Abstract
The de Broglie wave nature of matter is a paradigmatic example of quantum physics and it has been exploited in precision measurements of forces and fundamental constants. However, matterwave interferometry has remained an outstanding challenge for natural polypeptides, building blocks of life, which are fragile and difficult to handle. Here, we demonstrate the wave nature of gramicidin, a natural antibiotic composed of 15 amino acids. Its center of mass is delocalized over more than 20 times the molecular size in our timedomain TalbotLau interferometer. We compare the observed interference fringes with a model that includes both a rigorous treatment of the peptide’s quantum wave nature as well as a quantum chemical assessment of its optical properties to distinguish our result from classical predictions. The realization of quantum optics with this prototypical biomolecule paves the way for quantumassisted measurements on a large class of biologically relevant molecules.
Introduction
The wave nature of massive particles is a central aspect of quantum physics. The free evolution of particles is no longer described by classical trajectories, but instead by a wavelike propagation in multiple directions. Recombining the wavefronts leads to interference, where the probability amplitude for a particle arriving at a certain position depends on the phase difference of the partial waves. Since these phases are sensitive to even small perturbations, matterwave interferometry has become an important tool for atom optics^{1,2}, probing fundamental physics^{3,4,5,6,7} or serving in advanced quantum sensors^{8,9,10}. The de Broglie wave nature has also been shown for large molecules, from fullerenes^{11} and molecular clusters^{12} up to tailormade macromolecules^{13}. Such experiments probe the quantumtoclassical interface and can be used to characterize neutral molecules in the gas phase, through interference fringe deflection in electric and magnetic fields^{14} or minimally invasive spectroscopy^{15,16}.
Until today, quantum optics with fragile natural biomolecules has remained elusive due to the challenges in forming stable and intense molecular beams which can be detected with high efficiency and selectivity. Measurements on neutral biomolecules in the gas phase will, however, become valuable as they are solventfree and allow predicting and evaluating their electronic properties independent of any matrix environments^{17}. A typical matterwave experiment requires an efficient source to launch neutral particles in high vacuum, beam splitters to coherently prepare, separate and recombine the quantum wave function associated with the molecular centerofmass motion and an efficient detector with high sensitivity and mass resolution to record the result. For atom interferometry, these challenges have already been elegantly solved^{2}. For interferometry with complex biomolecules, sources are a prime challenge. While evaporation and sublimation can still be used for vitamins and tripeptides^{18,19}, it denatures and decomposes more complex polypeptides. And while matrix assisted laser desorption^{20} and electrospray ionization^{21} can volatilize even large proteins, they produce ions which are prone to dephasing and decoherence in quantum experiments. Direct laser desorption using nanosecond laser pulses has proven useful to entrain neutral peptides into cold noble gas jets where selected species could be detected using photoionization with VUV radiation^{22}. However, energetic nanosecond pulses typically ablate large amounts of clusters and nanoparticles^{23} in addition to the individual peptides that are desired.
In the following, we present a realization of matterwave interferometry of gramicidin A1, a linear antibiotic polypeptide composed of 15 amino acids with a mass m = 1882 amu = 3.13 × 10^{−24} kg. It has many desirable properties for such an experiment. And as a natural amino acid sequence, produced by the soil bacterium Bacillus brevis, it is representative for a large class of biologically relevant molecules. In addition, it contains four tryptophan residues, which is the only one of all 20 natural amino acids that is ionizable with a single vacuum ultraviolet (VUV) photon with energy 7.9 eV. This is crucial for diffraction and detection of the neutral peptides^{24}.
Results
Experiment
We use the idea presented in Fig. 1: A rotating carbon wheel coated with a biomolecular film serves as the sample supply. From there, the molecules are desorbed by pulsed laser light and entrained in a supersonically expanding noble gas jet. While nanosecond lasers are known to deliver intact peptide beams^{22,25}, ultrafast laser pulses with TW/cm^{2} intensities and pulse lengths of 290 fs allow for 30fold improvement in sample efficiency^{24}. The gramicidin beam is then skimmed, vertically and horizontally collimated to <1 mrad, and sent into the interferometer chamber. In our setup we obtain a velocity v = 600 ms^{−1} when using argon and v = 1200 ms^{−1} when using helium as a carrier gas. The different velocities are used to access different de Broglie wavelengths λ_{dB} = h∕mv, where h is Planck’s constant.
