{'fraction_non_alphanumeric': 0.026384597100071308, 'fraction_numerical': 0.011350130734490135, 'mean_word_length': 4.517704918032787, 'pattern_counts': {'":': 0, '<': 1, '<?xml version=': 0, '>': 1, 'https://': 0, 'lorem ipsum': 0, 'www.': 0, 'xml': 0}, 'pii_count': 0, 'substrings_counts': 0, 'word_list_counts': {'cursed_substrings.json': 1, 'profanity_word_list.json': 0, 'sexual_word_list.json': 0, 'zh_pornsignals.json': 0}}
Optics with an Atom Laser Beam

We report on the atom optical manipulation of an atom laser beam. Reflection, focusing and its storage in a resonator are demonstrated. Precise and versatile mechanical control over an atom laser beam propagating in an inhomogeneous magnetic field is achieved by optically inducing spin-flips between atomic ground states with different magnetic moment. The magnetic force acting on the atoms can thereby be effectively switched on and off. The surface of the atom optical element is determined by the resonance condition for the spin-flip in the inhomogeneous magnetic field. A mirror reflectivity of more than 98% is measured.

We report on the atom optical manipulation of an atom laser beam. Reflection, focusing and its storage in a resonator are demonstrated. Precise and versatile mechanical control over an atom laser beam propagating in an inhomogeneous magnetic field is achieved by optically inducing spin-flips between atomic ground states with different magnetic moment. The magnetic force acting on the atoms can thereby be effectively switched on and off. The surface of the atom optical element is determined by the resonance condition for the spinflip in the inhomogeneous magnetic field. More than 98 % of the incident atom laser beam is reflected specularly. The realization of atom lasers [1] opens up new intriguing perspectives in coherent atom optics. These novel atom sources are based on Bose-Einstein condensates [2] from which a coherent matter wave beam is extracted. The unique properties of atom lasers will make it possible to enter an experimental regime in atom optics that is not accessible for thermal atom sources. In light optics the availability of coherent sources has substantially increased the range of photonic applications. Similarly, it is expected, that coherent matter wave sources will have a profound impact on applications such as atom interferometry [3], atom holography [4] or the manipulation of atomic beams on a nanometer scale.
To fulfill these expectations it is crucial to invent atom optical elements that are adapted to the demands of the new highly coherent atom sources. For thermal atom sources a variety of atom optical elements have been investigated [5], which redirect, split or shape atomic beams using position-or time-dependent potentials. To preserve the coherence properties of atom lasers a very high "surface quality" of atom optical elements is required. The de Broglie wavelength of an atom laser beam can be well below ten nanometers. The effective surface roughness of atom optical elements should therefore be even smaller.
The most simple approach to realize a coherent matter wave source is to suddenly release a Bose-Einstein condensate from the magnetic trap. The mechanical manipulation of released condensates has been demonstrated using optical standing wave fields [6,7] suitably shaped off-resonant laser fields [8] and pulsed magnetic fields [9]. Due to the sudden switch-off of the confining potential the energy of the repulsive interaction between the atoms is transformed into kinetic energy. The velocity distri-bution of the released atoms is therefore much broader than the Heisenberg limit associated with the spatial size of the trapped condensate. The velocity spread is drastically reduced for atom lasers employing continuous output coupling, where a Fourier limited output can be approached [10] and interaction effects are minimized. The resulting monoenergetic atom laser beam is not susceptible to dispersive effects in the manipulation of coherent matter waves [8], which are unwanted in most atom optical applications.
In this Letter we report on the atom optical manipulation of an atom laser beam. We have realized a versatile atom optical element and demonstrate reflection, splitting and focusing of the atom laser beam, as well as its storage in a resonator. This is accomplished by optically inducing spin-flips between atomic ground states of different magnetic moment, thereby switching the force on and off that the atom laser beam experiences in an inhomogeneous magnetic field. By a suitable choice of the frequencies and polarizations of the Raman laser fields, the coupling between two specific ground states can be induced. This avoids restrictions in the coupling strengths and state selectivity that would be encountered when using rf or microwave fields.
