The current generation of high-energy titanium-sapphire (Ti:S) laser systems regularly achieve terawatt and in some cases petawatt peak powers, output energies of several tens of Joules and focused intensities greater than 1020
1. M. Aoyama, K. Yamakawa, Y. Akahane, J. Ma, N. Inoue, H. Ueda, and H. Kiriyama, “0.85-PW, 33-fs Ti : sapphire laser,” Opt. Lett. 28, 1594–1596 (2003). [CrossRef]
]. The pump lasers for such systems are generally frequency-doubled Q-switched YAG or YLF lasers with additional glass amplifiers, and are themselves complex and expensive laser systems. Making the most effective use of the costly pump radiation is a matter of economic good sense, but there are difficulties associated with this which require careful design to overcome. In developing the Ti:S amplifiers for the Astra Gemini laser system at the Central Laser Facility, we have used a novel approach to some aspects of pumping the crystals and the suppression of amplified spontaneous emission (ASE), which we present in this paper.
1.1. The Astra Gemini laser system
Astra Gemini is a petawatt-class Ti:S laser system at the Central Laser Facility at the Rutherford Appleton Laboratory in the U.K. When fully commissioned the system will deliver two beams to the customised experimental area, each with an energy of 15 J in a compressed pulse of 30 fs duration. The dual-beam design of Gemini will allow experiments to be conducted in many different geometries, with the capability of varying the focal length, relative timing and polarisation of the two beams in a variety of ways. Astra Gemini consists of two Ti:S amplifiers, each pumped by a total of 60 J of green light in two beams from a frequency-doubled Nd:glass laser system. The input to the amplifiers is the beam from the Astra system, consisting of 1.5J of infra-red (IR) light at 800nm in a 1 ns chirped pulse, which is split as it enters the Gemini laser area. In each of the Gemini amplifiers, the 800nm beam makes four passes of the Ti:S crystal, and is amplified from 750mJ to 25J. Beam quality is maintained by image-relaying from Astra, and within the amplifiers by spatial filters between the passes. After expansion from 50mm to 150mmdiameter, the pulses are compressed to 30fs with an efficiency of around 70%, and then transported to the experimental area on the ground floor below the laser. The design of Gemini provides for the use of long focal length focusing optics, variable pulse duration (by detuning the compressor lengths), energy control (by varying both the pump energy and the input to the amplifiers), and the introduction of additional beams at a later date.
2. Transverse gain in a strongly pumped crystal
Large-aperture Ti:S crystals for high-power amplifiers are available in diameters up to about 12 cm. The characteristics of the crystal growth process tend to produce a variation of Ti 3+
dopant concentration along the axis of the crystal, so to avoid excessive variations in absorption the thickness of the crystal is usually limited to a few centimetres. Typically, the crystal is pumped through its two faces with two or more beams, and the 800nm beam to be amplified traverses the crystal in a similar direction, as shown in Fig. 1
. Both the pump and the 800nm extracting beams are vertically polarised. In this geometry the absorbed energy per unit volume is greatest at the surfaces, and falls off exponentially towards the interior. As high-energy amplifiers are made larger in the quest for greater output energy, so the diameter of the pumped region and the transverse gain-length product at the surfaces increase, to the point where gain depletion caused by ASE can severely limit the energy extracted from the amplifier. This can be assessed quantitatively in the following way. We assume a four-level system and neglect fluorescence decay. Pump and extraction beams propagate collinearly parallel to the optical axis in the z-direction. The small signal gain coefficient go
can be expressed as
Fig. 1. Geometry of a high-power large-aperture Ti:sapphire amplifier.
is the stored energy per unit volume, σE
is the stimulated emission cross section, νlas
is the laser frequency and Fsat
is the saturation fluence [4
4. W. Koechner, Solid-State Laser Engineering (Springer, Berlin, Heidelberg, 1996).
]. The z
-dependence of go
results from the fact that the pump radiation gets attenuated as it propagates through the crystal. As Est
does not vary perpendicularly to z
we can express it as
is the area of the pumped region. Considering that Est
results from absorbed pump radiation and that pump absorption is described by the Lambert-Beer law, we can transform Eq. (2
), taking into account the quantum defect and neglecting other loss mechanisms:
where νp is the frequency of the pump radiation, Ep is the pump energy, α is the pump absorption coefficient and Fp is the pump fluence.