We send the peptides through our timedomain TalbotLau interferometer^{12}, where three pulsed VUV light gratings G^{(1)} − G^{(3)} ionize and remove the molecules in the antinodes of the laser fields (see Fig. 2). The gramicidin molecules arrive with a de Broglie wavelength of λ_{dB }= 350 fm (at v = 600 ms^{−1}) which is about 10^{4} times smaller than the molecular size. We select a velocity spread of Δv∕v ≃ 0.5%, defined by the duration of the carrier gas pulse (20 μs) and the beam width (3 × 3 mm^{2}) of the detection laser. This corresponds to a longitudinal (spectral) de Broglie coherence of ca. 200λ_{dB} ≃ 72 pm. Equally important is the transverse (spatial) coherence which sets an upper limit to the useful width of diffractive elements, across which matterwave phenomena are relevant. Upon arrival at G^{(1)}, it is of the order of 200 pm, too small for diffraction at d = 78.8 nm gratings. However, by defining a precise starting position of the molecules, one can increase their quantum mechanical momentum uncertainty, thus boosting transverse coherence further downstream such that the coherence function covers several effective slits in the second grating. The initial confinement in G^{(1)}, diffraction in G^{(2)} and position sensing in G^{(3)} is done by a position measurement: the molecules can only pass to the detector if they fly through the nodes of all three VUV grating. G^{(1)} thus prepares the required coherence, G^{(2)} diffracts the matterwave and interference results in a molecular density pattern that is modulated by G^{(3)} with nanoscale spatial sensitivity.
The gratings G^{(1)} − G^{(3)} are formed by reflecting three fluorine (F_{2} excimer, λ_{L }= 157.63 nm) laser beams from a single dielectric mirror. This makes the interferometer robust against vibrational dephasing but it also impedes scanning of G^{(3)} across the density pattern. However, a tilt γ of the molecular beam relative to the mirror surfaces allows us to scan the matterwave fringes across G^{(3)} by varying the pulse delay between G^{(2)} and G^{(3)}^{12,26}, as seen in Fig. 2b). For that purpose, we vary the pulse separation time T between the second and third grating in two complementary settings. In the resonant mode, T_{3} − T_{2} = T_{2} − T_{1} are set to the nth multiple of the Talbot time
with the grating period d = λ_{L}∕2. Then, the nearfield resonance condition is met and a clear interference pattern appears. The transmitted molecular signal \({S}_{{\rm{res}}}\) through G^{(3)} depends on the position of the grating nodes relative to the matterwave fringes. In the offresonant (reference) mode, the signal S_{off} is recorded while G^{(3)} is shifted by a variable time ∣τ∣ ≤ 200 ns. For our Talbot time and beam divergence α, the 200 ns shift is sufficient to smear out the interference pattern. The interference contrast is then defined as the normalized signal difference \({S}_{{\rm{N}}}=({S}_{{\rm{res}}}{S}_{{\rm{off}}})/{S}_{{\rm{off}}}\)^{12} (Fig. 2c).