The atom laser output is extracted from a 87 Rb Bose-Einstein condensate using continuous output coupling [11]. A weak and monochromatic radio-frequency field transfers the magnetically trapped atoms, which are condensed in the |F = 1, m F = −1 state, into the untrapped |F = 1, m F = 0 state (F : total angular momentum, m F : magnetic quantum number). Gravity accelerates the untrapped atoms downwards and a well collimated atom laser beam is formed, while the magnetic trap is still on. After ballistically propagating over a few hundred micrometers the atoms enter the spin-flip region, where two focused laser beams induce a two photon hyperfine Raman transition and transfer a variable fraction of atoms into the state |F = 2, m F = 1 with the magnetic moment 1 2 µ B (µ B : Bohr magneton). The state |F = 2, m F = 1 is low-field seeking and the atoms experience the potential of the magnetic trap. The gradient of our trap in the vertical direction exceeds the gravitational force by one order of magnitude. Therefore the atoms are slowed down until they reverse their direction of motion. Traveling upwards the atoms pass through the laser field for a second time where they are spin-flipped into the original state |F = 1, m F = 0 and continue their motion on a ballistic trajectory (see The frequencies of the two laser fields that induce the Raman transitions are adjusted to drive the single photon 5S 1/2 to 5P 1/2 transition off resonance (see Figure 2(a)). The polarizations of the laser beams are chosen such that the lower frequency field drives π-transitions and the higher frequency field drives σ-transitions. Here the quantization axis is chosen parallel to the local magnetic field vector, which is oriented vertically in the spin-flip region. For both laser fields the single photon detuning ∆ is large compared to the single photon Rabi frequencies Ω 1 and Ω 2 . Spontaneous scattering of photons is therefore suppressed and the coupling between the states |F = 1, m F = 0 and |F = 2, m F = 1 can be described by an effective two level system, with a coupling strength The resonance condition for the spin-flip transition is fulfilled if the frequency difference between the two Raman lasers is equal to the hyperfine plus Zeeman splitting of the two atomic states. Co-propagating laser beams are used in the experiment so that the Raman transition is not sensitive to the Doppler effect. The resonance condition mentioned above is fulfilled on a shell of constant magnetic field. In other words, the effective surface of the mirror in the inhomogeneous trapping potential is determined by the frequency difference between the two Raman laser beams, which can be controlled with high accuracy. The spin-flip therefore occurs in a region which is much better localized than the waist of the Raman laser beams. The distance between the spin-flip region and the coils, which produce the dc-magnetic field, is a few centimeters. Therefore static corrugations of the mirror surface on a smaller spatial scale, e.g. in the nanometer range, are not expected. To minimize fluctuations in the magnetic trapping field a highly stable current supply (∆I/I < 10 −4 ) is used and the trapping region is placed in a magnetic shield enclosure.
In the experiment Bose-Einstein condensates of typically 7 × 10 5 87 Rb atoms are produced in a quadrupole and Ioffe configuration (QUIC) trap [13] by evaporative cooling. The laser light used to drive the two photon Raman transition is generated by two extended cavity diode lasers [14]. A phase-locked-loop [15] is employed to stabilize the frequency difference between the two lasers to a frequency reference, which is tunable at around 6.8 GHz corresponding to the hyperfine splitting of the 87 Rb ground state. Each of the phase-locked lasers is amplified by injection locking another laser diode. The amplified laser beams pass through acousto-optic modulators (AOM) used for switching them on and off. Then the two beams are overlapped with orthogonal polarizations and fed into a single mode optical fiber. The fiber filters the spatial mode and ensures that the laser beams are exactly co-propagating. After the fiber the laser beams are directed into the vacuum chamber and propagate along the symmetry axis (y-direction) of the elongated magnetic trapping potential, in which the cigar shaped condensate is stored. The focus of the overlapping laser beams is positioned 400 µm below the condensate at z 0 = −400 µm. The beam waists are w z = 27 µm in the vertical and w x = 500 µm in the horizontal direction.
We experimentally determined the reflectivity of the spin-flip mirror, with the Raman lasers detuned by 70 GHz to the red of the D 1 line of 87 Rb and a magnetic field gradient of 200 G/cm [16]. An atom laser beam was extracted from the condensate for 4 ms. The Raman lasers were switched on 8.5 ms after the beginning of the output coupling for a duration of 2 ms. During this period of time a fraction of the atom laser beam was spin-flipped into the |F = 2, m F = 1 state and reflected. 5 ms later the magnetic trap was switched off and an absorption image was taken (see Figure 1(a)). The reflectivity of the mirror, i.e. the probability for spin-flipping the atoms, was derived from the absorption images. The reduced optical density in that part of the atom laser beam which passed through the spin-flip region when the Raman lasers were switched on was compared to the optical density of the unperturbed atom laser beam. In addition, the optical density of the reflected, i.e. spinflipped, part of the atom laser beam was measured. No loss of atoms was found in the reflection process. Figure 3 shows the mirror reflectivity vs. the power of the Raman laser beams. For laser powers of 1.2 mW a peak reflectivity in excess of 98% was found.
The measured reflectivity can be described by adiabatic transitions according to a Landau-Zener model. The adiabatic potential curves for the atoms in a onedimensional case are given by where V 1 (z) = mgz + hν hf + 1/2µ B B 2 0 + (B ′ z) 2 and V 0 (z) = mgz are the potentials for atoms in the |F = 2, m F = 1 and |F = 1, m F = 0 state, respectively (m: mass of 87 Rb, g: gravitational acceleration, h: Planck's constant). B 0 and B ′ denote bias field and radial gradient of the magnetic trap, which has a Ioffe-type magnetic field geometry (see Figure 2(b)).
