Terawatt-class femtosecond long-wave infrared laser

We utilized a nonlinear post-compression technique to generate 675-fs, 9.2-μm CO₂ laser pulses with a peak power of 1.6 TW. This achievement represents the highest peak power ever attained in the femtosecond pulse format within the long-wave infrared (LWIR) spectral range. The successful implementation of this post-compression technique opens avenues for the development of few-cycle, multi-terawatt 9–10 μm lasers, crucial for applications currently relying on near-infrared solid-state lasers, and which stand to benefit from the scaling of laser wavelengths into the long-wave infrared region.

1 Introduction

The favorable wavelength scaling makes high-peak-power lasers operating in the long-wave infrared (LWIR) spectral range (8–15 µm) attractive for numerous strong-field applications, including various promising schemes for laser-driven electron and ion acceleration [1–3], high-brilliance x-ray sources [4], energy transport through the atmosphere [5] and terahertz sources [6]. Carbon Dioxide (CO₂) gas lasers currently stand as the sole sources capable of providing LWIR pulses exceeding terawatt peak powers.

The highest reported peak power with single-beam CO₂ lasers is 15 TW, achieved with 3-ps pulses emitted at a 10.6 µm wavelength in a multi-pulse train format shaped by rotational modulation of the gain spectrum [7]. By suppressing such modulation through the utilization of high-pressure, multi-isotope laser mediums in conjunction with the implementation of chirped pulse amplification (CPA) techniques, we previously attained a peak power of 5 TW in a single 2 ps pulse at λ = 9.2 µm, marking the highest peak power for LWIR lasers operating in a single-pulse format. This innovative approach was pioneered in a more compact laser system operated at the BNL Accelerator Test Facility (ATF) for multi-disciplinary user experiments [8]. However, achieving strongly relativistic regimes of laser-matter interaction, including laser wakefield acceleration of electrons, necessitates reducing the laser pulse duration to 500 fs or shorter and increasing the peak power beyond 10 TW [4].

Paul Corkum first observed the compression of millijoule, picosecond, LWIR pulses to approximately 600 fs in a high-pressure CO₂ regenerative laser amplifier [9]. This phenomenon has been attributed to the spectral broadening of the pulse through self-phase modulation (SPM) in the amplifier’s discharge plasma, followed by its compression due to negative group velocity dispersion (GVD) in the NaCl windows of the amplifier. However, this approach is not compatible with the CPA method, which is essential for amplifying CO₂ laser pulses to the joule level and beyond.

Well-established for NIR CPA lasers, post-compression methods are based on utilizing the SPM approach by the Kerr effect in an optical material or a gas-filled capillary [10–12]. Positioned along the path of a laser beam, such a nonlinear optical component serves as a bandwidth expander, imposing quasi-linear frequency modulation across the pulse’s temporal envelope. The resulting, usually positive, frequency chirp allows for further pulse compression by a diffraction grating, a chirped mirror, or simply by using an optical material with negative GVD. Following this approach, controllable sub-picosecond post-compression has been experimentally explored in the mid-wave infrared at λ = 3.1 µm [13] and λ = 3.9 µm [14], and theoretically in the LWIR at λ = 10 µm [15–17].

Numerical simulations have suggested the possibility of compressing 2.5 ps, 500 GW CO₂ laser pulses down to 250 fs, with the peak power raised up to 2.2 TW using the nonlinear and dispersive properties of bulk NaCl crystals [15]. This proposed regime has been experimentally explored at the ATF, where spikes as short as 130 fs were recorded after the propagation of a 1-TW, 2-ps, λ = 9.2 µm CO₂ laser beam through a 10-cm thick NaCl slab. In this experiment, we validated our simulation model that predicts such behavior [18], but also discovered micro-filamentation within the NaCl slab that disrupts the output beam uniformity. This prompted us to search for a better combination of materials that would allow us to improve pulse compression by partly separating the post-compression process into two consecutive SPM and dispersive compression (DC) steps.

Such implementation required detailed knowledge of the response of a broad class of optical materials to high laser power at LWIR wavelengths, which remained largely unknown at the time. Our search for candidate materials included measurements of a nonlinear refractive index, $n_2$, nonlinear absorption, damage threshold, and other specific material responses to high-power irradiation. Based on the acquired data, we identified KCl and BaF₂ as a promising combination for the two-step post-compressor, with their relevant optical parameters shown in Table 1 [19].