Modeling
We model the expected signal by evolving the transverse Wigner function w(x, p_{x})^{27}, taking into account tilted and divergent molecular beams, as well as mirror and grating imperfections^{28}. As a phase space description, it allows comparing the experiment with both the quantum and the classical expectation within the same framework (see Methods). The free evolution of a particle with initial position x and momentum p_{x} is then described by a shearing transformation \(w\left(x,{p}_{x}\right)\to w\left(x{p}_{x}t/m,{p}_{x}\right)\). Additional terms are introduced to account for earth’s gravitational acceleration g and a tilt of the molecular beam by an angle γ with respect to the mirror surface, which results in an additional constant transverse momentum \({p}_{\gamma }=mv\tan (\gamma )\). The signal seen by the detector depends on the Talbot time T_{T}, the pulse delay τ of G^{(3)} with respect to the Talbot time and the relative shift of the grating nodes to the fringe pattern. Each grating modulates the molecular wave function both in its amplitude and phase via photon absorption and the optical dipole potential, respectively. The transmission function of the kth grating
depends on the number of absorbed photons \({n}_{0}^{({\rm{k}})}\) and the acquired phase shift \({\phi }_{0}^{({\rm{k}})}\) at an antinode, which both contribute to the dimensionless parameter β^{27}
It describes the ratio of the molecule’s wavelengthdependent absorption coefficient σ(λ_{L}) and its optical polarizability volume α_{V}(λ_{L}) (converted to the polarizability in SI units via α[SI] = 4πε_{0} × α_{V}(λ_{L})). The absorption cross section determines the ionization probability and thus controls the effective slit width in all three gratings. The optical polarizability determines the phase the gramicidin molecules acquire during their transit through G^{(2)}. It leaves the fringe periodicity unchanged but modulates the contrast. Since the molecules enter in a variety of different vibrational, rotational and conformational states, as well as orientations, the measured fringes represent an average over the internal properties.
An interferometer with three absorptive gratings would allow for the creation of classical Moirélike patterns. This assumes molecules to be particles following ballistic trajectories that are modified by the gradient forces arising from the interaction between the optical dipole potential of the grating and the molecule’s optical polarizability. The difference between the quantum and the classical expectations is encoded in how these optical properties enter the transmission function (see Methods). The behavior of the fringe contrast is governed by β, making this a crucial parameter for a quantitative distinction between classical and quantum effects. A thorough understanding of the final signal therefore requires knowledge about the electronic properties of gramicidin with respect to its ground and excited states. This is a challenge since gramicidin has many possible conformational states and one has to evaluate electronic properties for an ensemble populating a complex potential energy surface (PES). The gramicidin molecule contains 1010 electrons which renders electronic structure calculations demanding even without global optimization of the conformational space and when combined with density functional theory (DFT). Here, we perform short abinitio molecular dynamics (AIMD) simulations at 300 K, assuming the worst case of no internal cooling, to explore the conformational PES and get a measure of the dynamic polarizability volume of gramicidin (see Methods). Molecular geometries are extracted from the AIMD simulation every picosecond and are fed into subsequent DFT calculations to estimate the ensemble average of the optical polarizability volume \({\left\langle {\alpha }_{V}({\lambda }_{{\rm{L}}})\right\rangle }_{300{\rm{K}}}\).
In addition, the absorption cross section has to be determined as a thermal average \({\left\langle \sigma ({\lambda }_{{\rm{L}}})\right\rangle }_{300{\rm{K}}}\) for the calculation of β. The relevant relaxation channels after photon absorption are ionization and disscociation, since our detector is only sensitive to the depletion of the molecular beam: σ = σ_{PI} + σ_{PD}, where σ_{PI} and σ_{PD} are the photoionization and the photodissociation cross sections, respectively. A lack of detected fragments indicates a comparatively small σ_{PD}, making σ_{PI} a strong lower bound for the total cross section. It is measured under identical conditions in an independent experiment by monitoring the gramicidin ion count rate
as a function of the VUV photon fluence ϕ.
These tools at hand, we can now analyze the matterwave interferogram obtained with gramicidin, both in the first (n = 1) and fractional (n = 1∕2) Talbot order. We record them by shifting the third grating around the ’resonant’ interference mode in steps of 20 ns (n = 1) and 10 ns (n = 1/2) at a fixed time delay for the offresonant reference signal at τ_{off} = 200 ns (n = 1) and 100 ns (n = 1/2). For a finite divergence and tilt of the molecular beam, the fringe density pattern scans across the grating when τ is varied. We expect a sinusoidal modulation with a Gaussian envelope^{26} (see Figs. 2c and 3).
The modulation of the fringe visibility V_{0} allows us to more precisely determine the divergence angle α = 0.4 mrad from the width σ_{w} of the resonance dip
and the tilt angle γ = 1.7 mrad from the observed fringe period σ_{p}
We extract the model parameters α and γ from the data in Fig. 3, the absorption cross section from independent measurements and the VUV polarizability volume from our quantum chemical analysis.
