The excitation spectrum of magnons can be calculated from the equation of motion as follows,

Here, we suppose the spectrum intensity of the external force is determined by the pump focus shape in real space^{25}. Therefore the external force is expressed as follows,

where *σ*_{x}(*σ*_{y}) is the length of the focus along *x*(*y*) − axis, **r** = (*x*, *y*). The spatial distribution of the excitation intensity is plotted in Fig. 5(a). *f*(*t*) is the temporal excitation function defined as follows,

where *t*_{s} (*t*_{e}) is the start (end) time of the square-wave type excitation in time, *σ*_{t} is the parameter to describe smoothness of the square wave. The temporal evolution of the *f*(*t*) is plotted in Fig. 5(b). In calculating coherent oscillation, we need only the component where **k** = *k***e**_{x}, which is *F*_{k}(*ω*) since we consider parallel configuration. The calculated spectrum intensity is shown in Fig. 5(c). The intensity of the spectrum shows a peak at the crossing between dispersion relations of magnons and TA phonons as seen in the experimentally obtained excitation spectra in Fig. 3a and c.

## Data availability

The data that support the findings of this study are available from the corresponding author upon reasonable request.

## Code availability

The code that supports the findings of this study are available from the corresponding author upon request. All the analysis was performed by codes developed by Matlab 2017b software and Matlab signal processing toolbox.

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## Acknowledgements

The authors acknowledge Maki Umeda for technical support. This work was financially supported by JST ERATO Grant Number JPMJER1402, Japan, and JSPS KAKENHI (Grant Numbers JP19H05600, 21H04643, 18J21004, 22K14584), Japan, and JST CREST (Nos. JPMJCR20C1, JPMJCR20T2), Japan, and was partially supported by Institute for AI and Beyond of the University of Tokyo. T.H. acknowledges the support from GP-Spin at Tohoku University.

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T.H. performed the measurement, analyzed the data, and developed the theoretical model. T.H. and E.S. planned and E.S. supervised the study. T.H. wrote the paper with review and input from Y.H. and E.S. All the authors discussed the results and explanation of the experiments.

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### Cite this article

Hioki, T., Hashimoto, Y. & Saitoh, E. Coherent oscillation between phonons and magnons.
*Commun Phys* **5**, 115 (2022). https://doi.org/10.1038/s42005-022-00888-1

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DOI: https://doi.org/10.1038/s42005-022-00888-1

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