Combining Eq. (1
) and Eq. (3
) we can now obtain an expression for the transverse gain GT
which is the gain that is experienced by a photon travelling the entire diameter D
of the gain region, perpendicular to z
The gain is polarisation dependent, and is greatest for light polarised parallel to the c-axis of the Ti:S crystal. Therefore GT
is greatest in the direction perpendicular to the c-axis, as shown in Fig. 1
The longitudinal gain GL, the gain for photons traversing the crystal parallel to the optical axis, can be calculated by integrating Est along z, over the length l of the laser crystal. We then obtain
is the absorbed pump fluence, meaning input minus output fluence. If almost all the pump radiation is absorbed, i.e. Fabs
, where Fo
is the incident pump fluence, Eq. (5
) takes on a form that does not depend on α
or l. To find the relationship between GT
we consider GT
directly at the surface of the laser crystal where Fp
) is equal to the un-attenuated pump fluence Fo
and hence GT
Hence, the longitudinal gain does not depend on α or D, provided the pump radiation is fully absorbed. The transverse gain at the surface however grows exponentially with these two parameters. Minimising GT and the losses caused by transverse ASE therefore requires a laser crystal with low α and hence low doping density. Efficient use of the pump light, on the other hand, requires high absorption, which with low doping can be achieved only by a long absorption length. Despite not appearing explicitly in any of the equations above, the length of the crystal therefore plays a crucial role in minimising GT. The obvious choices for obtaining high pump absorption at low doping are to use a long crystal or several short crystals in series, but this would result in high costs and a large amount of material in the optical path, which is undesirable for several reasons. An attractive alternative approach is a thin, low-doped crystal and pump light recycling, a scheme in which the un-absorbed pump light is collected and reflected back into the crystal for a second pass, thus doubling the effective pump absorption length.
To illustrate the benefits of pump light recycling (or double-pass pumping) we calculated GT
) for two examples with a simple one-dimensional model. In this model first the the absorbed pump energy was calculated iteratively taking into account the depletion of the ground state, then the gain coefficient was calculated as in Eq. (1
). Parameters used were similar to those planned for the Astra Gemini system. In each case a 25mm thick Ti:S crystal is pumped from both sides with beams of 50mm diameter and pulse energies of 30 J per beam at a wavelength of 527nm. The first case is that of a highly doped crystal that absorbs 99% of the pump light in a single pass (α
), whereas in the second case the doping is such that 99% of the light is absorbed in two passes (α
, with only 90% of the light being absorbed in the first pass). The signal wavelength used for the calculation is 800nm and the gain saturation fluence is 1 Jcm-2
Fig. 2. Calculated transverse gain as a function of position along the optical axis of the laser crystal. Dashed line: highly doped crystal with single pass pumping; solid line: lightly doped crystal with double pass pumping.
The transverse gains as a function of position along the optical axis were calculated for these two cases and are shown in Fig. 2
. In the highly doped, single-pass pumped crystal much of the gain is concentrated at the crystal faces, with the transverse gain reaching a maximum value of 4800. In the lightly-doped crystal with double-pass pumping, the gain distribution is more even and the maximum transverse gain is only 170.
3. Pump beam homogenisation
Large aperture Ti:S amplifiers require a homogeneous, flat-topped distribution of the pump light, which is very difficult to achieve by using the direct output beam of a high energy, large-aperture Nd:Glass laser system operated at a high repetition rate. The technique of beam homogenisation provides a solution to this problem. Several approaches have been described, among them segmented mirrors [5
5. M. P. Kalachnikov, V. Karpov, H. Schonnagel, and W. Sandner, “100-terawatt titanium-sapphire laser system,” Laser Physics 12, 368–374 (2002).