The dynamic polarizability volume is computed by QChem^{29} using DFT with the rangeseparated hybrid exchangecorrelation functional LCωPBEh^{30}, which has been shown to perform well for the calculation of polarizabilites^{31}, and the 631G basis set. The CoupledPerturbed KohnSham method^{32} is used to calculate the optical polarizability volume for every extracted geometry at λ_{L} to obtain the ensemble average \({\left\langle {\alpha }_{V}({\lambda }_{{\rm{L}}})\right\rangle }_{300{\rm{K}}}\) = (157 ± 1) × 10^{−30 }m^{3}.
In order to obtain the photoionization cross section σ_{PI}, we measure and plot the number of ions N_{I} as a function of the photon fluence ϕ (see Methods, Fig. 4) and construct a fit according to Eq. (4). We find an ionization cross section of σ_{PI} = \({\left\langle \sigma ({\lambda }_{{\rm{L}}})\right\rangle }_{300{\rm{K}}}\) = (4.7 ± 0.2) × 10^{−20 }m^{2} and thus β ≃ 0.6. This value is used for simulating both the quantum and classical predictions.
The final result is shown in Fig. 3, which compares the experimental data (black circles), with a fit based on Eq. (5) (solid red line), the quantum simulation (dashed blue line) and the classical description (dotted green line). Figure 3a presents data for the first Talbot order, while Fig. 3b shows the n = 1/2 Talbot order, where the peptides are entrained in helium to double their mean velocity to 1200 ms^{−1}. In both cases, the resulting molecular density pattern at G^{(3)} has a fringe separation of d = 78.8 nm since at the half Talbot order (n = 1∕2), the halving of the fringe period in time is caused by the doubling of the molecular velocity.
In the first Talbot order, the experimental fringe contrast is very well described using quantum wave mechanics (blue dashed line) while a description using classical trajectories (green dotted line) misses the amplitude by almost an order of magnitude. On the other hand, both models approach each other and the experiment at the half Talbot order (Fig. 3b). At very short intervals between the gratings, there is too little time for the molecular matterwaves to spread out in space.
Claiming the quantum nature of the fringe pattern requires to check if there is any reasonable way to reproduce the observed fringe contrast at n = 1 in a classical model, for instance assuming molecular properties that differ from their computed or measured values. We find that β ≃ 100 rather than β ≃ 0.6 would be required for the classical curve to mimic the quantum result. This is vastly incompatible with the calculations and observations described above and also inconsistent with β values found in many other organic molecules and clusters^{28}. The quantum model appears to be the only plausible explanation for our experimental results.
One may also ask for the role of external forces, such as gravity, in this setting. The normalized signal difference is a function of the pulse separation time T and the Earth’s gravitational acceleration g via \({S}_{{\rm{N}}}(T)={V}_{0}\sin \left(2\pi (bg{T}^{2})/d\right)\), with b a constant offset on the laser mirror^{26}. At fixed Talbot order, gravity influences the absolute fringe height, but within the 100 ns fringe envelope, of Fig. 3 gravity does not cause any noticeable timedependence.
In summary, we have demonstrated matterwave interferometry with a complex native polypeptide, the antibiotic gramicidin. The fringe visibility of around 20% in the first Talbot order stands in marked discrepancy to a classical phase space description and is in very good agreement with quantum mechanics, including a detailed quantum chemical analysis of the molecular electronic properties. Our source techniques based on UV femtosecond desorption can volatilize fragile biomolecules in a more efficient way than other methods to date. While matterwave experiments with biomolecules in the gas phase do not elucidate biological function per se—which is related to electronic structure determining folding dynamics and interactions with matrix environments—our experiments show that quantum phenomena can be observed with building blocks of life under suitable boundary conditions. Molecular interference patterns can be used as flying nanorulers^{33} that will become important in studies of optoelectronic and structural properties of complex biomolecules.