Table 1

Table 1. Optical material properties at λ = 9.2 µm.

By selecting KCl as a material with high $n_2$ value and low second-order dispersion coefficient (${\beta }_2$) for the SPM stage, and BaF₂ as a material with low $n_2$ and high ${\beta }_2$ for the DC stage, we partially decouple the SPM and DC processes, thus enabling their independent and more efficient optimization. Utilizing this approach, we designed and experimentally demonstrated the post-compression of CO₂ laser pulses from 2 ps to less than 500 fs, achieving a 1.6-fold increase in peak power using a ∼0.5-J Gaussian beam filtered out from the central portion of a multi-joule ATF laser output [19].

In the reported experiment, we employ a similar two-component post-compression technique to the entire several-joule, 2-ps CO₂ laser beam. Autocorrelation measurements at the output of the post-compressor reveal gradual pulse compression with increasing input laser energy, with the shortest measured pulse reaching 675 fs. This separated short spike contains 1.3 J of energy, resulting in a peak power of 1.6 TW, marking the advent of the next-generation of high-power femtosecond laser sources in the long-wave infrared (LWIR) spectral domain. A simulation model [20], benchmarked to our observations, predicts the capability of further optimizing this compression scheme to achieve 4.5 TW in 500 fs.

The remainder of this paper is organized as follows: We describe our experimental setup in Section 2, present results in Section 3, discuss them in Section 4, and conclude in Section 5.

2 Experimental setup

In the reported experiment, we utilized the ATF’s multi-terawatt picosecond CO₂ laser setup, which comprises an optical parametric amplifier front end, a diffraction grating stretcher, a multi-pass regenerative laser amplifier, and a six-pass booster amplifier, along with a diffraction grating compressor [8]. Both laser amplifiers utilize a high-pressure isotopic CO₂ gas active medium pumped by high-voltage electric discharge. The output beam, limited by the 10-cm diameter amplifier’s output window, is further expanded and collimated to fit the 16-cm vertical aperture of diffraction gratings in the compressor. The laser produces a 2-ps full-width-half-maximum (FWHM) pulse with variable energy of up to 10 J, centered at the 9.2 µm wavelength.

We build this experiment upon our preliminary analysis and modeling, which predicted that a 3-TW, 2-ps CO₂ laser pulse could be compressed to approximately 500 fs at close to 5 TW peak power after passing through an optical setup depicted in Figure 1. As demonstrated in our earlier studies [18, 19], eliminating small-scale intensity modulations across the laser beam profile is crucial for controlling the post-compression process. To achieve this, a BaF₂ lens and a pinhole constitute a spatial filter. The selection of KCl and BaF₂ as the SPM and DC components, respectively, is based on their combination of the nonlinear refractive index ($n_2$) and GVD parameters, while their thicknesses have been calculated for the optimum compression of CO₂ laser pulses with an input energy of $E_{in}$ = 7 J.

Figure 1

Figure 1. Optimum configuration for a CO₂ laser pulse compression from 2 ps to 500 fs.

Efforts have been made to construct our experimental setup according to this model. However, real-life restrictions, such as manufacturer’s capabilities and space limitations within an in-vacuum transport line primarily purposed for delivering a 2-ps LWIR laser beam to user experiments, prompted certain alterations from the intended design. These alterations are visible when comparing Figure 1 with Figure 2, which represents our actual experimental setup.

Figure 2

Figure 2. Actual post-compressor setup: inserted images illustrate the LWIR beam profiles before and after a spatial filter.

A 2-ps, λ = 9.2 µm beam with a variable input energy, $E_{in}$, up to 8 J, generated by the CO₂ CPA laser system, is directed through the 11.5-m-long vacuum transport line accommodating essential optical components with apertures ranging from 125 to 150 mm. A thin (10-mm-thickness) BaF₂ lens with a focal length of 4 m, in combination with a 2.4-mm-diameter Teflon pinhole placed near the lens’s focal plane, is utilized for filtering out small-scale modulations and hot spots from the laser output beam. Energy losses on the BaF₂ lens and aperture filtering did not exceed 10%.

