Corrigendum: Photon number statistics uncover the fluctuations in non-equilibrium lattice dynamics

Nature Communications 6: Article number: 10249 (2015); Published: 22 December 2015; Updated: 1 February 2016 The affiliation details for Davide Boschetto are incorrect in this article. The correct affiliation details for this author are given below: Laboratoire d’Optique Appliquée, ENSTA ParisTech, CNRS, Ecole polytechnique, Université Paris-Saclay, 828 boulevard des Maréchaux, 91762 Palaiseau cedex, France.

I n a classical description, the displacement of the atoms along the vibrational eigenmodes of a crystal can be measured with unlimited precision. Conversely, in the quantum formalism positions and momenta of the atoms can be determined simultaneously only within the boundary given by the Heisenberg uncertainty principle. For this reason, in real materials, in addition to the thermal disorder, the atomic displacements are subject to fluctuations which are intrinsic to their quantum nature. While various evidences suggest that such quantum fluctuations may be of relevance in determining the onset of intriguing material properties, such as quantum para-electricity, charge density waves or even high temperature superconductivity [1][2][3][4][5][6][7] , the possibility of measuring quantum fluctuations in solids is the subject of an intense debate [8][9][10][11][12][13][14][15][16][17][18][19][20][21] .
The time evolution of atomic positions in materials is usually addressed by means of non-equilibrium optical spectroscopy. An ultrashort light pulse (the pump) impulsively perturbs the lattice and a second one (the probe), properly delayed in time, measures a response that is proportional to the spatially averaged instantaneous atomic positions. In those experiments, the time-dependent atomic displacements are often revealed by an oscillating response, commonly dubbed coherent phonon response [22][23][24][25][26][27][28][29][30][31][32] , at frequencies characteristic of the vibrational modes of the material. In this framework, it has been shown that a non-linear light-matter interaction can prepare non-classical vibrational states 8,13 such as squeezed states, where the fluctuations of the lattice position (or momentum) can fall below the thermal limit. A reduction below the vacuum limit is known as vacuum squeezing 16 .
Here we propose a joint experimental and theoretical approach to access the fluctuations of the atomic positions in time domain studies. An experimental apparatus that allows for the measurement of the photon number quantum fluctuations of the scattered probe pulses in a pump and probe set-up is adopted. The connection between the measured photon number uncertainty and the fluctuations of the atomic positions is given by a fully quantum mechanical theoretical description of the time domain process. Overall we prove that, under appropriate experimental conditions, the fluctuations of the lattice displacements can be directly linked to the photon number quantum fluctuations of the scattered probe pulses. Our methodology, that combines non-linear spectroscopic techniques with a quantum description of the electromagnetic fields, is benchmarked on the measurement of phonon squeezing in a-quartz.

Results
Shot-noise-limited pump and probe experiments. In the non-linear spectroscopy formalism, the excitation mechanism of phonon states in transparent materials is called impulsive stimulated Raman scattering (ISRS) 29 . The susceptibility tensor w (3) connects the induced third order polarization P (3) to three fields: E 1 ðo 1 Þ, E 2 ðo 2 Þ and E 3 ðo 3 Þ 33 . In conventional two pulses pump and probe experiments, the fields E 2 ðo 2 Þ and E 3 ðo 3 Þ are two different frequency components of the pump laser pulse. In particular, all photon pairs such that o 3 À o 2 ¼ O, where O is the frequency of the Raman active vibrational mode, contribute to ISRS 34 . The interaction of the probe field E 1 ðo 1 Þ with the photo-excited material induces an emitted field, E EF ðoÞ, which depends on the pump-probe delay and carries information about the specific Raman mode excited in the crystal. Experimental details are reported in (Supplementary Note 1). We choose a polarization layout designed to excite E-symmetry Raman optical modes in a-quartz at room temperature and get an emitted field with polarization orthogonal to the probe one 35 ( Supplementary Fig. 1).
The experimental layout is similar to standard pump and probe experiments. The sample is excited by an ultrashort pump pulse and the time evolution of the response is measured by means of a second much weaker probe pulse, which interacts with the photo-excited material at a delay time t. The unique characteristics of our set-up are: unlike standard experiments, where the response is integrated over many repeated measurements, our system can measure individual pulses; the apparatus operates in low noise conditions allowing for the measurement of intrinsic photon number quantum fluctuations. In detail, we adopt a differential acquisition scheme where each probe pulse is referenced with a second pulse which has not interacted with the sample. For each measurement, the differential voltage is digitized and integrated, giving the transmittance DT i for the ith measurement. For every given pump and probe delay t, we repeat this single-pulse measurements for N ¼ 4,000 consecutive pulses. Figure 1a gives a useful visual representation of the obtained data. For one pump and probe scan l, the normalized histogram of N ¼ 4,000 acquired pulses for each delay time is shown. Each histogram represents the distribution of the measured DT i for a specific delay time t. For a clearer visualization of the physically meaningful information in the time evolution of the statistical distribution, Fig. 1b reports the histogram centred at zero.