Methods
Sample preparation
Gramicidin D (Sigma Aldrich, CAS: 1405976) is used which is a mixture of different antibiotic compounds. The major component is gramicidin A1, a linear polypeptide composed of 15 amino acids. It has the chemical formula C_{99}H_{142}N_{20}O_{17}. The molecule sketched in Fig. 1 represents one specific configuration of gramicidin A1. The green ribbon follows the peptide sequence while the tryptophan, valine and isoleucine rest groups are explicitly shown. The source emits a large variety of structural conformers, which all contribute to the same matterwave interference pattern, since their mass and VUV optical properties are nearly identical. There are both molecular fermions and bosons in the sample, but quantum statistics is irrelevant in our singlemolecule interference experiments. All molecules are excited in several of their 828 vibrational modes and highly excited in their rotational degrees of freedom.
Molecular beam
The experiment runs at 100 Hz. In every cycle, an EvenLavie valve releases a 20 μs short and dense pulse of argon with a backing pressure of about 30 bar. A femtosecond laser (Topag PHAROS, 290 fs, 70 μJ, 343 nm) is focused (\(\varnothing\) = 100 μm) onto the surface of a glassy carbon wheel coated with gramicidin to create a cloud of isolated molecules. The argon (helium) pulses then entrain the molecules with a mean velocity of around 600 ms^{−1} (1200 ms^{−1}). Further downstream the particle beam is skimmed (Beam Dynamics skimmer, \(\varnothing\) = 2 mm), collimated to a rectangular shape of 0.6 × 1 mm^{2} (the longer axis parallel to the grating vectors) and finally transferred to the interferometer chamber via a differentially pumped stage. The pressure in the main chamber is 2 × 10^{−9} mbar, in the source chamber 1 × 10^{−8} mbar. Molecular beam velocities are determined by comparing the timing of the desorption laser with the detection laser pulse.
Grating lasers
The grating laser beams are emitted by three GAM EX50 fluorine lasers (λ_{L} = 157.6 nm, 4 mJ, 8 ns, flat top profile). All beams are reflected by the same dielectric mirror 3 × 5 cm^{2}, coated onto a 2 cm thick CaF_{2} substrate with the best technically available reflectivity in this wavelength range to date, i.e., R ≃ 97%. The laser waists are elongated parallel to the molecular beam axis z (10 × 1 mm^{2}) and spatially separated by ≈2 cm which allows molecules of different velocities to interact with a laser grating at the same time.
Mirror imperfections
For a perfectly flat mirror and in the absence of external accelerations, S_{N} is positive and equal to the theoretical visibility. In a real world scenario, S_{N} is given by the visibility of the molecular density pattern at the position of G^{(3)} and its relative displacement ΔD = Δx_{1} −2Δx_{2} + Δx_{3} of this Talbot image with respect to G^{(3)}. Here, Δx_{i} captures both the possible mirror corrugations at either grating site or the displacement of the molecular fringe due to external accelerations—for instance gravity. The molecular transmission is maximized for ΔD = nd and minimized for ΔD = (n + 1∕2)d with \(n\in {\mathbb{Z}}\). If the mirror surface had deformations exceeding 10 nm across the 10 mm grating laser beam profile, molecules of the same gas pulse but with different velocities would experience differently shifted interferometers. To avoid the ensuing reduction in fringe contrast, the effective grating width is set to <3 mm by the geometry of the final detection laser.
Vibrational stability
The most important vibration frequencies in the experiment are related to the frequencies of the turbomolecular pumps. Taking 3000 Hz as a higher order worst case scenario the amplitude required for a 1∕e contrast reduction is ≈15 nm, while the noise at that frequency is estimated to be ≈1 nm.
Coriolis force
Considering the latitude (48.22^{∘}N) and orientation (162^{∘}SSE) of the molecular beam on Earth and assuming a velocity of 600 ms^{−1} the Coriolis force on gramicidin causes a shift of around 1 nm. Even for large velocity spreads phase averaging can be neglected. Also pathlength differences arising from the Coriolis force are negligible for the mass considered here.