The laser beam, expanding over 3.3 m after passing through the pinhole, traverses a 50-mm-thick KCl slab serving as the SPM component. After further expansion over 2 m, the beam encounters two 35-mm-thick BaF₂ slabs serving as primary in-line DC elements. Not depicted in the scheme is a wedged NaCl Fresnel reflector redirecting a small percentage of the beam through a 30-mm-thick NaCl window, extracting it from the vacuum transport line for diagnostics. The remaining beam energy is terminated behind the Fresnel reflector.

An imaging lens with a 100 mm optical aperture in the beam diagnostics setup restricts the acceptance of the laser beam, which continues to expand after the spatial filter. This is one of the limiting factors considered when processing our experimental results.

In the experiment, the following laser characteristics were monitored: laser energy, measured with a pyroelectric joulemeter (Gentec-EO QE95); pulse duration, measured with a single-shot autocorrelator; spectrum bandwidth, measured with a grating spectrometer; and beam profile, observed with a pyroelectric array beam profiler (Ophir Spiricon Pyrocam IV). The same pyroelectric array was used for obtaining images from the autocorrelator and spectrometer. The designs of the home-made autocorrelator and spectrometer have been described elsewhere [20].

3 Experimental results

3.1 Beam profiles

As previously emphasized, spatial filtering of a laser beam is crucial for controlling the post-compression process. Beam profile images in Figure 2, obtained with a pyroelectric camera, illustrate the effect of spatial filtering. A larger collection of beam profile images in Figure 3, registered after the post-compressor, demonstrates the effect of beam diameter expansion as $E_{in}$ increases. A similar behavior can be observed at the immediate output from the final laser amplifier and has been attributed to the gain saturation effect, resulting in the flattening of the beam profile.

Figure 3

Figure 3. Individually normalized beam profiles at the output of the post-compression setup registered by a pyroelectric camera. Energy labels correspond to $E_{in}$ measured at the input to the post-compression setup.

This behavior is further explored in Figure 4, which shows azimuthally averaged beam profiles imaged from the plane 1 m behind the BaF₂ slabs, with the radial scale geometrically interpolated to the location of the KCl slab. We observe the evolution from Gaussian to super-Gaussian beam profiles as laser energy increases. At high laser energies, the peak intensity reaches saturation while the beam profiles continue to expand in their cross-section. The limited aperture of the collection optics, which included the 100 mm diameter imaging lens, prevents us from observing peripheral portions of these beams, explaining the sharp edges on the beam profiles in Figure 3 and Figure 4.

Figure 4

Figure 4. Azimuthally averaged radial intensity distributions at the location of the KCl SPM component. Energy labels indicate $E_{in}.$ The observed insignificant increase in the peak fluence for $E_{in}$ between 4 and 8 J is not surprising, considering gain saturation in the CO₂ amplifier.

The fluence calibration was initially performed for low-energy beams, which fit into the acceptance aperture, by comparing the integrated signal on a pyro-camera with the $E_{in}$ measured with a joulemeter after subtracting the 10% energy loss on the transmission through the spatial filter (including a BaF₂ lens and a pinhole). The pyro-camera’s linear response to the incident laser intensity allows extending the absolute fluence assignments to higher energy beams that do not fit into the restrictive aperture.

To estimate the collection efficiency of the imaging system for high-energy beams that do not fit into the observation field, we plot the dependence of the integrated signal (energy equivalent) collected by the pyroelectric camera on the input laser energy, $E_{in}$, as shown in Figure 5. At high laser energies, we observe a significant deviation of the experimental curve from the linear extrapolation due to truncated energy collection. Comparing the integrated signal with the linear extrapolation, we conclude that for the highest observed signal corresponding to $E_{in}$ = 8 J, up to 50% of the beam energy falls beyond the acceptance aperture.

Figure 5

Figure 5. Experimental dependance of the integrated signal (energy collected after the post-compressor) upon the input energy, $E_{in}$. A dashed line represents the linear extrapolation of low-energy data ($E_{in}\le$ 300 mJ).

3.2 Spectral broadening

Laser spectra before and after post-compression have been measured with an 8 nm resolution using a single-shot, slit-less spectrometer [21]. Typical spectra observed at low and high laser energies are shown in Figure 6.

Figure 6

Figure 6. Spectra recorded at (A) low laser energy ($E_{in}$ <0.6 J), (B) high energy ($E_{in}$ ≃7 J); and (C) their intensity profiles.