The pump and probe scan is repeated several times and each lth scan provides DT ðlÞ mean ¼ 1  Fig. 2a for a representative pump fluence of 14 mJ cm À 2 (a pump fluence-dependent study is reported later). The blue curve depicts the time evolution of the mean value of the transmittance DT mean , whereas the red curve shows the time evolution of its variance DT var . The Fourier transform of the mean (Fig. 2c, blue curve) has a single peak which is ascribed to the E-symmetry quartz vibrational mode with frequency O ¼ 128 cm À 1 ¼ 3.84 THz 36 . The same frequency component is observed in the Fourier transform of the variance (Fig. 2c, red curve). In addition, a second peak at twice the phonon frequency appears exclusively in the variance. A wavelet analysis of the variance oscillations allows for a time domain study of the two frequency components (Fig. 2b): one notices that while the fundamental frequency survives for roughly 7 ps, the 2O component vanishes within the first 2 ps. The different lifetimes between the O and 2O components of the variance are seen also by a close inspection of the raw data distribution plotted in Fig. 2b.
Note that the 2O in our data is visible only in experimental conditions where the noise is dominated by the quantum uncertainty, a situation which is known as shot-noise regime. In such conditions, DT var measures the quantum variance of the scattered probe photon number. A full characterization of the detection system is reported in (Supplementary Note 2), including the shot-noise characterization ( Supplementary Fig. 2) and the analysis of classical noise sources (Supplementary Figs 3 and 4). It should further be stressed that in experimental conditions where the noise is larger and dominated by classical sources, the 2O contribution to the noise becomes unmeasurable.
The presence of the 2O frequency component is suggestive of phonon squeezing, as it has been indicated by Raman tensor models 8,9,12 . Nevertheless, the experimental evidences up to date lack a direct comparison with a reliable quantum noise reference 10,11,13,20 . Hence, in these experiments the observation of the 2O frequency in the optical noise is considered as an indication of phonon squeezing, but not an unequivocal proof. In details, a 2O oscillating optical noise was reported in ref. 13, but later ascribed to an artifact 15 due to the experimental amplification process. In particular, it has been demonstrated that amplification artifacts become more relevant when, using a lock-in amplifierbased acquisition, the time constant of the lock-in increases with respect to the time between steps in the pump-probe delay. This gives rise to maxima in the noise where the derivative of the mean signal is maximal 15 . Here we use a pump power density, which is almost 3 orders of magnitude higher than in refs 13,15. In addition, we observe a 2O frequency component in the optical variance which exhibits maxima in correspondence with the minima of the derivative of the mean signal, hence ruling out possible artifacts of the kind described in (ref. 15).
Fully quantum description of ISRS. To predict how the fluctuations of the atomic positions in a lattice can be mapped onto the photon number quantum fluctuations of the probe field, we develop a theoretical approach to time domain studies, which treats quantum mechanically both the material and the optical fields involved in the non-linear processes. Several semiclassical models describe the possibility of generating 'classical' (coherent states) and non-classical vibrational states by photo-excitation. In particular, for transparent materials like quartz, the most commonly used approach is to adopt Raman tensor models where the interaction between photons and phonons is not mediated by dipole-allowed electronic transitions. In this condition, interactions linear in the phonon operators allow for the generation of coherent vibrational states, while high order interactions are required for the generation of non-classical squeezed states 9,12,32 . In materials with allowed dipole transitions, as in presence of excitons, different models based on electron-phonon coupling Hamiltonians have been proposed. In those models it has been shown that squeezed phonon states can result only by successive excitations with a pair of pulses 16,17 . All these models mainly adopt semiclassical approaches where the optical fields are described classically 33 , and therefore are unable to reproduce the quantum proprieties of the probe optical field that can be measured with the shot-noise-limited pump and probe set-up presented here. The key aspect of our approach, allowing us to bridge this gap, is to study both generation and detection of phonon states using a fully quantum formalism through an effective photon-phonon interaction, which is descriptive of experiments in transparent systems, such as a-quartz. The basic tool is a quantum Hamiltonian able to describe both pump and probe processes. Being linear and bilinear in the photon and phonon operators, this Hamiltonian accounts for the possible generation of coherent and squeezed phonon states through the pump process. In particular, it models also the detection of the photo-excited phonon states, describing the probing process by a fully quantum approach, providing in this way a direct comparison with the experimentally measured photon number quantum fluctuations of the scattered probe pulses 37 .
In this framework, the first step is to adopt a quantized description for the mode-locked pulsed laser fields 38 . Each mode of frequency o j ¼ o 0 þ jd, where o 0 is the pulse central frequency, d is a constant depending on the laser repetition rate and j is an integer, is quantized and described by single-mode creation and annihilation operatorsâ w j andâ j . In this framework, ISRS can be modelled by means of an effective impulsive interaction Hamiltonian, which is descriptive of both the pumping and the probing processes. In both processes, two optical fields with orthogonal polarizations (denoted with subscript x or y) are involved: two pump fields in the pumping process and the probe and the emitted field in the probing process. The interaction Hamiltonian has the form where 2J þ 1 is the total number of modes within a mode-locked optical pulse,b andb y are the phonon annihilation and creation operators; m d and m s are coupling constants ARTICLE and the function g ' j;j 0 takes into account the relations between the frequencies of the involved fields, with O the phonon frequency. A complete interaction Hamiltonian should contain also second order processes involving phonons with opposite momenta. However, since the probe detects only the kC0 optical transition, we can make use of an effective Hamiltonian that accounts only for this kind of process.