], micro lens arrays and diffractive optical elements [6
6. C. Kopp, L. Ravel, and P. Meyrueis, “Efficient beamshaper homogenizer design combining diffractive optical elements, microlens array and random phase plate,” J. Opt. A 1, 398–403 (1999). [CrossRef]
]. The working principle of all these methods is to divide the incident beam into many sub-apertures which are all expanded onto the same area in the so-called target plane which lies inside the laser crystal. The resulting distribution in the target plane is ideally a homogeneous top-hat profile with steep edges. Figure 3
illustrates that principle and also shows how such a scheme can be adapted for double-pass pumping.
Fig. 3. Illustration of pump beam homogenisation and recycling.
The pump beam with a diameter DP enters the beam homogeniser from the left, which is immediately followed by a condenser lens. This optic is positioned at a working distance d from the laser crystal. In the target plane, the light bundle has the diameter DT. To visualise the extent of the light bundle before and after the laser crystal, rays from opposite edges of the homogeniser are shown. After the crystal the light bundle diverges with a full angle θ≈DP/d. The transmitted pump is collected by a concave mirror, positioned to re-image the crystal plane onto itself. This ensures that the back-reflected distribution has the same diameter and also the same high degree of homogeneity as the original distribution. The highest intensity in this arrangement is found between the focusing mirror and the laser crystal where an image of the homogenisation optic is formed. To evaluate whether air breakdown is a concern at this location, the diameter DF of this image can be calculated using geometrical optics. One obtains
3.1. Implementation of homogenisation and double pass pumping
To implement the scheme illustrated in Fig. 3
on Astra Gemini, we have selected diffractive optical elements (DOE) for beam homogenisation, primarily because they were readily available in the required size and could be tailored to our requirements. The DOEs were manufactured by Silios Technologies. Eight phase levels were engraved into 1mm thick fused silica substrates by means of a plasma etching process. The devices produce multiple diffracted orders, but the phase structure is optimised to maximise the amount of light in one of the first-order beams, which is used for pumping the TiS crystal. The clear aperture of the DOEs is 65mm and they are anti-reflection coated for 527nm. They were specified so that DT
=50mm and d
=4.7m. Although not shown in Fig. 3
, the diffracted light is directed slightly downward such that the pump spot is centred 60mm below the optical axis. This off-axis geometry allows us to block the small portion of light in the zero order, which would otherwise be focused in the target plane by the condenser lens, and could potentially cause damage.
The optomechanical set-up of the pump beam path in Astra Gemini is implemented as follows. Each of the two Ti:S amplifiers is pumped by a frequency doubled Nd:Glass laser system (Quantel SA, France), each providing two beams with a diameter of 45mm. The two beams are slightly expanded to 50mm in a vacuum relay telescope. Each pump beam then passes through the beam homogenisation optics. The pump beams are folded to accommodate the long path length of 4.7m between homogeniser and Ti:S crystal. This is possible as the beam diameter stays confined until reaching the target plane and only becomes more divergent afterwards (see Fig. 3
). The long working distance was chosen in order to minimise the divergence of the pump beams after passing the laser crystal, which facilitates pump recycling, as described in the previous section. The initial pump beam paths lie in a horizontal plane above the centre of the laser crystal. The diffracted beams are deflected slightly downwards by the homogenisation optics, and the last folding mirror in each arm steers them downwards at a steeper angle so that they intersect in the centre of the laser crystal. The 800nm beams propagate in a horizontal plane level with the centre of the laser crystal. The transmitted pump light is collected by the concave pump recycling mirrors, which are positioned beneath the 800nm beam plane at a distance of 1.5m from the crystal, equal to their radius of curvature.
With a maximum pump energy of 30 J in one beam, a pump pulse duration of 30 ns, a first-pass pump light absorption of 90%, and an image spot size of 6.9mm(see Eq. (7
), the intensity inside this image spot is 2.7×108
, safely below the air breakdown threshold of 4×1010
7. S. A. Akhmanov, A. I. Kovrigin, M. M. Strukov, and R. V. Khokhlov, “Frequency dependence of threshold of optical breakdown in air,” Jetp Letters-USSR 1, 25–29 (1965).
]. As the DOE is a phase plate and not a micro lens array, there are no points in the system anywhere between the DOE and the crystal where small images or foci are formed.