The fine structure in the spectra is attributed to rotational modulation of the gain spectrum in the CO₂ laser amplifiers [21]. Spectral broadening observed at high laser energy is primarily due to frequency chirping induced by the KCl slab and partly by the BaF₂. Because of the limited acceptance aperture of the spectrometer, spectra measured at $E_{in}$ = 7 J must be considered as averaged over a central portion of the beam containing approximately 60% of the total laser energy.

3.3 Pulse duration

In a single-shot autocorrelator utilizing a 10 mm diameter, 1 mm-thick AgGaSe₂ crystal [21], a relative tilt introduced between the wave fronts of two split beams results in a linear variation in their relative time delay across the crystal. Consequently, a transverse profile of the λ = 4.6 µm sum-frequency signal reflects the temporal autocorrelation of the laser pulse intensity. The time resolution is contingent upon the angle between the beams, optical magnification, and the pixel size of the pyroelectric array. In our setup, the time resolution of the autocorrelation measurements was approximately 100 fs.

The autocorrelation measurements illustrated by Figure 7 reveal that the pulse duration decreases with an increase in $E_{in}$, reaching a minimum around 7 J, which might be considered optimum for the given post-compressor configuration. Two raw autocorrelation images are sampled, along with their intensity profiles, with time labels indicating the full-width-half-maximum (FWHM) of the autocorrelation curves, ${\tau }_{auto}$. The FWHM pulse duration, $\tau$, can be extracted from the autocorrelator function by applying a coefficient dependent upon the pulse shape. According to our computer simulation, ${\tau }_{auto}$/ $\tau$ = 1.6 for a laser pulse profile at the maximum compression observed in the experiment. The shortest measured laser pulse duration, $\tau$ = 675 fs, has been registered at $E_{in}$ = 7.2 J.

Figure 7

Figure 7. The dependence of the autocorrelation full-width-half-maximum (FWHM) on $E_{in}$ is illustrated in (A), while (B) displays autocorrelator images for two representative laser shots. Their corresponding time profiles are depicted in (C).

Note, however, that due to the limited aperture of the AgGaSe₂ crystal, the autocorrelator accepted only a central portion of the beam profiles presented in Figure 4, within a circle of 30 mm diameter.

4 Discussion

Let’s begin by comparing our experimental results with dedicated modeling simulations conducted for the actual configuration of the experiment. Firstly, we observe a close agreement between the experimental data (Figure 7) and simulated results (Figure 8A) for the autocorrelation curves. In contrast to the experiment, where we deduce the laser pulse duration from its measured autocorrelation function, in simulations, we perform this process in reverse order. Initially, we model the pulse evolution through a post-compressor. Subsequently, we extract from simulations the temporal profile and its autocorrelation function for a portion of the beam propagating through the 30 mm aperture (the autocorrelator acceptance). This operation yielded the aforementioned coefficient ${\tau }_{auto}$/ $\tau$ = 1.6. Its deviation from the value of 1.4, which would be valid for Gaussian pulses, accounts for the realistic temporal profile of the compressed pulse.

Figure 8

Figure 8. Autocorrelation function (A) and the compressed pulse shape (B) at $E_{in}$ = 7J, both simulated for the conditions of our experiment. Simulations show that an output NaCl vacuum window at the compressor output has a very minor effect on the compression process.

To calculate the energy in the compressed laser pulse, we account for 40% losses of the laser beam energy as it propagates through the post-compressor’s optical components due to Fresnel reflection on optical surfaces and absorption (in BaF₂). The transmitted 60% of $E_{in}$ is further reduced to 18% due to the aperture effect on the autocorrelator crystal. As a result, for $E_{in}$ = 7.2 J, the portion of the beam sampled by the autocorrelator contains the energy $E$ = 1.3 J, which is appropriately attenuated before being delivered to the autocorrelator to prevent optical damage.

For a Gaussian pulse, the peak power would be $P=0.94E/\tau$. However, according to our earlier study [19], the pulse’s deviation from the Gaussian shape, as well as a small percentage of the laser output energy spread into secondary pulses, reduce this coefficient from 0.94 to 0.83. For the measured $\tau$ = 675 fs, this leads to our empirical power estimate of $P=0.83E/\tau =$ 1.6 TW, which is in close agreement with the simulated peak power (see Figure 8B).