Optical polarizability volume at λ _{L}
The AIMD (BLYP^{34,35}/631G) simulations are performed using the TeraChem program package^{36,37}. During the AIMD run, a single molecule is propagated over 50 ps in time steps of 1 fs at a temperature of 300 K, which is controlled by a BussiParinello thermostat^{38} with a relaxation time of 0.1 ps. The dynamic polarizability volume is computed by QChem^{29} using DFT with the rangeseparated hybrid exchangecorrelation functional LCωPBEh^{30} and the 631G basis set. The CoupledPerturbed KohnSham method^{32} is used to calculate the optical polarizability for every extracted geometry at λ_{L} to obtain the ensemble average. LCωPBEh has been shown to perform well for the calculation of polarizabilites^{39}.
Ionization cross section at λ _{L}
In order to obtain σ_{PI}, we measure and plot the number of counted ions N_{I} as a function of the photon fluence ϕ (see Fig. 4), which is the total number of photons per unit area integrated over the laser pulse length:
where σ_{PI} and the total number of molecules N_{0} enter as fit parameters.
Data analysis
In order to calculate S_{N}, mass spectra are summed up and subtracted from the background in both measurement modes to obtain \({S}_{{\rm{res}}}\) and \({S}_{{\rm{off}}}\). There is a systematic error by assuming that the mass signals are proportional to the number of detected molecules. We thus consider a worst case scenario where every event at the detector is attributed to a single detected molecule N_{event} = 1. We then compare the amplitudes of our mass signals within a threshold value, that is derived from the standard deviation of the background noise. The probability of not detecting a particle P_{zero} is assumed to follow Poissonian statistics
with λ_{P} as the average number of counts per frame. The total number of detected molecules N within one measurement consisting of N_{frames} is then given by
while Gaussian error propagation delivers the 1σ errorbars of each data point.
Quantum model of the interference fringes
Our beam experiments are supported by phase space simulations as introduced by Nimmrichter and Hornberger for nearfield matterwave interferometry^{40} and refined for timedomain experiments^{27}. We here adapt the model to the details of our study. The simulations are based on the onedimensional Wigner function w(x, p_{x}) with x and p_{x} for the positions and the momenta of states, respectively. The Wigner function is defined as the transformation of the position density matrix \(\rho (x,x^{\prime} )=\left\langle x\right\hat{\rho }\leftx^{\prime} \right\rangle\)^{41}
where the molecular beam propagation at a time t is represented by the Hamiltonian \({{\mathcal{H}}}_{0}={p}_{x}^{2}/2m\) in absence of external fields. The Wigner function therefore transforms like
The formalism allows a simple comparison with classical phase space dynamics based on ballistic trajectories. Under free evolution the classical phase space density transforms like the Wigner function^{42}.
Position shifts due to constant accelerations parallel to the grating vectors (xaxis) can be included to account for gravitational, electric or magnetic forces. Additionally, a tilt of the molecular beam by the angle γ can be introduced as a constant momentum \({p}_{\gamma }=mv\tan (\gamma )\) parallel to the xaxis. The Wigner function for free propagation over a time t therefore reads
Transmission through the kth grating G^{(k)} is described by a complex transmission function t^{(k)}(x) acting on the position density matrix
while \({\left{t}^{({\rm{k}})}(x)\right}^{2}\) gives the probability for a particle at position x to remain in the beam and is assumed to follow poissonian statistics
where n^{(k)}(x) is the number of absorbed photons and shows a dperiodic modulation
While \({\left{t}^{({\rm{k}})}(x)\right}^{2}\) describes a pure absorptive grating, the additional phase modulation ϕ^{(k)}(x) is described by
Here \({n}_{0}^{({\rm{k}})}\) is the average number of absorbed photons in an antinode and \({\phi }_{0}^{({\rm{k}})}\) the eikonal phase, gained by integration of the interaction potential over the intensity profile of the laser. For the optical gratings they read^{43}
where E^{(k)} is the pulse energy, A_{L} the illuminated area, c the speed of light, σ(λ_{L}) the absorption cross section and α_{V}(λ_{L}) the optical polarizability at the grating wavelength λ_{L}. Taking imperfections into account such as a mirror reflectivity R = 0.97 and a grating coherence factor C = 0.76^{28}, there is an effective reduction of the coherent contribution to \({n}_{0}^{({\rm{k}})}\) and \({\phi }_{0}^{({\rm{k}})}\)