3.2. Results of homogenisation and double pass pumping
shows the measured intensity distribution of one pump beam. The image was recorded with a CCD camera that images the light leaking through a high reflective laser mirror and then falling on to a diffuser screen. Figure 5
shows the light distribution that is generated in the plane of the Ti:S crystal by one pump beam after passing the homogenisation optic. This image was recorded by placing a white alumina tile in the crystal plane and imaging it with a CCD camera. Both measurements were recorded with a single pulse at an energy of 26J while the pump laser was running at a repetition rate of 1 shot every 20 s. The raw beam profile shown in Fig. 4
is clearly not suitable for directly pumping the Ti:S amplifier. The nominal beam diameter of 45mm is denoted by the outermost diffraction rings, but most of the energy is concentrated in a much smaller area. Inside this area, the intensity could induce optical damage, while the outer region would be only weakly pumped. We have also found that this fill factor changes as the output energy of the pump lasers is varied.
With the homogenisation optics in place, however, a near-perfect top-hat-like intensity distribution is generated in the target plane, as shown in Fig. 5
. In the plateau region of the distribution (90% of the FWHM diameter), the relative RMS intensity modulations are 6% and the peak-to-valley modulations are 36%. These modulations are on a fine spatial scale and their effect is largely averaged out, firstly because two pump beams and two (inverted) back-reflected beams overlap inside the laser crystal and secondly because the 800nm beam to be amplified traverses the crystal four times at different off-axis angles.
We have so far characterised only two of our five beam homogenisers, which showed very similar results in terms of achieved homogeneity. The diffraction efficiencies into the first order beam were much greater than expected, being 93% for one and >95% for the other, compared with the 75%guaranteed by the supplier. This can be partly attributed to the small off-axis angle that results from the long working distance. Approximately 1% of the energy goes into the zero order, and the remaining few percent are distributed between the other diffracted orders.
Fig. 4. Intensity distribution of raw pump beam.
Fig. 5. Intensity distribution of homogenised pump beam in plane of Ti:S crystal.
4. Index-matched absorber
An ideal liquid for this purpose would (1) be a perfect index-match for sapphire; (2) have low toxicity; (3) not react chemically with engineering materials used for the containing cell; (4) readily dissolve an absorber for the laser wavelength (or be an absorber itself); (5) be cheap and easily available. Not surprisingly, no liquid exists that possesses all these properties.
4.1. Choice of index-matching liquid
TCG appeared attractive because the index-match is very good, the components are readily available, and its toxicity is low. We prepared a number of TCG solutions containing different concentrations of the salt. More than 20 grams of the crystalline solid could be dissolved in 2cm3 of glycerol with ultrasonic agitation, giving a pale green solution that contained a fine precipitate. The precipitate was settled by centrifugation, and the refractive index of the resulting clear liquid was measured with an Abbe refractometer. The highest refractive index obtained was 1.69 with the most concentrated solutions, and these invariably crystallised, turning almost completely solid after a day or two. We also discovered that the solution reacted vigorously with aluminium alloys. The small increase in index over BN did not justify the effort required to prepare the large quantities of the centrifuged solution needed (around 400cm3), so we decided to consider alternatives.
The first material suggested by [10
10. M. E. Graham, B. I. Davis, and D. V. Keller, “Immersion liquids for ruby lasers,” Appl. Opt. 4, 613–615 (1965). [CrossRef]
], BN, is classified as an irritant, but it is not corrosive or as harmful as diiodomethane, and it is also cheap and easily available. Our tests showed it to be compatible with steel, copper, brass, aluminium, and silicone rubber, but not butyl rubber (commonly used for o-rings). BN also readily dissolves the laser dye IR140, which absorbs at 800nm. We concluded that BN would be a suitable choice for our index-matching liquid, with IR140 dissolved in it as an absorber.
A stock solution of IR140 in BN containing 1mg/cm3
was almost opaque to visible light, so this solution was diluted to different concentrations to make absorption measurements with a spectrophotometer. The intention was to use a low concentration of dye in order to ensure bulk absorption of the ASE, rather than allowing all the light to be absorbed in an extremely thin layer of the liquid. Table 1
shows results from these tests.
Table 1. Absorption measurements of IR140 laser dye in 1-bromonaphthalene.