Thus far, we have verified the agreement between our measurements and simulations for a portion of the beam within the 30 mm aperture. Such benchmarking enhances our confidence in using our model for simulating the entire beam evolution. Figure 9A presents the results of these simulations, demonstrating the entire laser pulse compression to 1.2 ps at 2.5 TW peak power. This outcome appears to be less impressive than our earlier prediction illustrated by Figure 9B, where the same simulation program was applied to the post-compressor configuration shown in Figure 1.

Figure 9

Figure 9. Simulated 2-ps pulse compression at $E_{in}$ = 7 J for the entire beam under the conditions of our experiment (Figure 2) (A), and for the initially proposed scheme according to Figure 1 (B).

To understand the difference in performance, let’s estimate the stretching and compression capabilities for two cases: one shown in Figure 1 (ideal setup) and the other in Figure 2 (actual setup).

The self-induced phase shift across a collimated laser beam with intensity $I\left(t\right)$ after propagation through a nonlinear material of length $L$, with assumed negligible absorption and chromatic dispersion is given by: $∆\varphi \left(t\right)=-(\frac{{\omega }_0}{c})n_{2}LI\left(t\right)$, where $c$ is the speed of light, ${\omega }_0$ is the carrier frequency of the pulse, and $n_2$ is the nonlinear refraction coefficient.

Then, the induced frequency sweep over the laser pulse envelope is given by:

$∆\omega \left(t\right)=\frac{d\left(∆\varphi \right)}{dt}=-\left(\frac{{\omega }_0}{c}\right)n_{2}L\frac{dI}{dt}$

Approximating the top portion of a Gaussian pulse with a parabola, we obtain a linear chirp with the maximum frequency excursion: $∆{\omega }_{\mathit{max}}\approx \pm \left(\frac{{\omega }_0}{c}\right)n_{2}L\frac{I_0}{{\tau }_{in}}$, where ${\tau }_{in}$ is the initial pulse duration.

Comparing this with the expression for B-integral: $B=\frac{2\pi }{\lambda }{n}_2{LI}_0$ under the same simplified assumption that the laser pulse length and intensity do not evolve during its spectral stretching in the nonlinear material, makes it clear why the B-integral is considered as a measure of the spectrum stretching, as well as of the maximum potential compression for bandwidth limited pulses.

For the actual case and an input laser energy of 7.2 J, precise simulations accounting for pulse evolution over the optical components of the post-compressor reveal laser peak intensities of 1.82 × 10¹⁵ W/cm² on the KCl slab, 7.18 × 10¹⁴ W/cm² on the first BaF₂ slab, and 9.74 × 10¹⁴ W/cm² on the second BaF₂ slab. In this setup, KCl emerges as the primary contributor to the aggregate B-integral, reaching B = 3.16. Meanwhile, in the ideal case, simulated laser intensities peak at 2.59 × 10¹⁵ W/cm² on KCl and 2.65 × 10¹⁵ W/cm² on BaF₂. Notably, pulse compression in BaF₂ results in this element contributing nearly equally to the cumulative B-integral, which reaches B = 6.19. Correspondingly, simulated compressed pulse spectra appear wider for the ideal case, as is illustrated in Figure 10A. Furthermore, there is a notable alignment between the experimental and simulated spectra for the actual scenario, as depicted in Figure 10B, although fine structure is somewhat obscured due to the limited resolution of the spectrometer.

Figure 10

Figure 10. Simulated and experimental spectral broadening of the laser pulse due to post-compressor action: (A) Simulated spectra for actual and ideal cases integrated over the entire beam; (B) Experimental spectrum compared to the simulated spectrum integrated over the acceptance aperture of the spectrometer.

As for dispersive compression, we shall consider values of ${\displaystyle {\sum }_i}{{\beta }_2}_i{L}_i,$ where ${{\beta }_2}_i=\raisebox{1ex}{${\partial }^2{k}_i$}\!\left/ \!\raisebox{-1ex}{$\partial {\omega }^2$}\right.$ is the measure of the GVD for any particular optical element participating in the dispersive compression, and $L_i\text{\hspace{0.5em}is\hspace{0.17em}the\hspace{0.17em}length\hspace{0.17em}of\hspace{0.17em}that\hspace{0.17em}element}.$

For an ideal simulated case, the ${\displaystyle {\sum }_i}{{\beta }_2}_i{L}_i$ value comes to $-$ 1,170 fs², while for our actual experiment, the absolute number is higher, $-$ 2,140 fs², due to the thicker BaF₂ and additional NaCl window and lenses on the way to the autocorrelator.