The frequency difference ν 12 of the Raman lasers is detuned from the energy splitting of the trapped and untrapped atomic states by an amount ∆ 12 12 , where ∆ AC is the residual difference in light shift induced by the Raman lasers, that the atomic states experience. The spatial dependence of the Raman coupling is determined by the gaussian laser focus Ω(z) = Ω 0 e −2(z−z0) 2 /w 2 z . The atoms pass through the interaction region with a velocity v which gives rise to non-adiabatic behaviour. The probability for non-adiabatic passage is given by with Γ =h Ω 2 0 The efficiency of the adiabatic transition can thus be controlled by the atomic velocity v and Ω, which is proportional to the laser intensity. For the narrow longitudinal velocity spread of the atom laser beam the dependence on velocity of the Landau-Zener transition is negligible.
In a numerical simulation we have verified that the finite interaction time of the atoms with the laser beam and its gaussian shape results only in a slightly modified effective coupling strength and preserves the general form of the transition probability for our experimental parameters. The optical access in the experiment allowed us to demonstrate reflection of the atom laser beam for various dropping heights of up to 0.8 mm. However, it is instructive to examine how the laser power required for adiabatic transitions scales with the dropping distance. From the criterion for adiabaticity Ω0τ 2Γ > 1 [17], where τ = w z /v, we can estimate that the required Raman laser power P = √ P 1 × P 2 scales as P ∝ √ z 0 , where z 0 is the dropping distance in the gravitational potential. Since for dropping heights of 0.5 mm only 1 mW of laser power is required, applying this scheme to much larger dropping heights is realistic. This is in contrast to atom optical mirrors using optically induced dipole potentials, where several watts of laser power are needed for reflection of atoms from the same dropping distance [8]. Furthermore, in the latter case the required laser power scales as P ∝ z 0 .
We have experimentally determined the specularity of the reflection process by comparing the transverse width of the atom laser beam before and after the reflection process. We have found that after a propagation time of 18 ms the width decreases by 25 ± 5%, which is in accordance with the weak curvature of the mirror in axial direction. The transverse velocity spread of the atoms due to the reflection is well below 200 µm/s, which is the resolution limit in our experimental geometry. We can thus conclude that the reflection is completely specular within this limit. In comparison, evanescent wave mirrors or magnetic surface mirrors severely suffer from substantial diffuse reflection [18,19].
To demonstrate the versatility of the atom optical spinflip element we have demonstrated the storage of the atom laser beam in the resonator formed by the magnetic trapping potential. This was achieved by choosing a timing sequence for the Raman lasers such that the atoms in the atom laser beam were spin-flipped only once. We could then observe the storage of the atom laser beam in the resonator formed by the magnetic trapping potential ( Figure 4). In this configuration we could monitor the atom laser beam for more than 35 oscillation periods. Due to the axial curvature of the magnetic trapping potential the atom laser beam was focused. The initial width of the atom laser beam is 70 µm, which is determined by the axial size of the BEC ground state in the magnetic trap. After a propagation period of 18 ms a width of the atom laser beam of only 7 µm, limited by the resolution of our imaging system, is measured.
Focusing of the atom laser beam is a central step towards an atom laser microscope [20]. To achieve a highly monoenergetic atom laser beam of short de Broglie wavelength our novel atom optical element could be used to accelerate the beam. It should then be possible to focus the beam to spot sizes much smaller than achievable in confocal light microscopy and comparable to high energy electron microscopy. An atomic fountain geometry as required for atomic clocks and atom interferometers [21] could be realized by shaping magnetic field gradients and cascading atom optical spin-flip elements.
In conclusion, we have demonstrated and quantitatively studied a versatile atom optical element which allows manipulation of an atom laser beam with unprecedented precision in a free space environment. The experiments are crucial for future studies of fundamental properties of the atom laser and its applications.   . 2. (a) Level scheme of the 5S 1/2 hyperfine ground state of 87 Rb in a magnetic field (not to scale). The condensate is produced in the |F = 1, mF = −1 state and the atom laser is generated by coupling the condensate to the |F = 1, mF = 0 state using an rf transition. The Raman lasers drive the two-photon transition between the |F = 1, mF = 0 and |F = 2, mF = 1 state and are off resonance with the single photon excitation to the 5P 1/2 state.(b) Adiabatic potentials V+(z) and V−(z) in the presence of the Raman lasers. The curve shows the probability for an adiabatic transition as a function of the total intensity of the Raman laser beams. The full line is a fit to the data using the Landau-Zener model, as explained in the text. The scaling between the squared coupling strength Ω 2 0 and the laser intensity is taken as a free parameter.
FIG. 4. Atom laser beam stored in a resonator formed by the magnetic trapping potential. The elliptical cloud in the centre of each absorption image is the condensate. The stripe of varying width and length is the atom laser beam, which oscillates in the trap. Part of the atom laser beam which has not been recaptured can be seen in the first image of the upper row. Each image has a size of 2 mm×0.7 mm. The two images in the lowest row show enlargements of the first image in the first row and the second image in the second row. The propagation time was increased by 2 ms for each image.