In the mounting cell for the Ti:S crystal, described below, the liquid will be held in a 2 cm wide annulus around the crystal, so the path length to the inside of the cell and back to the crystal is 4 cm. With an absorption coefficient of 2.7cm-1, the transmission of this path would be 1.5×10-5, not allowing for additional absorption and scattering at the wall of the cell. This is about 2%of the Fresnel reflection from the crystal-liquid interface and is therefore negligible.
4.2. Design of Ti:S mounting cell
Fig. 6. Exploded view of the Ti:sapphire crystal cell and mounting.
4.3. Fluorescence and gain measurements
Fig. 7. Image of fluorescence of Ti:S crystal at 52 J pump energy; (a) without and (b) with index-matched absorber liquid. Images are normalised to maximum signal, signal values below 65% of maximum are shown in black.
Fig. 8. Single-Pass small-signal gain with and without crystal being immersed in index-matching absorber fluid, measured as function of pump energy.
shows images of the fluorescence of the Ti:S crystal pumped by 52 J of green light, with no 800nm beam present. Image 7(a)
was recorded with the “dry” crystal, whereas for image 7(b)
the crystal was immersed in the absorber liquid. The images were recorded with a CCD camera looking at one flat input face of the crystal at near-normal angle. An RG615 filter was used to suppress stray pump light and the exposure was started a few µ
s before the pump pulse and stopped 34µ
s later, by which time the fluorescence has completely decayed.
The most prominent difference between the two images is the appearance of an hour-glass shaped darker region along the horizontal axis in the absence of the absorber liquid. This is where the highest transverse gain occurs since the gain is polarisation-dependent and is highest for light polarised along the c-axis (see Fig. 1
). Therefore, the darker region is the signature of parasitic transverse lasing. A similar signature observed by Plé et al. [11
11. F. Plé, M. Pittman, F. Canova, and G. Jamelot, “Analysis and Solutions for Parasitic Lasing in Petawatt and Multi-Petawatt Ti:sapphire Laser Systems,” in Conference on Lasers and Electro-Optics/Quantum Electronics and Laser Science Conference and Photonic Applications Systems Technologies, Technical Digest (CD) (Optical Society of America, 2006), paper JWD4.
], was even more clearly defined than in our case, probably because a crystal with a polished cylindrical surface was used. We also observed a greatly reduced overall fluorescence signal for the dry crystal, compared to the crystal being immersed in the absorber liquid. Because of the normalised representation, this difference is masked in Fig. 7
For a quantitative assessment of the effect of the index matched absorber liquid we measured the small signal gain as a function of pump energy, first with the crystal dry and then with it immersed in the liquid. The result is shown in Fig. 8
. For this measurement, the 4-pass amplifier was seeded with a pulse energy of 6mJ at 800nm. Input and amplified pulse energies were measured with a pyroelectric energy meter (QE50, Gentec). The maximum output was 2.4 J after four passes. This output was less than 5% of the total pump energy, so the amplifier is clearly in the small-signal regime far from saturation, and the single-pass small-signal gain is equal to the fourth root of the total gain. Without the absorber liquid, the gain increases slowly up to about 30 J of pump energy. From this point the gain appears clamped, indeed further increase in pump energy leads to the gain dropping slightly. The highest gain value obtained lies far below what is required for efficient energy extraction, and is reached too early at around 60% of the maximum possible pump energy. This is an effective demonstration that ASE backscattering at the fine-ground crystal surface is sufficient to cause severe gain depletion. It is clearly imperative to eliminate the scattering in order to extract energy from the crystal efficiently and achieve high pulse energies. With the absorber liquid in use however, no gain clamping is observed. The gain curve starts to diverge from the one with no liquid at around 20 J of pump energy, and follows the model curve reasonably well. The gain continues to increase up to the maximum pump energy used, and shows no sign of levelling off. However, the fluorescence image in Fig. 7
does show a hint of the hourglass shape that is the signature of gain depletion by ASE, which suggests that the residual scattering at the crystal surface due to the imperfect index-match is having a slight effect. The integrated fluorescence signal from images similar to those in Fig. 7
shows near-identical behaviour to the small-signal gain curves of Fig. 8
with the absorber absent and present.