Using these parameters the complex transmission function of the optical gratings reads
Transmission through a grating is described by the convolution of the Wigner function and the transmission kernel
For optical gratings the transmission kernel T^{(k)}(x, p) consists of the Talbot coefficients \({B}_{{\rm{n}}}^{({\rm{k}})}(\chi )\), gained by Fourier expansion of the transmission function \({t}^{({\rm{k}})}\left(x\right)\)
with the dimensionless parameter β as the ratio of molecular absorption cross section and optical polarizability containing information about the electronic structure of the considered molecules
Transformation (Eq. 21) also holds for the classical case when we exchange the Talbot coefficients \({B}_{n}^{({\rm{k}})}(\chi )\) in Eq. (22) with classical coefficients \({C}_{n}^{({\rm{k}})}(\chi )\) the effect of the grating on classical ballistic trajectories. These coefficients are not periodic in χ. This changes \(\sin (\pi \chi )\to \pi \chi\) and \(\cos (\pi \chi )\to 1\) in Eq. (23)^{44,45}. For χ → 0, \({B}_{n}^{({\rm{k}})}(0)\) and \({C}_{n}^{({\rm{k}})}(0)\) are identical and describe the behavior of a purely absorptive grating. Both classical and quantum coefficients then simplify in terms of the modified Bessel functions I_{n}(x):
This formalism allows to describe the beam propagation through a TalbotLauInterferometer as sequences of free propagation followed by transmission through a grating. The initial state at the first grating is assumed to be an incoherent mixture with a spatial extension X_{0} ≫ d and a momentum P_{0} ≫ h∕d. The initial Wigner function at the first grating w_{0}(x, p_{x}) is described by the transverse momentum distribution D(p_{x}), which is gained by integration of the three dimensional momentum density distribution μ(p_{x}, p_{y}, p_{z}) over two dimensions: D(p_{x}) = ∫dp_{y} dp_{z}μ(p_{x}, p_{y}, p_{z}). This leads to
where p_{γ} denotes the additional constant momentum due to the tilt. According to Eq. (21), transmission through the first grating with the transmission kernel T^{(1)} leads to \({w}_{1}\left(x,{p}_{x}\right)\). Note that p_{γ} is a constant momentum. Therefore the substitution in the integral \(\int dp^{\prime} {T}^{(1)}(x,{p}_{x}p^{\prime} )D(p^{\prime} )\) with \(p^{\prime} ={p}_{0}+{p}_{\gamma }\) leads to \(dp^{\prime} =d({p}_{0}+{p}_{\gamma })=d{p}_{0}\). With iterative usage of Eq. (13) and Eq. (21), the Wigner function transforms to w_{2}(x, p_{x}) after free propagation for a time t = T_{1}, then to w_{3}(x, p_{x}) after transmission through the second grating and after another free propagation for a time t = T_{2}, it transforms to w_{4}(x, p_{x}), which denotes the state of the beam before interacting with the third grating. The corresponding transformations are listed below:
The third grating masks the fringe pattern of the traversing molecular beam in space. Finally, all molecules are detected independent of their transverse momentum. Therefore only the spatial density distribution of the beam is needed which is calculated by integrating w_{4}(x, p_{x}) over the momentum. \(\widetilde{D}(x)\) is the Fourier transform of the momentum distribution^{44,46}
Due to the broad initial momentum, \(\widetilde{D}(x)\) is assumed to be very narrow and to peak around \(\widetilde{D}(0)=1\). So only index pairs (k, l) which fulfill \(\leftk{T}_{1}+l{T}_{2}\right\ll {T}_{{\rm{T}}}\) contribute to the integral of \({w}_{4}\left(x,{p}_{x}\right)\) in Eq. (27). In the nearresonant and symmetric approximation one assumes T_{1} = T and T_{2} = T + τ, where τ denotes a small delay of the grating timing compared to the Talbot time \(\left\tau \right\ll {T}_{{\rm{T}}}\). This restricts the index pairs (k, l) to k = −l and changes the Wigner function w_{4}(x) to
Here Δx_{s} denotes the relative grating shift Δx_{s} = Δx_{1} − 2Δx_{2} + Δx_{3}. The spatial distribution of w_{4}(x) is scanned using the third grating, which acts as a purely absorptive mask. Therefore one can use \({B}_{l}^{(3)}(0)\) from Eq. (25). For sufficiently small delays τ and due to the random phase of the impinging matterwave, G^{(1)} can also be treated as a purely absorptive grating, with \({B}_{l}^{(1)}(d\ l\tau /{T}_{{\rm{T}}})={B}_{l}^{(1)}(0)\).