Notably, the maximum compression of a spectrally broadened, frequency-chirped pulse will be achieved when we introduce a relative delay to the leading portion of the chirped pulse such that the tail of the pulse catches up the head. This is achieved when ${\displaystyle {\sum }_i}{{\beta }_2}_i{L}_i\approx \raisebox{1ex}{${\tau }_{in}$}\!\left/ \!\raisebox{-1ex}{$2∆{\omega }_{\mathit{max}}$}\right.$, which is approximately proportional to the inverse of the B -integral. For our experimental conditions, this requires a GVD parameter about twice as high as in the ideal case simulations, which is close to our actual situation.

Note that in all our analytical estimates and simulations, we used the material data listed in Table 1.

5 Conclusion

In this study, we delve into the application of nonlinear post-compression techniques to CO₂ laser pulses, aiming to achieve high peak powers within the LWIR range. Our innovative methodology involves leveraging KCl for self-modulation and BaF₂ for dispersive compression, coupled with spatial filtering, ensuring consistent and reliable pulse compression across a wide spectrum of input laser energies. In our post-compression experiment, we achieved a significant breakthrough of high-power LWIR laser technology into sub-picosecond time domain by demonstrating 675 fs laser pulses at λ = 9.2 µm with supra-TW (1.6 TW) peak power for the first time.

The striking agreement between measured and simulated parameters allows us to utilize our model to extract crucial pulse characteristics, such as pulse duration and peak power, integrated over the entire beam. These parameters, though not directly measurable, are pivotal for comprehending and optimizing laser performance. Moreover, the comparison between experimental results and simulations, augmented by analytical insights, underscores the potential for substantial improvement in post-compression beyond the achieved results. By strategically repositioning our optical components, we envision further enhancing the compression process to attain even higher peak powers and shorter pulse durations, ushering in new horizons in LWIR laser technology.

With our validated model, we can confidently apply it to design subsequent iterations of the nonlinear post-compressor, customized to specific requirements. An illustrative example of such advancement is depicted in Figure 11, where we propose a scheme for compressing 2-ps, 9.2-μm laser pulses down to 150 fs. Our findings confirm that the post-compression method represents a viable approach for generating multi-terawatt LWIR pulses with only a few optical cycles.

Figure 11

Figure 11. Proposed scheme for LWIR pulse post-compression to 150 fs (A); simulated fluence before and after the post-compressor (B); simulated pulse before and after the post-compressor (C).

In conclusion, we have successfully implemented a nonlinear post-compression technique to achieve high-peak-power femtosecond laser pulses in the LWIR spectral range. Through our experimental and simulated analyses, we gained valuable insights into the pulse compression mechanism, emphasizing the importance of accurate modeling in optimizing laser performance. These findings contribute significantly to the development of high-power ultra-fast LWIR lasers across various applications, promising advancements in fields such as laser-driven particle acceleration and atmospheric remote sensing.

Data availability statement

The original contributions presented in the study are included in the article/Supplementary material, further inquiries can be directed to the corresponding author.

Author contributions

IP: Conceptualization, Data curation, Formal Analysis, Investigation, Methodology, Writing–original draft, Writing–review and editing. MB: Methodology, Resources, Writing–review and editing. AS: Methodology, Resources, Writing–review and editing. MP: Funding acquisition, Project administration, Supervision, Validation, Writing–review and editing. MNP: Conceptualization, Formal Analysis, Methodology, Software, Validation, Writing–review and editing.

Funding

The author(s) declare that financial support was received for the research, authorship, and/or publication of this article. This work is funded by the U.S. Department of Energy under contract DE-SC0012704, BNL Laboratory Directed Research and Development grant #20-010, and DOE Program grant B&R #KA2601020.

Conflict of interest

The authors declare that the research was conducted in the absence of any commercial or financial relationships that could be construed as a potential conflict of interest.

The author(s) declared that they were an editorial board member of Frontiers, at the time of submission. This had no impact on the peer review process and the final decision.

Publisher’s note

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