The whole theoretical description of the experiment can be rationalized in a four-step process as sketched in Fig. 3: (i) generation of phonon states in the pumping process, (ii) evolution of the produced vibrational state, (iii) probing process and (iv) read out of the emitted photon observables.
(i) Initially, the sample is in thermal equilibrium and it is described by a thermal phonon stater b , at inverse temperature b. The laser pump pulse is described by a multimode coherent state of high intensity n j i ¼ n À J j i Á Á Á n J j i, where n j are single-mode coherent states associated with all the frequency components within the pulse. Each n j is an eigenstate of the annihilation operatorâ j of photons in the mode of frequency o j , a j n j ¼ n j n j . We indicate with n the vector whose components are the amplitudes n j . The equilibrium (pre-pump) photon-phonon stater ¼ n j i n h j r b is instantaneously transformed intor n ¼ UrU y by means of the unitary operator U ¼ expf À iHg. Since the pumping operator U acts on a high intensity photon coherent state n, we can use the mean field approximation for the photon degrees of freedom and replaceâ with n andâ y with n* for both pump modes involved in equation (1), thus replacing U by The evolution operator generates coherent and squeezed phonon states, respectively, through the linear and quadratic terms in the phonon operatorsb andb y . The initial stater n contains information about both photons and phonons. Tracing over the photon degrees of freedom, the resulting stater n II describes the excited phonons brought out of equilibrium by the impulsive pump process.
(ii) The time evolution of the excited phonons is described by using an open quantum systems approach, namely by means of a suitable master equation of Lindblad form 39,40 that takes into account, besides the quantum unitary evolution, also the dissipative and noisy effects due to the interaction with a thermal environment.
(iii) The incoming probe pulses are in the multimode coherent state a j i. The probing process at time t is described by the same impulsive unitary operator U used for the pump. However, in this case we can apply the mean field approximation only to the probe photon operators with x polarization, which correspond to a much more intense field than those with y polarization. Moreover, since the probe field is much weaker than the pump field, the quadratic terms in the interaction Hamiltonian in equation (1) can now be neglected. The resulting unitary operator is Að where a 0 is the vector with components a 0 j ¼ m d P J j 0 ¼ À J g 1 j 0 ;j a xj 0 andÂð a 0 Þ is a collective photon annihilation operator such that ½Âð a 0 Þ;Â w ð a 0 Þ ¼ 1. The latter unitary operator acts on a state of the form a j i a j i r n II ðtÞ. The information about the phonons are extracted by measuring the emitted field photons. In particular, the emitted photon stater I ðtÞ is obtained by tracing away the phonon degrees of freedom.
(iv) The possible quantum features of the phonon state, for example, squeezing, can be read off as they are imprinted intô r I ðtÞ. In particular for each time delay t, we can compute the quantities hN y i t ¼Â w ð a 0 ÞÂð a 0 Þ t and D 2 tN y ¼ hN 2

Discussion
The proposed effective interaction model is further validated by a pump fluence dependence study. Figure 5 shows the amplitude of the 2O peak in the Fourier transform of the variance, DT var , as a function of the pump fluence. A fluence dependence study of the O peak is reported in (Supplementary Fig. 5). The functional behaviour obtained from the model predictions (continuous line in Fig. 5) agrees with the experimental data only in presence of a pump-induced squeezing of the phonon mode (m s a0). The increase of the 2O peak amplitude with the pump fluence allows us to give a direct estimation of the uncertainties of the phonon-conjugated quadratures, which are reported in the inset of Fig. 5 for the different excitation fluences (calculation details are given in (Supplementary Note 3)). For high pump fluences, the uncertainty on one of the phonon quadratures falls below the MATTER (System II) LIGHT (System I) The comparison of the predicted noise with the experimental photon number quantum uncertainty, measured in shot-noise conditions, allows us to unveil non-classical vibrational states produced by photo-excitation. A future extension of the model taking into account the role of the electronic degrees of freedom would allow to extend such a study from transparent materials to complex absorbing systems.
In conclusion, a Raman active phonon mode has been impulsively excited via ISRS in a a-quartz by means of a pump and probe transmittance experiment with single-pulse differential acquisition in noise conditions limited by intrinsic probe photon number fluctuations. A fully quantum mechanical effective model where both phonons generation and detection are studied through the same effective coupling Hamiltonian establishes a direct connection between the measured photon number quantum fluctuations of the emitted probe field and the fluctuations of the atomic positions in a real material. Our approach is used here to reveal distinctive quantum properties of vibrational states in matter, in particular the squeezed nature of photo-excited phonon states in a-quartz. Finally, we stress that our approach can be applied in future studies addressing the role of unconventional vibrational states in complex systems 3,6 , and the thermodynamics of vibrational states 41,42 possibly in the quantum regime.