Convolution of Eq. (29) with the transmission Kernel T^{(3)}(x, p) and integration over the whole phase space leads to the detected signal S(Δx) behind the third grating
The periodic modulation of \(S\left(\Delta x\right)\) is observed by scanning over the phase of Eq. (31). This can be done either by changing the grating shift Δx_{s} or the momentum contribution p_{γ}τ∕m. A slight delay of the third grating timing τ modulates the phase, as well as the signal amplitude, due to the contribution of τ to the sharp peaked function \(\widetilde{D}\).
Periodicity of the observed fringes
The simulations in Fig. 3 show that only quantum interference can explain the observed normalized fringe signal and the role of complex (real and imaginary) optical gratings is important. In an interferometer with three binary transmission gratings, quantum theory would predict a halving of the fringe period at half the Talbot order n = 1/2^{47}. However, this prediction becomes intensity dependent when using optical gratings. Figure 5 shows the quantum and classical expectation for the molecular density at G^{(3)} in the half Talbot order as a function of laser power, i.e., as a function of the mean number of photons absorbed in the antinodes of each grating, n_{0,eff}. For n_{0,eff} = 3, as used in our experiments, dperiodic fringes are expected in both the n = 1 and the n = 1/2 Talbot order, classically and quantum mechanically. However, for n = 1, the quantitative distinction between both models is clear and with a large margin in our experiment (see main text).
Data availability
The data that support the findings of this study—in particular the raw data of Fig. 3 incl. measured data, error bars, fit, classical and quantum prediction—are available from the corresponding authors upon reasonable request.
Code availability
The proprietary Matlab code that has been developed throughout the years and used to produce the classical and quantum predictions as described in the methods section is available to the editor and reviewers on request from the corresponding authors.
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Acknowledgements
A.S. acknowledges funding by the Austrian Science Fund (FWF) within the LiseMeitner fellowship M 2364. M.A. has received funding from the European Research Council (ERC) under the European Union’s Horizon 2020 research and innovation program (Grant Nr. 320694). U.S. was supported by the Austrian Science Fund (FWF) within program W1210N25. The computational results presented were partly obtained using the Vienna Scientific Cluster (VSC) within 70918. We are grateful to NSF for computing time provided on XSEDE resources via award TGMCB090110. We are thankful to Nadine AsenbaumDörre, Philipp Haslinger, Andrea Grimaldi, and Gustavo G. Rondina for fruitful discussions and previous work and support. We thank Marcel Mayor, Valentin Köhler and Jonas Schätti for joint explorations of biomolecular beam methods, as well as Klaus Hornberger and Stefan Nimmrichter for their development of the Wigner phase space formalism and code for Talbot Lau interferometry throughout previous years, parts of which were adapted by A.S. and P.R. to the needs of our present work.
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The experiments were conceived by A.S. and M.A. The interference experiments were realized by A.S., G.R. and P.R. The source has been designed and adapted to the OTIMA experiment by A.S., G.R., P.R., U.S., and P.G. Data analysis was performed by A.S., G.R., J.R., and P.R. and Quantum chemical simulations were modeled and analyzed by A.S. and T.M. and realized by T.M. The manuscript was written by A.S. and M.A. with contributions from all authors.
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Shayeghi, A., Rieser, P., Richter, G. et al. Matterwave interference of a native polypeptide. Nat Commun 11, 1447 (2020). https://doi.org/10.1038/s41467020152802
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DOI: https://doi.org/10.1038/s41467020152802
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